On the variationally consistent computational homogenization of elasticity in the incompressible limit

Mikael Öhman; Kenneth Runesson; Fredrik Larsson

doi:10.1186/s40323-014-0017-1

Advanced Modeling and Simulation in Engineering Sciences Cover Image

Research Article

Open Access

On the variationally consistent computational homogenization of elasticity in the incompressible limit

Mikael Öhman†¹Email author,
Kenneth Runesson†¹ and
Fredrik Larsson†¹

†Contributed equally

Advanced Modeling and Simulation in Engineering Sciences20152:1

https://doi.org/10.1186/s40323-014-0017-1

Received: 13 March 2014

Accepted: 30 September 2014

Published: 14 February 2015

Abstract

Background

Computational homogenization is a well-established approach in material modeling with the purpose to account for strong micro-heterogeneity in an approximate fashion without excessive computational cost. However, the case of macroscopically incompressible response is still unresolved.

Methods

The computational framework for Variationally Consistent Homogenization (VCH) of (near) incompressible solids is discussed. A canonical formulation of the subscale problem, pertinent to a Representative Volume Element (RVE), is established, whereby complete macroscale incompressibility is obtained as the limit situation when all constituents are incompressible.

Results

Numerical results for single RVEs demonstrate the seamless character of the computational algorithm at the fully incompressible limit.

Conclusions

The suggested framework can seamlessly handle the transition from (macroscopically) compressible to incompressible response. The framework allows for the classical boundary conditions on the RVE as well as the generalized situation of weakly periodic boundary conditions.

Keywords

Multiscale Computational homogenization Incompressibility Mixed variational formulations

Background

Computational homogenization is a well-established approach in material modeling with the purpose to account for strong micro-heterogeneity in an approximate fashion without excessive computational cost. Such an approach can be applied to the situation when the intrinsic material properties are linear, leading to direct “upscaling”. It can also be applied to the more complex situation when the subscale properties are nonlinear and/or the subscale problem is inherently transient, whereby it is necessary to resort to nested macro-subscale computation (FE²). Since the literature on classical as well as computational homogenization is abundant, it is neither necessary nor possible to give a comprehensive account. Selected references are [1-3] addressing different aspects on homogenization and multiscale modeling. An important issue is the choice of boundary conditions (and data) for the subscale RVE-problem. Selected references are [4-8]. In particular, [8] presents a quite general framework based on “weak periodicity”. How to accommodate the coalescence of microcracks presents a special challenge, e.g. [9]. How to incorporate interfaces and thin membranes are discussed in [10-12].

Despite the extensive developments, there are still fundamental issues that need to be further addressed. Among these issues we note, (i) variational consistency and the macrohomogeneity condition in the context of selective homogenization (in particular, for multi-field problems) (cf. [13,14]), (ii) how to establish bounds on the effective properties within a given confidence interval, and (iii) high contrast material properties of the constituents (e.g. rigid inclusions or pores) for which the classical Dirichlet and Neumann conditions give poor results.

The particular aspect considered in this paper, which represents an unresolved issue even in the simplest case of elastic response, is that of Variationally Consistent Homogenization (VCH) in the limit of macroscopic incompressibility. This situation is encountered when the micro-constituents of a composite are intrinsically incompressible (or nearly incompressible), which infers macroscale incompressibility as well. An example is when a composite of metallic particles (or fibers) embedded in an elastomer matrix is subjected to stresses that are sufficiently large to cause significant plastic deformations in the particles. Another class of problems is characterized by an initially compressible macroscale response, which may become incompressible as the result of the deformation process. An important example is the evolving porous microstructure of a PM-product during the process of sintering, whereby the homogenized response is compressible until the porosity vanishes inferring incompressible macroscale response, cf. [15]. This process is thus characterized by a transition from the compressible to incompressible regimes.

Applying traditional deformation controlled boundary conditions to macroscopically incompressible RVEs is technically possible, see e.g. Moran et al. [16] and Öhman et al. [14]. However, in such cases, special care must then be taken in applying compatible deformations (i.e. no scaling). This leads to a singular, but solvable, RVE-problem. This approach, however, raises three significant issues: (i) FE² is only possible with approximate penalty methods, (ii), the situations of macroscopically compressible and incompressible response require different solution strategies, (iii) the average pressure is not coupled between the scales. One attempt to adress these issues based on a mixed variational framework, was presented by Öhman et al. [17]. In this paper, an alternative formulation is presented, where the mixed variational format on the macroscale is derived directly via homogenization. As compared to [17], extension is also made to weakly periodic boundary condition for the RVE.

The paper is outlined as follows: The appropriate variational setting of the fine-scale elasticity problem in a mixed format is given. Next, the corresponding VCH framework and macroscale problem are outlined. The canonical form of the RVE-problem, based on weakly periodic boundary conditions is established, followed by the Dirichlet and Neumann type boundary conditions resulting in upper and lower bounds on the RVE response. Numerical examples of RVE-problems are then shown, followed by conclusions.

Methods

Subscale modeling of isotropic elasticity allowing for the incompressible limit

A mixed displacement-pressure weak format

We consider a generic micro-heterogeneous, i.e. polycrystalline, material in a given body whose macroscopic configuration occupies the region Ω in space with (presumed smooth) boundary Γ. We are then lead to defining a Representative Volume Element (RVE), that represents the topology of the micro-heterogeneous microstructure, as shown in Figure 1. The total domain occupied by the cubic RVE is denoted

with external boundary

.

Figure 1
**Generic micro-heterogeneous material consisting of inclusions in matrix (example).**

We consider a model material as follows: The stress is decomposed in terms of deviator and pressure as σ=σ _d−p I where $p \overset {\text {def}}{=} -\frac 13\text {tr}(\boldsymbol {\sigma }\!)$, and the strain is decomposed in terms of deviator and dilation as $\boldsymbol {\epsilon } = \boldsymbol {\epsilon }_{\mathrm {d}} + \frac {1}{3} e\boldsymbol {I}$ where $e\overset {\text {def}}{=} \text {tr}(\boldsymbol {\epsilon }) = \boldsymbol {u} \cdot \boldsymbol {\nabla }$. With the kinematic definition $\boldsymbol {\epsilon }_{\mathrm {d}}[\!\boldsymbol {u}]\overset {\text {def}}{=} \,[\!\boldsymbol {u}\otimes \boldsymbol {\nabla }]^{\text {sym}}-\frac {1}{3}[\!\boldsymbol {u}\cdot \boldsymbol {\nabla }]\boldsymbol {I}$, we introduce the constitutive relations

$$ \boldsymbol{\sigma}_{\mathrm{d}} = \hat{\boldsymbol{\sigma}}_{\mathrm{d}}(\boldsymbol{\epsilon}_{\mathrm{d}}[\!\boldsymbol{u}]\!), \quad \boldsymbol{u}\cdot\boldsymbol{\nabla} = e = \hat{e}(p) $$

(1)

Hence, $\hat {\boldsymbol {\sigma }}_{\mathrm {d}}(\bullet)$ and $\hat {e}(\bullet)$ denote suitable constitutive functions. Obviously, in the simplest case of linear isotropic elasticity, we have $\hat {\boldsymbol {\sigma }}_{\mathrm {d}}(\boldsymbol {\epsilon }_{\mathrm {d}})=2G\boldsymbol {\epsilon }_{\mathrm {d}}$ and $\hat {e}(p)=-\frac {1}{K}p$, where G(x),K(x) for x∈Ω are the standard elastic moduli that fluctuate strongly. Moreover, intrinsic incompressibility is defined as $\hat {e}(p)=0$ for any value of p. We are now in the position to formulate the strong format of the fine-scale problem under standard quasistatic conditions and small strain kinematics:

$$\begin{array}{*{20}l} -\left[\hat{\boldsymbol{\sigma}}_{\mathrm{d}}(\boldsymbol{\epsilon}_{\mathrm{d}}[\!\boldsymbol{u}]\!)-p\boldsymbol{I}\right]\cdot\boldsymbol{\nabla} & = \boldsymbol{f} \quad\qquad\,\text{in}\,\, \Omega \end{array} $$

(2a)

$$\begin{array}{*{20}l} -\boldsymbol{u}\cdot\boldsymbol{\nabla} + \hat{e}(p) & = 0 \qquad\quad\,\text{in}\,\, \Omega \end{array} $$

(2b)

$$\begin{array}{*{20}l} \boldsymbol{u} & = \boldsymbol{u}_{\text{pre}} \quad\quad\text{on}\,\, \Gamma^{\mathrm{D}} \end{array} $$

(2c)

$$\begin{array}{*{20}l} \boldsymbol{t}\overset{\text{def}}{=}\left[\hat{\boldsymbol{\sigma}}_{\mathrm{d}}(\boldsymbol{\epsilon}_{\mathrm{d}} [\!\boldsymbol{u}]\!)-p\boldsymbol{I}\right]\cdot\boldsymbol{n} & = \boldsymbol{t}_{\text{pre}} \quad \quad\,\text{on}\,\, \Gamma^{\mathrm{N}} \end{array} $$

(2d)

The corresponding weak format is: Find $\boldsymbol {u}\in \mathbb {U}, p\in \mathbb {P}$ s.t.

$$\begin{array}{*{20}l} a(\boldsymbol{u};\delta\boldsymbol{u}) + b(p,\delta\boldsymbol{u}) &= l(\delta\boldsymbol{u}) &\quad& \forall \delta\boldsymbol{u} \in \mathbb{U}^{0} \end{array} $$

(3a)

$$\begin{array}{*{20}l} b(\delta p,\boldsymbol{u}) + c^{*}(p;\delta p) &= 0 &\quad& \forall \delta p \in \mathbb{P} \end{array} $$

