Chaplygin gas and effective description of inhomogeneous universe models in general relativity
Abstract
In the framework of spatially averaged inhomogeneous cosmologies in classical general relativity, effective Einstein equations govern the dynamics of averaged scalar variables in a scale–dependent way. A particular cosmology may be characterized by a cosmic equation of state, closing the hierarchy of effective equations. In this context a natural candidate is provided by the Chaplygin gas, standing for a unified description of dark energy and dark matter. In this paper, we suppose that the inhomogeneous properties of matter and geometry obey the Chaplygin equation of state. The most extreme interpretation assumes that both dark energy and dark matter are not included as additional sources, but are both manifestations of spatial geometrical properties. This feature is an important conceptual difference in comparison with the standard approach of a Friedmann–Lemaître–Robertson–Walker universe filled with dust and another fundamental field characterized by the Chaplygin equation of state. We finally discuss the consequences of the resulting scenario for effective cosmological parameters in order to establish the framework of a future confrontation with observations, and we note that the standard Chaplygin gas may not be ruled out by them.
pacs:
04.20.q, 04.40.b, 95.35.+d, 95.36.+x, 98.80.Es, 98.80.Jk1 Introduction
Does an inhomogeneous universe evolve on average like a homogeneous solution in the framework of general relativity? This question is not new [26] and naturally emerges in view of the nonlinearity of the theory and, in particular, from the generally non–commuting operations of averaging and time evolution [27]. The main difficulty to answer it resides in the notion of averaging and in its construction (see, e.g., [19], section 2.2 of [4], and references therein).
Our universe is supposed to verify the strong cosmological principle which demands homogeneity and isotropy at all scales. This standard approach, known as Friedmann–Lemaître–Robertson–Walker (FLRW) cosmology, is widely used in order to describe the dynamics of our universe and the formation of its constituents. It however leaves in suspense an explanation about the origin of dark energy and dark matter, which respectively represent in this model about and of the total content of the universe. This last point might actually reveal a symptom of a deeper problem linked to this approach. Indeed, in FLRW cosmology one determines background quantities regardless of the scale and makes them evolve according to a homogeneous–isotropic solution of Einstein equations. Our first query could be reformulated in order to note the central aspect of this issue: Are the background quantities well defined within standard cosmology, i.e. as a suitable average over the inhomogeneities? Is their evolution well approximated in this framework, i.e. is the time dependence of the homogeneous–isotropic averaged state well approximated by a homogeneous–isotropic solution?
We shall adopt an approach that averages, in a domain–dependent way, the scalar parts of Einstein’s equations with respect to synchronous free–falling observers in a dust model [13, 14], a realization of the averaging problem that does not answer the above questions in the affirmative. The average evolution of an inhomogeneous universe differs from the evolution of a homogeneous one; in other words, even if we are entitled to describe structure formation in terms of perturbations of a background, this latter is generally not a member of the homogeneous solutions (see also [35, 36]). This difference of evolution is driven by the non–trivial geometrical structure of an inhomogeneous space, featuring deviations that are known as “backreaction”. These backreaction effects can act on average, at least qualitatively, as the dark components.
The set of equations obtained within this approach should be closed to derive the evolution of all the involved quantities, namely the effective scale factor, the averaged scalar curvature deviation and the kinematical backreaction variable. In recent papers, attention was turned to a closure under the assumption of global constraints such as a globally stationary universe [15, 16], or by exploring the solution space with exact scaling laws for the backreaction and the averaged scalar curvature [18, 38], or by symmetry requirements such as spherical symmetry (e.g. [11, 21, 28, 37, 40, 45], and references therein). In this work we want to choose the closure relation by focusing on the particularity of the model to unify the dark components through backreaction. According to this point of view, the Chaplygin gas (CG) seems to be an interesting lead since it unifies dark matter and dark energy in only one fluid, obeying an exotic equation of state [31, 32, 34]. This unification is made through the evolution of this particular fluid and it can be extended to a unification where both dark components are simultaneously modelled thanks to the scale dependence of our approach^{1}^{1}1A ‘simultaneous’ unification has also been proposed in the context of an inhomogeneous, but fundamental CG in [8].. These points motivate us to build a model in which the generically existing coupling between the backreaction and the averaged scalar curvature deviation, which encodes the particular geometrical structure evolution of an inhomogeneous universe, is furnished by a scale–dependent CG equation of state^{2}^{2}2A study of inhomogeneous spherically symmetric spacetimes, presenting nonlinear perturbations constructed from the fluctuations of local variables with respect to background quantities called quasi–local scalars, has been given in [44]. As an example the CG is employed in [44] and relates the quasi–local variables’ pressure and density. The reader may find connections between quasi–local variables and our averaging procedure in [43]..
In section 2 we introduce the equations that govern the average evolution of an inhomogenous universe model and briefly discuss them. We present in section 3 the CG and some of its properties. In section 4 we suppose that the backreaction and the averaged scalar curvature deviation are coupled according to the CG equation. The CG then describes a particular geometrical structure of the inhomogeneous universe and does not correspond to any fundamental field. Finally, in section 5, we reformulate the results obtained in terms of effective cosmological parameters; we compare this model to the Friedmannian framework and we study in particular the acceleration of a spatial domain.
2 Effective description of inhomogeneous universe models
Restricting attention to a universe filled with irrotational dust, i.e. irrotational pressureless matter, we spatially average the scalar parts of Einstein equations (the Hamiltonian constraint, Raychaudhuri’s equation and the continuity equation) with respect to a collection of comoving (generalized fundamental) observers over a compact, restmass preserving spatial domain , and obtain the following set of equations ([13, 14, 19], [41] for details):
(1)  
(2)  
(3)  
(4) 
where is the effective volume scale factor
(5) 
with the initial volume of the domain and its volume at a proper time , the density of irrotational dust averaged over , the spatial scalar curvature averaged over and the kinematical backreaction
(6) 
with the rate of expansion and the rate of shear with the shear tensor components .
Equations (1) and (2) govern the kinematics of the effective scale factor and equations (3) and (4) express the conservation law for the dust matter and the backreaction terms, respectively. It is important to point out that might evolve differently from its Friedmannian counterpart (as we shall discuss in subsection 4.3). Upon introducing the averaged scalar curvature deviation , we may rewrite equation (1) in the form
(7) 
Looking now at equations (2) and (7) one should note that both the backreaction and the averaged curvature, through , induce a change in the averaged dynamics of the domain in comparison with the Friedmannian framework. Equation (2) states that a positive backreaction contributes to accelerate the expansion of the domain and then plays against gravity: effectively mimics a dark energy behaviour over . The domain will actually undergo an acceleration of its expansion only if the ‘intensity’ of dark energy is sufficient, which is the case when . A negative backreaction contributes to decelerate the domain expansion and therefore adds to gravity: effectively mimics a dark matter behaviour over . For the averaged model we may suppose that backreaction acts as dark matter on small scales (e.g. galaxy cluster and void scales) and as dark energy on the largest scales (CMB and high–redshift supernovae). In the present work, this differentiation with respect to the spatial scale will however not be made explicit. An explicit multi–scale dynamics can be formulated to refine such a description [46].
We shall assimilate here the properties of the spatial geometrical structure to a domain–dependent CG. To this aim we first describe the backreaction variables in terms of an effective perfect fluid whose energy density and pressure read^{3}^{3}3In this work we prefer to consider the deviation term to describe the fluid, instead of the full averaged scalar curvature . First, incorporate the deviation from a general Friedmannian model, being equivalent to the pair only in a zero–curvature Friedmannian model. Second, the kinematical backreaction and the curvature deviation both vanish on the background and are gauge–invariants (as shown to second–order in perturbation theory [39]).
(8) 
We stress here that, since it is an effective description, this fluid does not have to satisfy any energy conditions (as discussed in [18]). We therefore reformulate equations (1) and (2) casting them into Friedmannian form
(9)  
(10) 
Using the last two equations together with equation (3) one obtains the conservation law for the backreaction fluid
(11) 
which, if written out, reflects the generic coupling between the curvature deviation and the kinematical backreaction—a simple reformulation of equation (4):
(12) 
3 The Chaplygin gas
The CG is a perfect fluid obeying the state equation
(13) 
where and are respectively the energy density and the pressure of the fluid in a comoving frame and is a positive constant. It was first introduced as a cosmological fluid unifying dark matter and dark energy by Kamenshchik et al [34] and has been since widely studied in this context (see, e.g., [2, 3, 9, 10, 20, 23, 22, 25, 29, 30, 31, 32]). The equation of state (13) has also raised interest in particle physics thanks to its connection with string theory [12] and its supersymmetric extension [33]. The generalization of the CG [5, 34],
(14) 
with a free positive parameter, is commonly used in cosmological models; however in the present work we shall consider for simplicity the case , i.e. the standard CG^{4}^{4}4A generalization of our ideas, using equation (14), is straighforward. We emphasize that, even if the standard CG does not seem to well fit with observations in a FLRW model, this must not be the case in our approach, since observational data have to be reinterpreted before the need for such a generalization is justified (cf section 6).. Assuming that the gas verifies the energy conservation law over a spatial domain ,
(15) 
we obtain, making use of relation (13), the expressions
(16) 
where determines the initial conditions of the CG and both and depend on the domain. Note that equations (16) describe the evolution of a homogeneous CG which is the one of interest in our work since the backreaction terms are, due to the averaging procedure, homogeneous over a spatial domain. However, since we average over inhomogeneities, there certainly exist interesting links to the inhomogeneous CG (for an investigation of the latter the reader is referred to [8]).