(3b)

where

$$\begin{array}{*{20}l} a(\boldsymbol{v};\boldsymbol{w}) &\overset{\text{def}}{=} \int_{\Omega} \boldsymbol{\epsilon}_{\mathrm{d}}[\!\boldsymbol{w}]: \hat{\boldsymbol{\sigma}}_{\mathrm{d}}(\boldsymbol{\epsilon}_{\mathrm{d}}[\!\boldsymbol{v}]\!) \mathrm{d} V \end{array} $$

(4)

$$\begin{array}{*{20}l} b(q,\boldsymbol{v}) &\overset{\text{def}}{=} - \int_{\Omega} q\,\boldsymbol{v}\cdot\boldsymbol{\nabla} \mathrm{d} V \end{array} $$

(5)

$$\begin{array}{*{20}l} c^{*}(q;r) &\overset{\text{def}}{=} \int_{\Omega} r\,\hat{e}(q) \mathrm{d} V \end{array} $$

(6)

$$\begin{array}{*{20}l} l(\boldsymbol{v}) &\overset{\text{def}}{=} \int_{\Omega} \boldsymbol{v}\cdot\boldsymbol{f} \mathrm{d} V + \int_{\Gamma^{\mathrm{N}}} \boldsymbol{v}\cdot \boldsymbol{t}_{\text{pre}} \mathrm{d} S \end{array} $$

(7)

The solution space and the test space $\mathbb {U}^{0}$ are defined in standard fashion. In particular, all $\boldsymbol {v}\in \mathbb {U}$ are characterized by v=u _pre on Γ ^D, whereas all $\boldsymbol {v}\in \mathbb {U}^{0}$ satisfy v=0 on Γ ^D. The pressure space does not satisfy any boundary conditions.

It is illuminating (although not necessary from an operational point of view) to invoke the potential Π(u,p)

$$ \Pi(\boldsymbol{u},p) \overset{\text{def}}{=} \Lambda(\boldsymbol{u},p) - l(\boldsymbol{u}) \quad\text{with}\quad \Lambda(\boldsymbol{u},p) \overset{\text{def}}{=} \int_{\Omega} \left[\psi_{\mathrm{u}}(\boldsymbol{\epsilon}_{\mathrm{d}}[\!\boldsymbol{u}]\!) - p\,\boldsymbol{u}\cdot\boldsymbol{\nabla} + \psi_{\mathrm{p}}^{*}(p)\right] \mathrm{d} V $$

(8)

where ψ _u(ε _d) and $\psi _{p}^{*}(p)$ are constitutive energy densities^a such that

$$ \hat{\boldsymbol{\sigma}}_{\mathrm{d}}(\boldsymbol{\epsilon}_{\mathrm{d}})= \frac{\partial\psi_{\mathrm{u}}(\boldsymbol{\epsilon}_{\mathrm{d}})}{\partial\boldsymbol{\epsilon}_{\mathrm{d}}}, \quad \hat{e}(p)=\frac{\partial\psi_{\mathrm{p}}^{*}(p)}{\partial p} $$

(9)

The stationarity conditions of Π(u,p) are

$$\begin{array}{*{20}l} \Pi'_{u}(\boldsymbol{u},p;\delta\boldsymbol{u}) &= a(\boldsymbol{u};\delta\boldsymbol{u}) + b(p,\delta\boldsymbol{u}) - l(\delta\boldsymbol{u}) =0 &\quad& \forall \delta\boldsymbol{u} \in \mathbb{U}^{0} \end{array} $$

(10a)

$$\begin{array}{*{20}l} \Pi'_{p}(\boldsymbol{u},p;\delta p) &= b(\delta p,\boldsymbol{u}) + c^{*}(p;\delta p) = 0 &\quad& \forall \delta p \in \mathbb{P} \end{array} $$

(10b)

which are identical to the weak form in (3).

Variationally Consistent Homogenization

VMS-ansatz and scale separation

The appropriate variational setting of the homogenized problem is obtained upon replacing the integrands in the weak forms in (4)–(7) by running averages of the type

(11)

representing a smoothing approximation on a RVE. In practice, the RVE’s are finite-sized and occupies the subscale region

with boundary

. The typical dimension of an RVE is

. The RVE is centered at the macroscale position

for any given $\bar {\boldsymbol {x}}\in \Omega $. Boundary integrals can be homogenized in similar fashion, by considering Representative Surface Elements Γ _#

$$ y \to \langle y \rangle_{\#} \overset{\text{def}}{=} \frac{1}{|\Gamma_\#|} \int_{\Gamma_\#} y\, \mathrm{d}S $$

(12)

The weak forms in (4)–(7) are thus approximated as

(13)

(14)

(15)

(16)

where the RVE-functionals in (13)–(16) are defined as

(17)

(18)

(19)

(20)

Likewise, we homogenize the volume-specific energy potential Λ(u,p):

(21)

where the RVE-functional

is given as

(22)

In the spirit of the Variational MultiScale method (VMS) [18], we introduce the ansatz that the fields $\boldsymbol {u}\in \mathbb {U}$ and $p\in \mathbb {P}$ can be decomposed into macroscale (smooth) and subscale (fluctuating) parts inside each RVE via the unique hierarchical split $\mathbb {U} = \mathbb {U}^{\mathrm {M}} \oplus \mathbb {U}^{\mathrm {s}}$ and $\mathbb {P} = \mathbb {P}^{\mathrm {M}} \oplus \mathbb {P}^{\mathrm {s}}$. As a result, we may assume that it is possible to solve for the fluctuation fields $\boldsymbol {u}^{\mathrm {s}}\in \mathbb {U}^{\mathrm {s}}$ and $p^{\mathrm {s}}\in \mathbb {P}^{\mathrm {s}}$ as “local approximations” on each RVE for given macroscale solutions $\boldsymbol {u}^{\mathrm {M}}\in \mathbb {U}^{\mathrm {M}}$ and $p^{\mathrm {M}}\in \mathbb {P}^{\mathrm {M}}$, i.e. we construct the complete solution on each RVE as^b.

(23a)

(23b)

On the boundary of the macroscale domain, Γ, we assume smooth variation of u defined by the explicit relations u=u ^M, p=p ^M on Γ _#.

In addition, the test function $\delta \boldsymbol {u}\in \mathbb {U}^{0}$ in (3a) is replaced by $\delta \boldsymbol {u}^{\mathrm {M}}\in \mathbb {U}^{{\mathrm {M}},0}$, whereas $\delta p\in \mathbb {P}$ in (3b) is replaced by $\delta p^{\mathrm {M}}\in \mathbb {P}^{\mathrm {M}}$. Altogether, these assumptions infer that $\boldsymbol {u}^{\mathrm {M}}\in \mathbb {U}^{\mathrm {M}}$ and $p^{\mathrm {M}}\in \mathbb {P}^{\mathrm {M}}$ can be solved from the homogenized problem

$$\begin{array}{*{20}l} a\!\left(\tilde{\boldsymbol{u}}\!\left\{\boldsymbol{u}^{\mathrm{M}},p^{\mathrm{M}}\right\};\delta\boldsymbol{u}^{\mathrm{M}}\right) + b\!\left(\tilde{p}\!\left\{\boldsymbol{u}^{\mathrm{M}},p^{\mathrm{M}}\right\},\delta\boldsymbol{u}^{\mathrm{M}}\right) &= l\!\left(\delta\boldsymbol{u}^{\mathrm{M}}\right) &\;\;& \forall \delta\boldsymbol{u}^{\mathrm{M}} \in \mathbb{U}^{{\mathrm{M}},0} \end{array} $$

(24a)

$$\begin{array}{*{20}l} b\!\left(\delta p^{\mathrm{M}},\tilde{\boldsymbol{u}}\!\left\{\boldsymbol{u}^{\mathrm{M}},p^{\mathrm{M}}\right\}\right) + c^{*}\!\left(\tilde{p}\!\left\{\boldsymbol{u}^{\mathrm{M}},p^{\mathrm{M}}\right\};\delta p^{\mathrm{M}}\right) &= 0 &\;\;& \forall \delta p^{\mathrm{M}} \in \mathbb{P}^{\mathrm{M}} \end{array} $$

(24b)

Explicit format of macroscale (homogenized) problem

In practice, the scales are linked by expressing $\boldsymbol {u}^{\mathrm {M}}(\bar {\boldsymbol {x}},{\boldsymbol {x}})$ ^c and $p^{\mathrm {M}}(\bar {\boldsymbol {x}},\boldsymbol {x})$ using Taylor series expansions of suitable order for $\bar {\boldsymbol {x}}\in \Omega $ and in terms of the macroscale solution $\bar {\boldsymbol {u}}(\bar {\boldsymbol {x}})$ and $\bar {p}(\bar {\boldsymbol {x}})$ respectively. We thus introduce the macroscale fields $(\bar {\boldsymbol {u}},\bar {p})\in \bar {\mathbb {U}}\times \bar {\mathbb {P}}$ such that the macroscale solutions u ^M,p ^M inside each RVE are expanded as follows:

(25a)

(25b)

Hence, u ^M is assumed to have linear variation in pertinent to standard “first order homogenization”, whereas p ^M is constant in . Now, we require that

(26a)

(26b)

which leads to the constraints

(27a)

(27b)

As a result, the hierarchical split ($\mathbb {U} = \mathbb {U}^{\mathrm {M}} \oplus \mathbb {U}^{\mathrm {s}}$ and $\mathbb {P} = \mathbb {P}^{\mathrm {M}} \oplus \mathbb {P}^{\mathrm {s}}$) is guaranteed.