We now recall briefly of the different aspects of the CG according to the sign of .
3.1 Choosing a positive integration constant
We follow [34] to present the behaviour of the CG for a positive . Expressions (16) become for small values of the scale factor, ,
(17) 
which indicates that the CG can behave as a dark matter component. For large values of the scale factor, , it follows that
(18) 
which reflects the dark energy–like behaviour of the CG in its last stage. Finally, one may also develop (16) for large values of to obtain
(19) 
Between the phases (17) and (18) the CG can be seen as a mixture of a cosmological constant and a stiff fluid whose pressure and energy density are equal.
To resume, for a positive , the CG acts first as dark matter and then as dark energy whose state equation evolves towards the one of a cosmological constant.
3.2 Choosing a negative integration constant
As already noticed in [42] the CG presents another interesting feature for a negative since its density increases with the scale factor. In this situation it plays the role of phantom dark energy, and it evolves at late times towards a cosmological constant. For the pressure and energy density to be well defined one needs
(20) 
It therefore exists a minimal value for the scale factor, , implying that this case describes a bouncing universe model at early times.
4 Evolution of the kinematical backreaction and the curvature deviation
4.1 Backreaction fluid as a Chaplygin gas
As we have outlined in section 2, the backreaction fluid inherits a simultaneous unification of the dark components thanks to its scale dependence. We want to build a model in which this fluid is assimilated to the Chaplygin gas in order to physically shape the behaviour of the backreaction and the curvature deviation on a given spatial scale, while also allowing for a metamorphosis of the ‘dark character’ through evolution. In this model, the Chaplygin gas emerges from the inhomogeneous structure of the universe, and is not related to any fundamental field. We then consider that the backreaction fluid responds to the scale–dependent state equation (13) over a spatial domain . Using definitions (8), we rewrite expression (13) in the form
(21) 
Since no energy condition has to be verified by the backreaction fluid, we may also consider the Chaplygin equation of state (13) with a negative energy density (and hence a negative if one wants to preserve the negativity of the pressure). However, we shall restrict ourselves in this paper to the case where the backreaction fluid satisfies (13) under the usual conditions, i.e. with a positive energy density and a positive ^{5}^{5}5We do not impose here any other energy conditions on the backreaction fluid.. We thus have to respect, in view of expression (21), the following constraints, which we call the Chaplygin fluid constraints:
(22) 
or, equivalently,
(23) 
In this situation, the curvature deviation of any domain is negative at any time whatever its dynamics could be. We also note that and evolve in such a way that relation (21) is always satisfied (see figure 1). Rewriting equation (21) as a function under the Chaplygin fluid constraints, we derive, for a given , the maximal value of the deviation term obtained for . We shall see in subsections 4.3 and 4.4 that these values form an attractor for the dynamics of the system.
4.2 Exact evolution equations
(24)  
(25) 
We may express the constants and in terms of the initial values of the backreaction and the curvature deviation over ,
(26)  
(27) 
and determine the evolution of and in the form
(28)  
(29) 
where the new terms are defined as
(30) 
The Chaplygin fluid constraints imply and . The evolution of and is entirely determined by the initial values and of the domain or, equivalently, by and . The opposite sign of gives the sign of , equation (27), and therefore defines the behaviour of the Chaplygin backreaction fluid.
4.3 Evolution of the curvature deviation
The rate of change shows that the curvature deviation grows with . For large values of the scale factor, , we get
(31) 
which takes the form, using equation (26),
(32) 
where has been introduced before. Thus, for a given , the curvature deviation increases towards its attractor , for which the departure from the Friedmannian curvature is maximum. For the curvature deviation is initially set to and then does not evolve. It is important to remark that there exists an infinite number of couples or, equivalently, which yield the same under the Chaplygin fluid constraints. For all of them will live on the same iso– curve and will tend towards the same attractor (see figure 1).