We can thus establish at the outset, before any further analysis, that the displacement and pressure fields within each RVE are implicit functions of the values $\bar {\boldsymbol {u}}$, $\bar {\boldsymbol {h}}$, $\bar {p}$, such that $\boldsymbol {u} = \tilde {\boldsymbol {u}}\{\bar {\boldsymbol {u}}, \bar {\boldsymbol {h}}, \bar {p}\}$ and $p = \tilde {p}\{\bar {\boldsymbol {u}}, \bar {\boldsymbol {h}}, \bar {p}\}$.

With the representations in (25) and the constraints in (26) and (27), we are in the position to compute the homogenized quantities that enter the system (24):

(28)

(29)

(30)

(31)

(32)

(33)

The applied macroscale loads $\bar {\boldsymbol {f}}$, $\bar {\boldsymbol {t}}_{\text {pre}}$ and “moments” $\,\bar {\bar {\boldsymbol {f}}}$, $\bar {\bar {\boldsymbol {t}}}_{\text {pre}}$ are defined as

(34)

(35)

Remark.

Henceforth, we restrict to the situation when and |Γ _#|→0; hence $\bar {\bar {\boldsymbol {f}}}$ and $\bar {\bar {\boldsymbol {t}}}_{\text {pre}}$ will vanish. We will also focus on the homogenization of $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ and $\bar {e}$, so $\bar {\boldsymbol {f}}$ and $\bar {\boldsymbol {t}}_{\text {pre}}$ are considered as given macroscopic quantities.

The variationally consistent macroscale “flux” variables $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ and $\bar {e}$ are obtained from homogenization of the constitutive functions as follows:

(36)

By combining (23) with (25) we note that $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ and $\bar {e}$ are indeed implicit functions of the values of the macroscale variables $\bar {\boldsymbol {u}}$, $\bar {\boldsymbol {h}}$ and $\bar {p}$, pertinent to the considered RVE.

Finally, upon inserting (28)–(33) into the system (24), we obtain the macroscale problem: Find $(\bar {\boldsymbol {u}},\bar {p})\in \bar {\mathbb {U}}\times \bar {\mathbb {P}}$ that solve

$$\begin{array}{*{20}l} \bar{a}(\bar{\boldsymbol{u}},\bar{p};\delta\bar{\boldsymbol{u}}) + \bar{b}(\bar{p},\delta\bar{\boldsymbol{u}}) &= \bar{l}(\delta\bar{\boldsymbol{u}}) \quad\quad \forall \delta\bar{\boldsymbol{u}} \in \bar{\mathbb{U}}^{0} \end{array} $$

(37a)

$$\begin{array}{*{20}l} \bar{b}(\delta\bar{p},\bar{\boldsymbol{u}}) + \bar{c}^{*}(\bar{\boldsymbol{u}},\bar{p};\delta\bar{p}) &= 0 \quad\quad\qquad\!\! \forall \delta\bar{p} \in \bar{\mathbb{P}} \end{array} $$

(37b)

where

$$\begin{array}{*{20}l} \bar{a}(\bar{\boldsymbol{u}},\bar{p};\bar{\boldsymbol{w}}) &\overset{\text{def}}{=} \int_{\Omega} \boldsymbol{\epsilon}_{\mathrm{d}}[\!\bar{\boldsymbol{w}}]: \bar{\boldsymbol{\sigma}}_{\mathrm{d}}\{\bar{\boldsymbol{u}}, \bar{p}\}\, \mathrm{d} V \end{array} $$

(38)

$$\begin{array}{*{20}l} \bar{b}(\bar{q},\bar{\boldsymbol{u}}) &\overset{\text{def}}{=} - \int_{\Omega} \bar{q}\,\bar{\boldsymbol{u}}\cdot\boldsymbol{\nabla}\, \mathrm{d} V \end{array} $$

(39)

$$\begin{array}{*{20}l} \bar{c}^{*}(\bar{\boldsymbol{u}},\bar{p};\bar{r}) &\overset{\text{def}}{=} \int_{\Omega} \bar{r}\,\bar{e}\{\bar{\boldsymbol{u}}, \bar{p}\}\, \mathrm{d} V \end{array} $$

(40)

$$\begin{array}{*{20}l} \bar{l}(\bar{\boldsymbol{u}}) &\overset{\text{def}}{=} \int_{\Omega} \bar{\boldsymbol{u}}\cdot\bar{\boldsymbol{f}}\, \mathrm{d} V + \int_{\Gamma^{\mathrm{N}}} \bar{\boldsymbol{u}}\cdot\bar{\boldsymbol{t}}_{\text{pre}}\, \mathrm{d} S \end{array} $$

(41)

If we consider the macroscale fields, $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ and $\bar {e}$, we conclude that they are implicit functions of the fields $\bar {\boldsymbol {u}}$ and $\bar {p}$. The macroscale spaces $\bar {\mathbb {U}}$ and $\bar {\mathbb {P}}$ are chosen as the standard ones for the fine-scale problem.

Canonical formulation of RVE-problem

Preliminaries – Concept of weak periodicity of fluctuation displacement

To avoid unnecessary technical complexity, we henceforth consider the situation without volume load, i.e. f=0. As a preliminary for establishing the proper variational format of the RVE-problem, we consider the most general weak form of the quasi-static momentum balance by introducing the boundary integral with boundary tractions:

(42a)

(42b)

or, more explicitly,

(43a)

(43b)

which is supposed to hold true for all possible δ u,δ p in suitable function spaces (as discussed below). However, this problem is not solvable without further specification of the solution fields u,p,t. In this paper we adopt a recently proposed variational framework allowing for weak satisfaction of micro-periodicity, cf. Larsson et al. [8], and this framework will be briefly summarized in what follows. We then assume that the subscale fluctuation field u ^s is periodic across the RVE boundaries w.r.t. the chosen local coordinate axes. This model assumption, which may be termed “micro-periodicity”, is a key ingredient (and frequently adopted) in the literature on mathematical homogenization and can be viewed as an approximation between the stiffer Dirichlet and the weaker Neumann boundary conditions. Indeed, both these cases can be obtained as special cases of the most general variational format of periodicity (as will be discussed further below).

In order to formulate the conditions on micro-periodicity, we consider the RVE in Figure 2, where the boundary

has been split into two parts:

. Here,

is the image boundary (later chosen as the computational domain for boundary integration), whereas

is the mirror boundary. We shall now introduce the proper mapping

such that any point

is mirrored in a self-similar fashion to the corresponding point

; hence, x ⁻=φ _per(x ⁺).

Figure 2
**RVE in 2D with “image” and “mirror” boundaries.**

In particular, we express micro-periodicity of the displacement fluctuation field as

(44)

or, equivalently, in terms of the “jump” between the fluctuation fields on the image and mirror parts of the boundary as follows:

(45)

Subsequently, we shall not enforce the condition (45) strongly as the point of departure; rather it is done weakly. To this end, we assume that the boundary tractions $\boldsymbol {t}\overset {\text {def}}{=}\boldsymbol {\sigma }\cdot \boldsymbol {n}$ satisfy the following anti-symmetry condition for any regular mirror point

(46)

as depicted in Figure 2. We now evaluate, upon using (46), the boundary term in (42a) and (43a), as follows:

(47)

A weak statement of the micro-periodicity constraint, given in strong form in (46), is

(48)

where the space of test functions that “live” only on the image boundary is given as .

RVE-problem – Original “variationally consistent” weak format

In order to establish the most straightforward formulation of the RVE-problem, based on micro-periodicity, we first use the constraints in (27) and introduce the following spaces for the fluctuation fields:

(49)

(50)

It is then obvious that, for given macroscale values $\bar {\boldsymbol {u}}$, $\bar {\boldsymbol {h}}$, and $\bar {p}$, we can introduce the unique decompositions

(51a)

(51b)

Next, we aim for a unique decomposition of the tractions (which are anti-periodic by assumption) in a fashion that is similar to (51). To this end, we first associate each traction field t along with the average stress $\bar {\boldsymbol {\tau }}[\!\boldsymbol {t}] \in \mathbb {R}^{3\times 3}$, defined as

(52)

This definition for the average stress is chosen so that for any stress field τ in equilibrium and such that t=τ·n on we obtain . We also conclude that

(53)

As a direct consequence of (52), we may introduce the unique split

(54)

where is the space of the traction fluctuations that are self-equilibrating and thus defined as

(55)

The proof of uniqueness of the split in (54) follows from the identity

$$ \boldsymbol{t} = \bar{\boldsymbol{\tau}}[\!\boldsymbol{t}]\cdot\boldsymbol{n}\, + \,[\!\boldsymbol{t} - \bar{\boldsymbol{\tau}}[\!\boldsymbol{t}]\cdot\boldsymbol{n}] $$

(56)

and the fact that

$$ \bar{\boldsymbol{\tau}}[\!\boldsymbol{t} - \bar{\boldsymbol{\tau}}[\boldsymbol{t}]\cdot\boldsymbol{n}] = \bar{\boldsymbol{\tau}}[\!\boldsymbol{t}] - \bar{\boldsymbol{\tau}}[\!\bar{\boldsymbol{\tau}}[\boldsymbol{t}]\cdot\boldsymbol{n}] = \bar{\boldsymbol{\tau}}[\!\boldsymbol{t}] - \bar{\boldsymbol{\tau}}[\!\boldsymbol{t}] = \boldsymbol{0} $$

(57)

Hence, . □

As preliminaries for establishing the RVE-problem, we establish two identities: Firstly, from (53) and (54) follows that

(58)

Secondly, it follows from (25a) and the properties of

that

(59)

whereby it is noted that the macroscale part of u is “filtered out”.

We are now in the position to establish the subscale problem: For given values $\bar {\boldsymbol {u}}$, $\bar {\boldsymbol {h}}$, and $\bar {p}$, that represent the macroscale fields (and which solve the macroscale problem), find the subscale fluctuations that solve the system

(60a)

(60b)

(60c)

where the RVE-functionals were introduced in (17)–(19) and (48).

By inspecting the system in (60), we note that it is not the entire $\bar {\boldsymbol {h}}$ that is used as input to the RVE-problem. In fact, it is readily concluded that it is only the deviatoric part $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}=\bar {\boldsymbol {h}}^{\text {sym}}_{\mathrm {d}}$ that enters as “data” to the RVE-problem. In other words, neither $\bar {\boldsymbol {u}}$, the volumetric part $\bar {h}_{\mathrm {v}}\overset {\text {def}}{=}\bar {\boldsymbol {h}}:\boldsymbol {I}$, nor the skew-symmetric part $\bar {\boldsymbol {h}}^{\text {skw}}=\frac {1}{2}\!\left [\bar {\boldsymbol {h}}-\bar {\boldsymbol {h}}^{\mathrm {T}}\right ]$ will affect the RVE-solution. In conclusion, ($\bar {\boldsymbol {\epsilon }}_{\mathrm {d}},\bar {p})$ are the macroscale variables that are used as data for the RVE-problem; hence, the solution of (60) is parameterized as $\boldsymbol {u}^{\mathrm {s}}=\boldsymbol {u}^{\mathrm {s}}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$, $p^{\mathrm {s}}=p^{\mathrm {s}}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$, and $\boldsymbol {t}^{\mathrm {s}}=\boldsymbol {t}^{\mathrm {s}}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$. In a postprocessing step the homogenized “fluxes” can be represented as

(61a)

(61b)

Note that $\bar {e}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}\neq \bar {h}_{\mathrm {v}}$ in general!

From the aforesaid, it appears that there is a problem associated with the presented “consistent” format in the sense that the strong form of the continuity equation does not (necessarily) represent that one of the fine scale. The reason is that the formulation (60b) “filters out” any imposed constant volumetric strain $\bar {\lambda }$; hence, the strong format generally reads

$$ - \boldsymbol{u}\cdot\boldsymbol{\nabla} + \hat{e}(p) + \bar{\lambda} = 0, \quad \bar{\lambda}\in\mathbb{R} $$

(62)

Clearly, testing (62) with a constant pressure, we obtain .

Remark.

In the special case of intrinsically incompressible material response, defined by $\hat {e}(p)=0$ in , for any p, then we have . However, from (60b), (60c) it is concluded that the solution of the RVE-problem is , whereby we obtain $\bar {\lambda }=\bar {h}_{\mathrm {v}} \neq 0$. It is only when the macroscale solution represents incompressible response, i.e. when $\bar {h}_{\mathrm {v}} = 0$, that we obtain $\bar {\lambda } = 0$. In conclusion, the RVE-problem is able to provide an “incompressible solution” even in the case that the macroscale solution represents compressible response. This anomaly is the main motivation for establishing an alternative format of the problem, which is discussed next.

Macrohomogeneity condition (VCMC)

The Variationally Consistent Macrohomogeneity Condition (VCMC) (or generalized Hill-Mandel condition) is reviewed in Appendix ‘Variationally Consistent Homogenization (VCH)’. In order to establish its localized form for the present problem, we first identify the tangent spaces

(63a)

(63b)

whereby and represent sensitivity fields (or directional derivatives) for given changes and of the macroscale fields within each RVE.

The macrohomogeneity condition is satisfied if, for any given state u ^M, p ^M localized to the considered RVE, the following relations hold:

(64a)

(64b)

In order to show that this condition is, indeed, satisfied automatically by the solution of the RVE-problem as defined in (60), it suffices to consider (60c). Upon differentiating this relation w.r.t. u ^M and p ^M, we obtain

(65)

for any (by definition of (u ^s)^′ {u ^M,p ^M;du ^M,dp ^M}). Now choosing δ t ^s=t ^s in (65), we obtain

(66)

Finally, upon choosing in (60a) and in (60b) while noting the identity in (66) we recover (64). In conclusion the VCMC is satisfied.

Remark.

In the present case there is, obviously, no need to compute the sensitivities du ^s=(u ^s)^′ and dp ^s=(p ^s)^′ explicitly. However, it is always possible to compute the sensitivities of all the fluctuation fields, u ^s, p ^s, and t ^s from the (linear) system obtained by linearizing (60). This system is closely related to the sensitivity problem that must be established as part of computing the pertinent macroscale tangent tensors exploited in Newton iterations on the macroscale problem. The explicit format of that sensitivity problem is discussed in Appendix ‘Sensitivity problem’ for the Canonical format of the RVE-problem that is introduced subsequently.

RVE-problem – Canonical weak format

A generalized formulation of the RVE-problem that does not contain the above-mentioned inconsistency with the strong format is considered next. Firstly, we introduce the following spaces for the total (macroscale and fluctuation) fields:

(67)

(68)

(69)

Secondly, the fine-scale fields within an RVE are decomposed as

(70a)

(70b)

where $\boldsymbol {x}_{\mathrm {m}}\overset {\text {def}}{=}\frac {1}{3}[\!\boldsymbol {x}-\bar {\boldsymbol {x}}]$, and where $\bar {e}$ is an additional scalar quantity which, at the outset, does not depend on the macroscale field(s).

Remark.

As a consequence of the ansatz in (70a), the rigid body motion is removed; $\bar {\boldsymbol {u}} = \boldsymbol {0}$ and $\bar {\boldsymbol {h}}^{\text {skw}} = \boldsymbol {0}$. Hence, the ansatz u is not identical to the solution u=u ^M+u ^s as expressed in (51a).

We now propose the alternative, subsequently denoted canonical, formulation of the RVE-problem as follows: For given values $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$, $ \bar {p}$, that represent the macroscale fields (which solve the macroscale problem), find the subscale fields that solve the system

(71a)

(71b)

(71c)

(71d)

If follows from (72) that the new variable $\bar {e}$ correctly obtains the value in accordance with (61b). To show this result, we first use the divergence theorem to obtain the identities

(72)

Using these identities together with (71b), (71c), we deduce

(73)

The solution of the “canonical” problem (71) contains, in fact, the solution of the original “variationally consistent” problem in (60); however, without the apparent drawback that is associated with that format. The fluctuations

$$\begin{array}{*{20}l} \boldsymbol{u}^{\mathrm{s}}\{\bar{\boldsymbol{\epsilon}}_{\mathrm{d}}, \bar{p}\} &= \boldsymbol{u}\{\bar{\boldsymbol{\epsilon}}_{\mathrm{d}}, \bar{p}\} - \bar{\boldsymbol{\epsilon}}_{\mathrm{d}} \cdot[\!\boldsymbol{x} - \bar{\boldsymbol{x}}] - \bar{e}\{\bar{\boldsymbol{\epsilon}}_{\mathrm{d}}, \bar{p}\}\,\boldsymbol{x}_{\mathrm{m}} \end{array} $$

(74a)

$$\begin{array}{*{20}l} p^{\mathrm{s}}\{\bar{\boldsymbol{\epsilon}}_{\mathrm{d}}, \bar{p}\} &= p\{\bar{\boldsymbol{\epsilon}}_{\mathrm{d}}, \bar{p}\} - \bar{p} \end{array} $$

(74b)

$$\begin{array}{*{20}l} \boldsymbol{t}^{\mathrm{s}}\{\bar{\boldsymbol{\epsilon}}_{\mathrm{d}}, \bar{p}\} &= \boldsymbol{t}\{\bar{\boldsymbol{\epsilon}}_{\mathrm{d}}, \bar{p}\} - \left[\bar{\boldsymbol{\sigma}}_{\mathrm{d}}\{\bar{\boldsymbol{\epsilon}}_{\mathrm{d}}, \bar{p}\} - \bar{p}\boldsymbol{I}\right]\cdot \boldsymbol{n} \end{array} $$

(74c)

are identical to that solve the system (60). This important result can be shown by introducing the unique split of the unknowns

(75)

(76)

(77)

Firstly, inserting these relations into (71c) and testing with $\delta \check {\boldsymbol {\tau }}$ we obtain

(78)

which gives

$$ \delta\check{\boldsymbol{\tau}}:\left[\check{\boldsymbol{h}} - \bar{\boldsymbol{\epsilon}}_{\mathrm{d}} - \frac13\bar{e}\boldsymbol{I}\right] = 0 \quad \forall \delta\check{\boldsymbol{\tau}} \in \mathbb{R}^{3\times 3} \quad\implies\quad \check{\boldsymbol{h}} = \bar{\boldsymbol{\epsilon}}_{\mathrm{d}} + \frac13 \bar{e}\,\boldsymbol{I}. $$

(79)

Next, testing (71a) with $\delta \check {\boldsymbol {h}}$ we obtain

(80)

which gives

$$ \delta\check{\boldsymbol{h}} :[\!\bar{\boldsymbol{\sigma}}_{\mathrm{d}} - \check{p} \boldsymbol{I} - \check{\boldsymbol{\tau}}] = 0 \quad \forall \delta\check{\boldsymbol{h}} \in {\mathbb{R}}^{3\times 3} \quad\implies\quad \check{\boldsymbol{\tau}} = \bar{\boldsymbol{\sigma}}_{\mathrm{d}} - \check{p} \boldsymbol{I}. $$

(81)

Lastly, from (71d) we obtain

(82)

With (81), this result implies that $\check {p} = \bar {p}$.

Now, testing (71a)–(71c) with the fluctuations δ u ^s, δ p ^s, and δ t ^s respectively, we obtain exactly the original system in (60). Hence, we compute the identical quantities $\boldsymbol {u}^{\mathrm {s}} \{\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}, \bar {p}\}$ and $p^{\mathrm {s}}\{\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}, \bar {p}\}$. Finally, the canonical form results in the identical responses $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$ and $\bar {e}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$ as expressed in (61). Since the macroscopic response variables are identical, the VCMC is still fulfilled.