4.4 Evolution of the backreaction
For large values of the scale factor, , we have
(33) 
or, equivalently, using equation (26),
(34) 
where has been introduced before. The backreaction tends at late times towards a domain–dependent cosmological constant whose value is given by the initial conditions and on the domain. The same remark as in subsection 4.3 can be made for . One needs to distinguish the following cases (see figure 1).

For the backreaction is always positive and hence only acts as dark energy over the domain. In this situation, since is negative, behaves as dark energy whose intensity decreases until reaching the attractor . We recall in this case the existence of a minimal scale factor . implies .

For the system is initially set on the attractor; thus it does not evolve. The backreaction always acts as a cosmological constant.

for we have a positive . Two subcases arise according to the initial value :

for the backreaction acts as dark energy whose intensity increases until reaching the attractor ;

for the backreaction changes its sign during its evolution. It first behaves as dark matter whose intensity decreases, and then as dark energy whose intensity increases until reaching the attractor. The moment of the transition dark matter–dark energy depends on the initial values of the domain since .

We conclude by emphasizing some of the characteristics of the model. First, the CG relates the backreaction terms of our inhomogeneous universe model and therefore furnishes a particular manifestation of its inhomogeneous structure. Our model does not suppose the existence of any other fundamental field, contrary to the approach of a FLRW universe filled with dust and CG. Second, the role and the evolution of the backreaction depend on the domain considered and on its initial values. As a consequence this model could be seen as an effective multi–scale model. For instance might act as dark matter on small scales (situation (iii)(b)) with a dark energy transition occuring at very late times, and as different kinds of dark energy on larger scales (situations (i), (ii) and (iii)(a)).
4.5 Another approach: the backreaction fluid as a scalar field
The backreaction fluid might also be described by a minimally coupled real scalar field , called the morphon field [18], evolving in an effective potential , as follows:
(35) 
where for a standard scalar field (with a positive kinetic energy) and for a phantom scalar field (with a negative kinetic energy). The last expressions together with relations (8) give
(36) 
The system evolves towards the maximal value of the curvature deviation , as seen in subsection 4.3, which corresponds to the minimal value of the potential. With correspondence (36) the integrability condition (12) implies that , for , obeys the scale–dependent Klein–Gordon equation
(37) 
The above correspondence allows us to interpret the kinematical backreaction effects in terms of the properties of scalar field cosmologies, notably quintessence or phantom–quintessence scenarii that are here routed back to models of inhomogeneities. The morphon field may also be characterized by the domain–dependent equation of state , which assumes in our model the form
(38) 
For , the morphon field acts as dark matter and ‘standard’ dark energy as mentioned in subsection 3.1. In this situation we have and at late times. For , it behaves as phantom dark energy as mentioned in subsection 3.2. In this case we have, since , and at late times. We stress again that the phantom character is an effective property in our description; no fundamental phantom field is assumed to exist [18]. Finally, for , the morphon field mimics a scale–dependent cosmological constant and we have .
(39)  
(40) 
The scalar field dynamics can be reconstructed by evaluating the following integral, e.g. to find :
(41) 
where the prime denotes the derivation w.r.t. the volume scale factor. This relation does not seem analytically integrable in the general case. In the vacuum with a zero–Friedmaniann curvature (), expression (41) becomes
(42) 
From this last relation, we get the following expression for a standard scalar field ( and ):
(43) 
where is an integration constant. The potential is then written [34]
(44) 
For a phantom scalar field ( and ) we get from the relation (42)
(45) 
and the potential reads
(46) 
Note that this last expression can be obtained directly from relation (44) by the simple reparametrization . This is obvious in view of the form of the kinetic term of the morphon field: for a standard scalar field it is written and for a phantom field .
In the following section, we reformulate the different results obtained in this section in terms of effective cosmological parameters and we study the dynamics of the model.