An illustrative comparison between the two RVE formulations are shown Figure 3. Despite the different displacement fields, the homogenized responses, $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ and $\bar {e}$, are the same.

Figure 3
**Comparison of the RVE-problem formulations.** Original formulation (left) and Canonical formulation (right).

Remark.

Fine-scale incompressibility within the RVE is defined by , which gives . As a result, . In practice, there is (of course) no need to establish s a separate system, since $\bar {e}=0$ is obtained directly as part of the solution of (71) in this case.

Variational properties of the RVE-problem – Energy bounds from RVE-functional

Variational properties for the canonical formulation of the RVE-problem – The RVE-potential

In order to establish bounds on the homogenized properties based on the results from the Dirichlet and Neumann problems, we shall introduce an appropriate “RVE-potential” as follows:

(83)

where is the “intrinsic” energy potential that was defined in (22).

We now define the volume-specific “macroscale energy density”^d as the value of at the following generalized saddle-point:

(84)

A stationary point of is defined by the relations

(85a)

(85b)

(85c)

(85d)

It is readily seen that the system in (85) is precisely that of (71), and we may parameterize its solution as

$$ \boldsymbol{u}=\boldsymbol{u}\{{\bar{\boldsymbol{\epsilon}}}_{\mathrm{d}}, \bar{p}\}, \,\, p=p\{{\bar{\boldsymbol{\epsilon}}}_{\mathrm{d}}, \bar{p}\}, \,\, \boldsymbol{t}=\boldsymbol{t}\{{\bar{\boldsymbol{\epsilon}}}_{\mathrm{d}}, \bar{p}\}, \,\, \bar{e}=\bar{e}\{{\bar{\boldsymbol{\epsilon}}}_{\mathrm{d}}, \bar{p}\} $$

(86)

At the stationary point, we may use the result in (85c) to conclude that

(87)

whereby the energy at the stationary point is deduced to become

(88)

We now deduce that serves as the “macroscale energy density” for $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ and $\bar {e}$ in the sense that we have the macroscale constitutive relations

(89)

Details of the proof are given in Appendix ‘Homogenized macroscale energy’.

From the solution of the RVE-problem, $\bar {e}$ is obtained directly as a primary variable. The deviatoric stress $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ is obtained by post-processing:

(90)

Variational properties for Dirichlet boundary conditions

In order to establish a suitable variational setting we replace the solution space with defined as

(91)

where

(92)

while are the same spaces as for the generic problem. The generalized saddle-point problem (84) can now be rephrased as

(93)

where

(94)

The only possibility to obtain a finite value of while evaluating the sup over is to set $\check {\boldsymbol {\epsilon }}_{\mathrm {d}} = \bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\check {e} = \hat {\bar {e}}$. Hence, we replace the saddle-point problem by

(95)

where

(96)

A stationary point of is defined by the relations

(97a)

(97b)

(97c)

and this system of equations takes the explicit form: For given values $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}, \bar {p}$, find the subscale fields that solve the system

(98a)

(98b)

(98c)

Finally, the macroscale energy density at the stationary point becomes

(99)

From the RVE-problem in (98), $\bar {e}$ is obtained directly as a primary variable. The deviatoric stress $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ is obtained by post-processing:

(100)

However in practice $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ is conveniently obtained as the reaction forces associated with the prescribed $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$.

Remark.

The VMCM in (64) is still valid for the restricted space . Since , (64a) is satisfied for all $\delta \boldsymbol {u}^{\mathrm {s}}\in \mathbb {U}^{{\mathrm {D}},\mathrm {s}}$.

Variational properties for Neumann boundary conditions

The Neumann condition represents the weakest possible way of enforcing the micro-periodicity condition. Here it is considered as a model assumption; however, it is also possible to view this choice as a (crude) FE-approximation of the deviatoric traction field. The pertinent RVE-problem is obtained from the general format upon restricting the space , i.e. introducing defined as

(101)

while and are left unrestricted. Clearly, the choice of restricts the tractions to become piecewise constant on each of the three positive boundary faces of the RVE-cube. The generalized saddle-point problem (84) can then be rephrased as

(102)

where

(103)

The only possibility to obtain a finite value of while evaluating the inf over $\hat {\bar {e}}\in \mathbb {R}$ is to set $\check {p} = \bar {p}$. As a direct consequence the variable $\hat {\bar {e}}$ disappears in the resulting expression, cf. (105) below. Moreover, from (90) we see that for tractions we obtain .

Hence, we replace the saddle-point problem by

(104)

where

(105)

A stationary point of is defined by the relations

(106a)

(106b)

(106c)

and this system of equations takes the explicit form: For given values $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}, \bar {p}$, find the subscale fields that solve the system

(107a)

(107b)

(107c)

Finally, we obtain the macroscale energy density as

(108)

From the RVE-problem in (107), $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ is obtained directly as a primary variable. The volumetric strain $\bar {e}$ is obtained by post-processing:

(109)

Remark.

The VMCM in (64) is still valid for the restricted space . Since , (64a) is valid for all .

Macroscale tangent relations

In order to solve the (generally nonlinear) macroscale problem (37) in the FE²-setting using Newton iterations, we need the pertinent tangent operators. Linearizing the implicit relations $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$ and $\bar {e}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$ we obtain

$$ \mathrm{d}\bar{\boldsymbol{\sigma}}_{\mathrm{d}} = \bar{\textbf{\textsf{E}}} : \mathrm{d}\bar{\boldsymbol{\epsilon}}_{\mathrm{d}} + \bar{\boldsymbol{E}}\, \mathrm{d}\bar{p}, \quad \mathrm{d}\bar{e} = \bar{\boldsymbol{C}} : \mathrm{d}\bar{\boldsymbol{\epsilon}}_{\mathrm{d}} - \bar{C}\, \mathrm{d}\bar{p} $$

(110)

thereby defining the tangents $\bar {\textbf {\textsf {E}}}$ (4th order), $\bar {\boldsymbol {E}}$ (2nd order), $\bar {\boldsymbol {C}}$ (2nd order), and $\bar {C}$ (scalar). Since a potential exists, it follows that $\bar {\textbf {\textsf {E}}}$ possesses major symmetry and that $\bar {\boldsymbol {E}} = \bar {\boldsymbol {C}}$, cf. Öhman et al. [14].

In order to compute the tangent operators, it is necessary to first compute the relevant sensitivity fields w.r.t. changes of the macroscale variables $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\bar {p}$, and they are solved from the pertinent tangent problem. On should then note that the particular sensitivity fields that are actually exploited (and needed) and the corresponding explicit formulation of the tangent problem depend on the chosen formulation of the RVE-problem (in terms of the boundary conditions: Weakly Periodic, Dirichlet, Neumann). Here, we shall give details only on the “generic” choice of the weakly periodic conditions.

Remark.

In the case of macroscale incompressibility, $\bar {\boldsymbol {C}}$ and $\bar {C}$ will vanish.

As a point of departure for computing the tangent tensors, we note that $\bar {e}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$ is a primary variable in the RVE-problem, whereas $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$ is post-processed via (90). We thus need to compute sensitivities of $\bar {e}$ and t from the tangent problem. To begin with, we establish the linearized form of (71) at the solution state to obtain

(111a)

(111b)

(111c)

(111d)

which must be valid for any given perturbations $\mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\mathrm {d}\bar {p}$ giving rize to the corresponding perturbations du, dp, dt, and $\mathrm {d}\bar {e}$ in the solution fields.

Next, we introduce orthonormal base dyads G _i, i=1,2,…,8 to ensure that the deviatoric tensors ε _d and σ _d are, indeed, deviatoric in character. In other words we do not use the conventional base dyads e _i⊗e _j, i,j=1,2,3, but we rather introduce the new set of base dyads such that the requirement G _i:I=0 for i=1,2,…,8 is fulfilled. Examples of such (generally unsymmetric) dyads with Cartesian components, are

$$ \boldsymbol{G}_{1} = \frac{1}{\sqrt{6}}\left[\begin{array}{ccc} 2 & 0 & 0\\ 0 & -1 & 0\\ 0 & 0 & -1\end{array}\right],\; \boldsymbol{G}_{2} = \left[\begin{array}{ccc} 0 & 0 & 0\\ 0 & 1 & 0 \\ 0 & 0 & -1\end{array}\right],\; \boldsymbol{G}_{3} = \left[\begin{array}{ccc} 0 & 1 & 0\\ 0 & 0 & 0 \\ 0 & 0 & 0\end{array}\right],\; \ldots,\; \boldsymbol{G}_{8} = \left[\begin{array}{ccc} 0 & 0 & 0\\ 0 & 0 & 0 \\ 0 & 1 & 0\end{array}\right]. $$

(112)

with respect to this basis, we have the representation

$$ \boldsymbol{\epsilon}_{\mathrm{d}} = \sum\limits_{k} (\boldsymbol{\epsilon}_{\mathrm{d}})_{k} \, \boldsymbol{G}_{k},\quad (\boldsymbol{\epsilon}_{\mathrm{d}})_{k} = \boldsymbol{G}_{k} : \boldsymbol{\epsilon}_{\mathrm{d}} $$

(113)

$$ \boldsymbol{\sigma}_{\mathrm{d}} = \sum\limits_{k} (\boldsymbol{\sigma}_{\mathrm{d}})_{k} \, \boldsymbol{G}_{k},\quad (\boldsymbol{\sigma}_{\mathrm{d}})_{k} = \boldsymbol{G}_{k} : \boldsymbol{\sigma}_{\mathrm{d}} $$

(114)