5 Effective cosmological parameters
5.1 Constraints and evolution equations for the cosmological parameters
Expressed through the domain–dependent cosmological parameters
(47)  
(48) 
where is the volume Hubble functional, the averaged Hamiltonian constraint (1) assumes the form [19]
(49) 
The Chaplygin fluid constraints (22) may be expressed as
(50) 
(51)  
(52) 
where the new terms are defined by
(53) 
The sign of determines the behaviour of and . One may reformulate constraints (50) in terms of the initial conditions,
(54) 
5.2 Evolution of the Hubble functional
Equation (49) together with equations (51) and (52) provide the evolution equation for the Hubble functional (see appendix A for the study of in a particular case):
(55) 
tends, at late times, towards
(56) 
5.3 Evolution of the cosmological density parameters
One finds, for large values of the scale factor,
(57) 
It is interesting to note that the cosmological parameters tend towards a value independent of the initial conditions (see appendix A for the study of and in a particular case). We may also introduce the cosmological parameter , the so–called X–matter, defined as
(58) 
We have noticed in section 2 that the kinematical backreaction might explain the origin of dark matter and dark energy, and we have presented its behaviour in subsection 4.4. If one wants to compare our model to a scale–dependent Friedmannian cosmology in terms of cosmological parameters, has to be considered as the origin of the dark components, instead of alone. This simply means that the curvature deviation, since it also participates in the departure from the Friedmannian framework, may also act, qualitatively, as the dark components. In fact we know from previous work that the curvature deviation is actually quantitatively more important than the backreaction term itself [19].
We depict in figure 2 two situations to illustrate our model. The initial moment is chosen to be the epoch of the CMB, and we set ^{6}^{6}6This choice allows us to roughly compare our model to the concordance model. In this situation we have ., and . In the upper figure, the X–matter only stands for dark energy; corresponds to (the dark energy in the concordance model) and to (respectively the baryons and the dark matter in the concordance model). In the lower figure, the X–matter stands for dark energy and dark matter (since it can play both roles, it is regarded in this case as a result of different contributions on different scales); corresponds to and to . The two situations describe a universe initially close to a homogeneous–isotropic Friedmannian universe () with zero–curvature (). This low deviation, however, becomes larger with the growth of the scale factor to reach in the first case (where the superscript denotes the ‘today’–value), and in the second case ^{7}^{7}7If we choose the initial moment to be the CMB epoch, is chosen to roughly correspond to the ‘today’–value of the scale factor in a Friedmannian cosmology. Under the assumption that the metric of our universe does not significantly differ from a Euclidean metric, the scale factor, calculated through this metric (equation (5)), evolves in our model approximately like its Friedmannian counterpart. Thus, we are entitled to assume . However, backreaction terms, encoding the inhomogeneities, involve first and second derivatives of the metric and can therefore not be neglected, even if the metrical amplitudes are considered to be near–Euclidean (see the discussion in [17] and numerical applications therein).. The origin and magnitude of the dark energy (first situation) and of both dark energy and dark matter (second situation) are then entirely explained by the particular geometrical structure of an inhomogeneous space obeying the Chaplygin equation of state.
5.4 Another approach: the morphon equation of state
Using the effective cosmological parameters, we rewrite equation (38) as
(59) 
5.5 Dynamics of the fluid volume
Depending on the initial conditions, the domain might undergo a decelerated or an accelerated expansion at different periods of its evolution. To learn how it behaves we throw an eye on the volume deceleration parameter
(60) 
At late times, since , the fluid volume undergoes an accelerated expansion, we are indeed dealing with a cosmological constant in this situation. Three different cases occur for the dynamics of the domain (see figure 4, and appendix A for a detailed analysis in a particular case):

its expansion is first decelerated then accelerated;

its expansion is always accelerated;

its expansion is accelerated, then decelerated and again accelerated.
The latter case is an interesting situation: the kinematical backreaction is responsible for two accelerated phases. Our model only concerns the matter–dominated universe; however this situation allows to imagine that the primordial inflation and the one occuring today might be driven by the same effect studied in a more general model.
6 Concluding Remarks
We have built in this paper a model in which the backreaction fluid acts as a domain–dependent effective CG, focusing for simplicity on the case where its effective energy density is positive. The behaviour of the kinematical backreaction only depends on the initial conditions of the domain and may correspond to dark matter or different types of dark energy according to the scale and the time evolution. Our model kinematically resembles a Friedmannian cosmology with two fluids (dust and CG), but conceptual implications differ. First, the origin of dark energy (or, in the extreme case, of both dark components) is related to the non–trivial geometrical structure of an inhomogeneous space; we do not assume the existence of other fundamental constituents or fields. Second, the geometrical structure that complies with the Chaplygin equation of state can in principle be verified by concrete inhomogeneous models and also observationally; the model is no longer phenomenological in the sense that no free parameters remain. Free parameters in the standard approach (being homogeneous) are here traced back to the initial data for the inhomogeneities and are therefore, in this sense, not arbitrary. Any fitting of observational data of our model will lead to unambiguous initial data that can be constraint by structure formation. Third, one has to be careful when cosmological observables are derived. Indeed, angular diameter and luminosity distances, for instance, depend on metrical properties. These latter are affected and related, in our description, to the averaged scalar curvature, which evolves differently compared with its Friedmannian counterpart. It is therefore necessary to reinterprete observational data, using e.g. the lines of the analysis performed for the exact scaling solutions in [38]. In light of this remark it is premature to exclude [1, 6, 7, 24] the standard Chaplygin equation of state as providing a good match with observational data. The construction of an effective metric for a cosmology with a Chaplygin backreaction fluid and a comparison with observations are the subjects of a future work.