Next, we express the pertinent sensitivities via the representations

$$\begin{array}{*{20}l} \mathrm{d}\boldsymbol{u} &= \sum\limits_{k} \boldsymbol{u}_{\mathrm{d}}^{(k)} (\mathrm{d}\bar{\boldsymbol{\epsilon}}_{\mathrm{d}})_{k} + \boldsymbol{u}_{\mathrm{p}}\,\mathrm{d}\bar{p} \end{array} $$

(115a)

$$\begin{array}{*{20}l} \mathrm{d} p &= \sum\limits_{k} p_{\mathrm{d}}^{(k)} (\mathrm{d}\bar{\boldsymbol{\epsilon}}_{\mathrm{d}})_{k} + p_{\mathrm{p}}\,\mathrm{d}\bar{p} \end{array} $$

(115b)

$$\begin{array}{*{20}l} \mathrm{d}\boldsymbol{t} &= \sum\limits_{k} \boldsymbol{t}_{\mathrm{d}}^{(k)} (\mathrm{d}\bar{\boldsymbol{\epsilon}}_{\mathrm{d}})_{k} + \boldsymbol{t}_{\mathrm{p}}\,\mathrm{d}\bar{p} \end{array} $$

(115c)

$$\begin{array}{*{20}l} \mathrm{d}\bar{e} &= \sum_{k} \bar{e}_{\mathrm{d}}^{(k)} (\mathrm{d}\bar{\boldsymbol{\epsilon}}_{\mathrm{d}})_{k} + \bar{e}_{\mathrm{p}}\,\mathrm{d}\bar{p} \end{array} $$

(115d)

We thus obtain the following sets of tangent problems:

$\mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}} = \boldsymbol {G}_{k}$ while $\mathrm {d}\bar {p} = 0$: For k=1,…,8, solve for the sensitivities $\boldsymbol {u}_{\mathrm {d}}^{(k)}$, $p_{\mathrm {d}}^{(k)}$, $\boldsymbol {t}_{\mathrm {d}}^{(k)}$, $\bar {e}_{\mathrm {d}}^{(k)}$ from the system

(116a)

(116b)

(116c)

(116d)
$\mathrm {d}\bar {p} = 1$ while $\mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}} = \boldsymbol {0}$: Solve for the sensitivities u _p, p _p, t _p, $\bar {e}_{\mathrm {p}}$ from the system

(117a)

(117b)

(117c)

(117d)

Now, upon linearizing (90) and using the representation for dt in (115c), we obtain

(118)

(119)

Directly from (115d), we obtain

$$ \mathrm{d}\bar{e} = \underbrace{\sum\limits_{k} \bar{e}_{\mathrm{d}}^{(k)}\, \boldsymbol{G}_{k}}_{\bar{\boldsymbol{C}}} : \mathrm{d} \bar{\boldsymbol{\epsilon}}_{\mathrm{d}} + \underbrace{\bar{e}_{\mathrm{p}}}_{-\bar{C}}\,\mathrm{d}\bar{p} $$

(120)

Macroscale tangent relations for the Dirichlet and Neumann boundary conditions are detailed in Appendix ‘Sensitivity problem’.

Bounds on the macroscale energy density

Since we have derived the Dirichlet and Neumann problems by respectively restricting the solution spaces as

(121)

it follows from (93), (102), and (84) that

(122)

In other words, the Dirichlet and Neumann boundary conditions represent upper and lower bounds on the macroscale energy density that is obtained with periodic boundary conditions for any given realization of the RVE and for a given macroscale state $(\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}, \bar {p})$. We note that choosing any discretization of in (84) leads to a lower bound of $\bar {\psi }\{{\bar {\boldsymbol {\epsilon }}}_{\mathrm {d}}, \bar {p}\}$.

In the case of linear elasticity, the tangent operators represent the upscaled (=homogenized) constant operators in the representations

$$ \bar{\boldsymbol{\sigma}}_{\mathrm{d}} = \bar{\textbf{\textsf{E}}} : \bar{\boldsymbol{\epsilon}}_{\mathrm{d}} + \bar{\boldsymbol{E}}\, \bar{p}, \quad \bar{e} = \bar{\boldsymbol{C}}:\bar{\boldsymbol{\epsilon}}_{\mathrm{d}} - \bar{C}\,\bar{p} $$

(123)

whereby we obtain

(124)

Results and discussion

Preliminaries

Computations were carried out for a random composite with spherical particles embedded in a matrix, whereby both constituents are assumed to be homogeneous and isotropic linear elastic. The intrinsic properties are thus defined by the free energy expressions

$$ \psi_{\mathrm{u}}(\boldsymbol{\epsilon}_{\mathrm{d}}) = G |\boldsymbol{\epsilon}_{\mathrm{d}}|^{2},\quad \psi^{*}_{\mathrm{p}} = -\frac12 C\, p^{2} $$

(125)

where G and C (=K ⁻¹) are the shear stiffness and bulk compliance respectively. This choice corresponds to the standard relations $\hat {\boldsymbol {\sigma }}_{\mathrm {d}}(\boldsymbol {\epsilon }_{\mathrm {d}}) = 2 G\,\boldsymbol {\epsilon }_{\mathrm {d}}$ and $\hat {e}(p) = -C\, p$. The parameter set associated with the matrix and particles are (G _mat,C _mat) and (G _part,C _part), respectively.

All computational results were obtained for cubic Statistical Volume Elements (SVEs). The target volume fraction of (non-overlapping, spherical particles) if 10% and their size-distribution, in terms of diameter, is uniform in the range $\left [\frac {2}{3},\frac {4}{3}\right ]$, thus with a mean value of 1. Two examples of realizations with SVE-size

and

are shown in Figure 4 and Figure 5, respectively.

Figure 4
**SVE-cube with sample realization of particle composite of size 6×6×6.**

Figure 5
**SVE-cube with sample realization of particle composite of size 9×9×9.**

Now, for sufficiently large size of the SVE (for any given realization of a random composite), we may assume that the macroscale response is isotropic corresponding to the effective moduli $\bar {G}$ and $\bar {C}$ ($=\bar {K}^{-1}$). However, even for a smaller SVE-size, it is possible to compute an “apparent” value of $\bar {G}$ by the minimization

$$ \min \frac{1}{2} \sum\limits_{ijkl} (\bar{\textbf{\textsf{E}}} - 2 \bar{G} \textbf{\textsf{I}}_{\mathrm{d}})_{ijkl}^{2} \implies \bar{G} = \frac12 \frac{\sum_{ijkl}(\textbf{\textsf{I}}_{\mathrm{d}})_{ijkl}(\bar{\textbf{\textsf{E}}})_{ijkl}}{\sum_{ijkl} (\textbf{\textsf{I}}_{\mathrm{d}})_{ijkl}^{2}} $$

(126)

where I _d is the deviatoric fourth order identity tensor such that the isotropic part of $\bar {\textbf {\textsf {E}}}$ can be expressed as $\bar {\textbf {\textsf {E}}}_{\text {iso}} = 2 \bar {G} \textbf {\textsf {I}}_{\mathrm {d}}$ in standard fashion.

For the finite element analysis of the SVE-problems, tetrahedral elements with so-called Mini-element approximations are utilized. This type of element is defined by linear approximation plus a bubble function for u and linear approximation for p, cf. [19].

The RVE‐problems with the different boundary conditions are implemented in the open source C++ code OOFEM (www.oofem.org) [20] and are available under the name MixedGradientPressure. However, due to the difficulty of constructing , the present implementation of the weakly periodic boundary conditions is based on global polynomials for discretizing . Thus, only a lower bound for the true periodicity is obtained. Due to the high computational cost, only the Neumann and Dirichlet boundary conditions are used in the numerical examples in this paper.

Homogenization of macroscopically incompressible response — A convergence study

The first series of SVE-computations were carried out for macroscopically incompressible response, which is obtained when both matrix and particles are completely incompressible. Taking the shear modulus for the matrix, G _mat, as the reference modulus, we choose G _part=5 G _mat, whereas C _mat=C _part=0. Convergence results for the two extremes of Dirichlet and Neumann boundary conditions are shown in Figure 6. The mean value and variance of the homogenized shear modulus $\bar {G}$ are shown for increasing SVE-size, represented by

. Here, a certain number of realizations are used for each value of

, starting with 200 realizations for the smallest SVE size

and ending up with only 4 realizations for the largest SVE-size

that has approximately 500 thousand degrees of freedom. The Salome platform was used for generating the SVEs and the decrease of the number of realizations was due to the meshing code failing when inclusions badly intersect the boundary, which becomes increasingly likely with increasing

. However, as seen in Figure 6, the variance is small in the homogenized results for

and the mean values are still accurate. An RVE is obtained when the variance goes to zero, and the mean value converges, which is the case when the SVE-size is sufficiently large. In the present case, for engineering purposes, we consider

sufficiently large to qualify as an RVE.

Figure 6
**Statistical comparison of the influence of the boundary conditions (Dirichlet, Neumann) on the macroscale shear modulus,** $\bar {G}$ .

Seamless transition from macroscopically compressible to incompressible response

In the second series of computations, we show how the homogenization scheme can seamlessly handle the transition from the macroscopically compressible to the incompressible response. Here, it is assumed that incompressible particles, defined by G _part=5 G _mat and C _part=0 (as before), are embedded in a matrix material with C _mat≥0. Only the situation with Dirichlet boundary conditions is considered (without affecting the generality of the main conclusion from the results). In Figure 7 it is shown how the homogenized properties are affected by the matrix compliance, C _mat, for a given (fixed) realization and given SVE-size

, cf. Figure 5), thus defining an RVE. Clearly, rather than choosing C _mat as the variable material property, one may choose Poisson’s ratio ν _mat via the elementary relation

$$ \nu = \frac{3-2\,C\,G}{6 + 2\,C\,G} $$

(127)

Figure 7
**Homogenized results from a single RVE with Dirichlet boundary condition.** Dependence of effective properties $\bar {C}$ and $\bar {G}$ on the bulk compliance C _mat for fixed values of G _part=5 G _mat and C _part=0.

which is also used in Figure 7.

The computational results verify that the homogenization framework is able to handle the transition from macroscale compressibility to incompressibility when C _mat→0 in a seamless fashion without any algorithmic changes. That macroscopical incompressibility is verified by the computed value $\bar {C} = 0$. It is also noted in Figure 7 that the affect on $\bar {G}$ is more pronounced, however quite limited, when incompressibility is approached.

Conclusions

In this paper we have introduced a variationally consistent homogenization scheme for heterogeneous solids, whose constituents may be incompressible in the extreme case. The mixed control of the homogenized quantities, $(\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}, \bar {p}) \to (\bar {\boldsymbol {\sigma }}_{\mathrm {d}}, \bar {e})$, is what enables the macroscopically incompressible response, whereas traditional strain-controlled homogenization, $\bar {\boldsymbol {\epsilon }} \to \bar {\boldsymbol {\sigma }}$, leads to a singular problem when applied to fully incompressible microstructures. The transition from macroscopically compressible to incompressible states (which is the extreme result when all constituents are incompressible) is handled in a completely seamless fashion. Based on a mixed formulation on the fine scale, it has been demonstrated how the concept of variationally consistent homogenization can be adopted to derive the pertinent two-scale problem. The proposed canonical formulation of the problem on an underlying Representative Volume Element (RVE) is an extension of the formulation presented in Öhman et al. (2013), allowing for a general choice of boundary conditions. Moreover, the canonical formulation has been shown to satisfy the generalized macrohomogeneity condition. The FE-setting on both scales (macroscale and RVE) is based on the standard (u,p)-formulation, and the Mini-element approximation with a bubble function is adopted for the RVE-problem. All implementation and numerical results pertain to 3D-cubes.

It was shown that theoretical bounds on the “homogenized energy density” for weakly periodic boundary conditions on the RVE are obtained by imposing Dirichlet and Neumann boundary conditions. The computational results from a statistical analysis verify the convergence of these bounds with increasing SVE-size. As to the computational cost of solving the RVE-problem with the different types of boundary conditions for the standard compressible problem and the present (in)compressible one, it is concluded that the Neumann boundary condition is quite cost-neutral. However, applying the Dirichlet boundary condition to the canonical RVE-format means a noticeable additional cost, since the additional (global) variable $\bar {e}$ is required in order to account for the (possibly vanishing) macroscale volumetric deformation. In this context, we remark that imposing weak periodicity would infer a further increased computational cost associated with the boundary discretization of tractions in ; hence, it is conjectured that exploiting the standard Dirichlet and Neumann conditions computations and drawing conclusions about their bounding character would be a most competitive approach in FE²-computations.

As to future developments, it is desirable to further exploit the concept of weakly periodic boundary conditions; however, constructing basis functions for in 3D is not a trivial task. Of course, it is also of interest to compare with the classical condition of strongly periodic fluctuations, which is defined by replacing (92) with

(128)

and performing the corresponding steps up to (98). However, this method has the definite drawback that the meshing software must produce strictly periodic meshes.

In a forthcoming paper, the proposed theoretical framework will be applied to the problem of sintering, a characteristic of which is that the microstructure evolves from being highly porous to becoming completely dense. The “compaction” process is driven by surface tension along the particle-pores boundaries until the pore have completely disappeared, cf. Öhman et al. (2013).

Endnotes

^a * indicates “complementary energy”

^b Curly brackets {(∙)} indicate implicit and/or nonlocal functional dependence on (∙).

^c Double arguments, i.e. $\boldsymbol {u}(\bar {\boldsymbol {x}},\boldsymbol {x})$, are used to explicitly point out the underlying scale separation.

^d , the “effective energy density”, for sufficiently large RVE.

Appendix

Variationally Consistent Homogenization (VCH)

VMS-approach – Scale separation and homogenization

Classical model-based homogenization can be formulated in the spirit of the Variational MultiScale method (VMS), cf. [21,22]. We introduce the abbreviated notation $z = (\boldsymbol {u}, p) \in \mathbb {Z} = \mathbb {U} \times \mathbb {P}$, where

represents the space of fine-scale (non-homogenized) solutions to the system (3), which may conveniently be abbreviated in abstract form as the residual equation^e

$$ R(z; \delta z) \overset{\text{def}}{=} R_{\Omega}(z; \delta z) + R_{\Gamma}(z;\delta z) = 0\quad \forall\;\delta z\in \mathbb{Z}^{0} $$

(129)

where $\mathbb {Z}^{0} = \mathbb {U}^{0} \times \mathbb {P}$ is the test space and where each $\boldsymbol {u}\in \mathbb {U}^{0}$ vanishes on the Dirichlet part of Γ.

A multiscale formulation of (129) is defined by the hierarchical split $\mathbb {Z} = \mathbb {Z}^{\mathrm {M}} \oplus \mathbb {Z}^{\mathrm {s}}$, where $\mathbb {Z}^{\mathrm {M}}$ contains smooth macroscale functions and $\mathbb {Z}^{\mathrm {s}}$ is the hierarchical complement of $\mathbb {Z}^{\mathrm {M}}$ that, typically, represents the fine-scale features. It is assumed that each $z\in \mathbb {Z}$ can be split uniquely as z=z ^M+z ^s such that $z^{\mathrm {M}} \in \mathbb {Z}^{\mathrm {M}}$ and $z^{\mathrm {s}} \in \mathbb {Z}^{\mathrm {s}}$. Therefore, solve $z^{\mathrm {M}} \in \mathbb {Z}^{\mathrm {M}}$, $z^{\mathrm {s}} \in \mathbb {Z}^{\mathrm {s}}$ such that (129) can be represented by the set of equations

$$\begin{array}{*{20}l} & R\!\left(z^{\mathrm{M}} + z^{\mathrm{s}}; \delta z^{\mathrm{M}}\right) \quad = 0 \quad \quad\quad\forall\;\delta z^{\mathrm{M}} \in \mathbb{Z}^{{\mathrm{M}},0} \end{array} $$

(130a)

$$\begin{array}{*{20}l} & R\!\left(z^{\mathrm{M}} + z^{\mathrm{s}}; \delta z^{\mathrm{s}}\right) \quad\;\, = 0 \quad\quad \quad \forall\;\delta z^{\mathrm{s}} \in \mathbb{Z}^{\mathrm{s}} \end{array} $$

(130b)

Without introducing further assumptions (approximations), the dimension of the original problem has not changed, i.e. (130) represent two global problems whose solution requires the same computational effort as does (129). In order to reduce the problem dimension based on homogenization (via the assumption of scale separation), we introduce the following key assumptions:

The integrands in the pertinent volume integrals are replaced by a running volume average on RVE’s of the type introduced in (11) such that, typically, the residual in (130a) can be rewritten in terms of the contributions defined on each RVE as

(131)

where is the RVE-residual that is localized to the Representative Volume Element (RVE). In practice (in FE-analysis), quadrature is used such that the evaluation of is carried out only in the Gauss points.

Furthermore, for the sake of simplicity we assume smoothness of boundary terms, such that R _Γ(z;δ z ^M)≈R _Γ(z ^M;δ z ^M), i.e. no boundary homogenization is necessary.
Local approximations for the fluctuation field z ^s are introduced in the spirit of VMS. This means that is the approximate solution^f of the fine-scale equation (130b) for given z ^M, i.e. (130b) is replaced by “closed” RVE-problems (in the macroscale quadrature points) associated with a particular choice of boundary conditions on . In this paper we obtain such “closed” RVE-problems by choosing weakly periodic boundary conditions.

Returning to (130a), we now replace this problem by the approximate, homogenized, problem

(132)

which has the same dimension as (130a). We note that (132) represents a valid homogenization problem for any given choice of ; however, to preserve typical Galerkin properties, such as symmetry of the macroscale tangent operator when such symmetry is inherent in the underlying fine-scale problem, it is crucial to satisfy the VCMC.

Variationally Consistent Macrohomogeneity Condition (VCMC)

We shall assume that there exists a potential Π(z) such that (132) represents the stationary point of Π(z), i.e. it is assumed that

$$ R(z;\delta z) = \Pi'(z;\delta z) \overset{\text{def}}{=} \frac{\mathrm{d}}{\mathrm{d}\epsilon}\Pi(z+\epsilon\delta z)|_{\epsilon = 0} = 0\quad \forall\;\delta z \in \mathbb{Z}^{0} $$

(133)

Next, we introduce the crucial approximation (restriction) $z \approx z^{\mathrm {M}} + \tilde {z}^{\mathrm {s}}\{z^{\mathrm {M}}\}$ before evaluation of the stationarity conditions, whereby we obtain

$$ \begin{aligned} \Pi_{z^{\mathrm{M}}}'\{z^{\mathrm{M}};\delta z^{\mathrm{M}}\} & \overset{\text{def}}{=} \frac{\mathrm{d}}{\mathrm{d}\epsilon}\Pi(z^{\mathrm{M}}+\epsilon \delta z^{\mathrm{M}}+\tilde{z}^{\mathrm{s}}\{z^{\mathrm{M}}+\epsilon \delta z^{\mathrm{M}}\})|_{\epsilon = 0} \\ & = R(z^{\mathrm{M}} + \tilde{z}^{\mathrm{s}}\{z^{\mathrm{M}}\}; \delta z^{\mathrm{M}} + (\tilde{z}^{\mathrm{s}})'\{z^{\mathrm{M}};\delta z^{\mathrm{M}}\}) = 0\quad \forall\;\delta z^{\mathrm{M}}\in\mathbb{Z}^{{\mathrm{M}},0} \end{aligned} $$

(134)

where $(\tilde {z}^{\mathrm {s}})'\{z^{\mathrm {M}};\delta z^{\mathrm {M}}\}$ denotes the sensitivity (or directional derivative) of $\tilde z^{\mathrm {s}}$ for a variation δ z ^M of the macroscale solution z ^M. Hence, the choice of test function in (134) is restricted as compared to (133), and this restriction represents a “generalized Galerkin property” in terms of the underlying macroscale functions in $\mathbb {Z}^{\mathrm {M}}$. Moreover, and most importantly, (134) is completely equivalent to the homogenized problem (132) if it is possible, for any given $z^{\mathrm {M}}\in \mathbb {Z}^{\mathrm {M}}$, to satisfy the constraint

$$ R(z^{\mathrm{M}} + \tilde z^{\mathrm{s}}\{z^{\mathrm{M}}\}; (\tilde{z}^{\mathrm{s}})'\{z^{\mathrm{M}};\mathrm{d} z^{\mathrm{M}}\}) = 0\quad \forall\;\mathrm{d} z^{\mathrm{M}}\in\mathbb{Z}^{{\mathrm{M}},0}(z^{\mathrm{M}}) $$

(135)

or, equivalently,

$$ R(z^{\mathrm{M}} + \tilde z^{\mathrm{s}}\{z^{\mathrm{M}}\}; \mathrm{d}\tilde{z}^{\mathrm{s}}) = 0\quad \forall\;\mathrm{d}\tilde{z}^{\mathrm{s}}\in\tilde{\mathbb{Z}}'^{\mathrm{s}}(z^{\mathrm{M}}) $$

(136)

where the test space $\tilde {\mathbb {Z}}'^{\mathrm {s}}(z^{\mathrm {M}})$, which is the tangent space to the approximation space, is defined as

$$ \tilde{\mathbb{Z}}'^{\mathrm{s}}(z^{\mathrm{M}})\overset{\text{def}}{=}\{\mathbb{Z}^{\mathrm{s}}\ni \mathrm{d} z^{\mathrm{s}} = (\tilde{z}^{\mathrm{s}})'\{z^{\mathrm{M}};\mathrm{d} z^{\mathrm{M}}\},\, \mathrm{d} z^{\mathrm{M}}\in \mathbb{Z}^{{\mathrm{M}},0}\} $$

(137)

Hence, any $\mathrm {d} \tilde {z}^{\mathrm {s}}\in \tilde {\mathbb {Z}}'^{\mathrm {s}}(z^{\mathrm {M}})$ is a sensitivity of the fluctuation field $\tilde {z}^{\mathrm {s}}$ for a differential change of the macroscale field z ^M within the considered RVE. It is computed from the tangent problem that is associated with the RVE-problem. We refer to (135) or (136) as a “Variationally Consistent (generalized) Macrohomogeneity Condition” (VCMC). Obviously, a sufficient condition for these identities to hold true is to require the RVE-residual to vanish on each RVE (in each quadrature point), i.e. to ensure that

(138)

An even stronger condition is to require that for any δ z ^s in a given set of functions that is defined locally for the considered RVE without requiring any implicit (or explicit) coupling to the sensitivity field $(\tilde {z}^{\mathrm {s}})'\{z^{\mathrm {M}};\delta z^{\mathrm {M}}\}$, which obviously defines a restricted choice of test functions. In such a case, the VCMC can be identified as precisely the classical Hill-Mandel macrohomogeneity condition.

Finally, we remark that the VCMC ensures that the macroscale tangent operator becomes symmetrical, since it holds that

$$ R'(z;\delta z_{1},\delta z_{2}) = \Pi^{\prime\prime}(z;\delta z_{1},\delta z_{2}) \overset{\text{def}}{=} \frac{\mathrm{d}}{\mathrm{d}\epsilon}\Pi'(z+\epsilon\delta z_{2};\delta z_{1})|_{\epsilon=0}\quad \forall\;\delta z_{1},\delta z_{2} \in \mathbb{Z}^{0} $$

(139)

With the introduced approximation $z^{\mathrm {s}} \approx \tilde {z}^{\mathrm {s}}\{z^{\mathrm {M}}\}$, the test functions in (139) are chosen as

$$ \delta z_{i} \approx \delta z_{i}^{\mathrm{M}} + (\tilde{z}^{\mathrm{s}})'\{z^{\mathrm{M}};\delta z_{i}^{\mathrm{M}}\} \quad \forall\;\delta z_{i}^{\mathrm{M}}\in\mathbb{Z}^{{\mathrm{M}},0}, \,\, i=1,2 $$

(140)

Homogenized macroscale energy

In order to show that serves as the “macroscale energy density” for $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$ and $\bar {e}$, expressed by the relations (89), we first recall the identity

(141)

where the RVE-potential was defined in (83). Working out the total differential w.r.t. $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\bar {p}$ at equilibrium, we obtain

(142)

where we introduced the sensitivities w.r.t. changes in $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\bar {p}$ as follows:

(143)

(144)

(145)

(146)

Combining these with the (85), we can see that the last four terms in (142) vanish, i.e. . What remains of the total differential is thus

(147)

Now, we may use (85a) and choose $\delta \boldsymbol {u} = \mathrm {d}\bar {\boldsymbol {\epsilon }}\cdot [\!\boldsymbol {x} - \bar {\boldsymbol {x}}]$ to obtain

(148)

Finally, combining this result with (147), we obtain

(149)

which proves (89).

Sensitivity problem

Dirichlet boundary condition

Using the perturbations $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}} + \mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\bar {p} + \mathrm {d}\bar {p}$ in the linearized form of (98) at equilibrium we obtain

(150a)

(150b)

(150c)

which must hold for any given $\mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\mathrm {d}\bar {p}$. We thus consider the cases:

$\mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}} = \boldsymbol {G}_{k}$ while $\mathrm {d}\bar {p} = 0$ (with $\boldsymbol {u}^{{\mathrm {M}}(k)}_{\mathrm {d}} \overset {\text {def}}{=} \boldsymbol {G}_{k} \cdot [\!\boldsymbol {x} - \bar {\boldsymbol {x}}]$): For k=1,…,8, solve for the sensitivities $\boldsymbol {u}_{\mathrm {d}}^{\mathrm {s}(k)}$, $p_{\mathrm {d}}^{(k)}$, $\bar {e}_{\mathrm {d}}^{(k)}$ from the system

(151a)

(151b)

(151c)
$\mathrm {d}\bar {p} = 1$ while $\mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}} = \boldsymbol {0}$: Solve for the sensitivities $\boldsymbol {u}_{\mathrm {p}}^{\mathrm {s}}$, p _p, $\bar {e}_{\mathrm {p}}$ from the system

(152a)

(152b)

(152c)

Upon using the identity , we deduce the tangent operators from

(153)

Tangent operators associated with $\bar {e}$ are obtained directly from the sensitivity analysis

$$ \mathrm{d}\bar{e} = \underbrace{\sum_{k} \bar{e}_{\mathrm{d}}^{(k)} \boldsymbol{G}_{k}}_{\bar{\boldsymbol{C}}} : \mathrm{d}\bar{\boldsymbol{\epsilon}}_{\mathrm{d}} + \underbrace{\bar{e}_{\mathrm{p}}}_{-\bar{C}} \mathrm{d}\bar{p} $$

(154)

Neumann boundary condition

Using the perturbations $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}} + \mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\bar {p} + \mathrm {d}\bar {p}$ in the linearized form of (107) at equilibrium we obtain

(155a)

(155b)

(155c)

which must hold for any given $\bar {\boldsymbol {\epsilon }}_{\mathrm {d}}$ and $\mathrm {d}\bar {p}$. We thus consider the cases:

$\mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}} = \boldsymbol {G}_{k}$ while $\mathrm {d}\bar {p} = 0$: For k=1,…,8, solve for the sensitivities $\boldsymbol {u}_{\mathrm {d}}^{(k)}$, $p_{\mathrm {d}}^{(k)}$, $\bar {\boldsymbol {\sigma }}_{\mathrm {d},\mathrm {d}}^{(k)}$ from the system

(156a)

(156b)

(156c)
$\mathrm {d}\bar {p} = 1$ while $\mathrm {d}\bar {\boldsymbol {\epsilon }}_{\mathrm {d}} = \boldsymbol {0}$: Solve for the sensitivities u _p, p _p, $\bar {\boldsymbol {\sigma }}_{\mathrm {d},\mathrm {p}}$ from the system

(157a)

(157b)

(157c)

Directly from the solution we obtain tangent operators associated with $\bar {\boldsymbol {\sigma }}_{\mathrm {d}}$:

$$ \mathrm{d}\bar{\boldsymbol{\sigma}}_{\mathrm{d}} = \underbrace{\sum\limits_{k} \bar{\boldsymbol{\sigma}}_{\mathrm{d},\mathrm{d}}^{(k)} \otimes \boldsymbol{G}_{k}}_{\bar{\textbf{\textsf{E}}}}: \mathrm{d}\bar{\boldsymbol{\epsilon}}_{\mathrm{d}} + \underbrace{\bar{\boldsymbol{\sigma}}_{\mathrm{d},\mathrm{p}}}_{\bar{\boldsymbol{E}}} \mathrm{d}\bar{p} $$

(158)

For tangent operators associated with $\bar {e}$, we obtain

(159)

Abbreviations

RVE:: Representative volume element

SVE:: Statistical volume element

VCH:: Variationally consistent homogenization

VMS:: Variational multiScale

VCMC:: Variationally consistent macrohomogeneity condition

Declarations

Acknowledgements

The work was funded by the Swedish Research Council.

Authors’ Affiliations

(1)

Department of Applied Mechanics, Chalmers University of Technology

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