Acknowledgements:
We wish to thank Charly Nayet and Brice Riba for useful discussions. Also, we wish to thank Ugo Moschella, Alexander Kamenshchik, Roberto Sussman and Gary Tupper for their useful comments on the manuscript and interesting suggestions. This work was supported by ‘Fédération de Physique André Marie Ampère’. XR acknowledges support by École Doctorale, Lyon.
References
References
 [1] L. Amendola, F. Finelli, C. Burigana and D. Carturan: WMAP and the generalized Chaplygin gas. JCAP 0307, 005 (2003)
 [2] P. P. Avelino, L. M. G. Beca, J. P. M. de Carvalho, C. J. A. P. Martins and P. Pinto: Alternatives to quintessence model building. Phys. Rev. D 67, 023511 (2003)
 [3] R. Bean and O. Dore: Are Chaplygin gases serious contenders for the dark energy? Phys. Rev. D 68, 023515 (2003)
 [4] J. Behrend: Metric renormalization in general relativity. arXiv:0812.2859 (2008)
 [5] M. C. Bento, O. Bertolami and A. A. Sen: Generalized Chaplygin gas, accelerated expansion and dark energy–Matter unification. Phys. Rev. D 66, 043507 (2002)
 [6] M. C. Bento, O. Bertolami and A. A. Sen: Generalized Chaplygin gas model: dark energy  dark matter unification and CMBR constraints. Gen. Rel. Grav. 35, 2063 (2003)
 [7] M. C. Bento, O. Bertolami and A. A. Sen: WMAP constraints on the generalized Chaplygin gas model. Phys. Lett. B 575, 172 (2003)
 [8] N. Bilic, G. B Tupper and R. D. Viollier: Unification of dark matter and dark energy: the inhomogeneous Chaplygin gas. Phys. Lett. B 535, 17 (2002)
 [9] N. Bilic, R. J. Lindebaum, G. B. Tupper and R. D. Viollier: Nonlinear evolution of dark matter and dark energy in the Chaplygin gas cosmology. JCAP 0411, 008 (2004)
 [10] N. Bilic, G. B Tupper and R. D. Viollier: Cosmological tachyon condensation. Phys. Rev. D 80, 023515 (2009)
 [11] K. Bolejko and L. Andersson: Apparent and average acceleration of the universe. JCAP 0810, 003 (2008)
 [12] M. Bordemann and J. Hoppe: The dynamics of relativistic membranes. Reduction to 2–dimensional fluid dynamics. Phys. Lett. B 317, 315 (1993)
 [13] T. Buchert: On average properties of inhomogeneous fluids in general relativity: 1. dust cosmologies. Gen. Rel. Grav. 32, 105 (2000)
 [14] T. Buchert: On average properties of inhomogeneous fluids in general relativity: 2. perfect fluid cosmologies. Gen. Rel. Grav. 33, 1381 (2001)
 [15] T. Buchert: A cosmic equation of state for the inhomogeneous universe: can a global far–from–equilibrium state explain dark energy? Class. Quant. Grav. 22, L113 (2005)
 [16] T. Buchert: On globally static and stationary cosmologies with or without a cosmological constant and the dark energy problem. Class. Quant. Grav. 23, 817 (2006)
 [17] T. Buchert, G. F. R. Ellis and H. Van Elst: Geometrical order–of–magnitude estimates for spatial curvature in realistic models of the universe. Gen. Rel. Grav. 41, 2017 (2009)
 [18] T. Buchert, J. Larena and J.–M. Alimi: Correspondence between kinematical backreaction and scalar field cosmologies – the ’morphon field’. Class. Quant. Grav. 23, 6379 (2006)
 [19] T. Buchert: dark energy from structure – a status report. Gen. Rel. Grav. 40, 467 (2008)
 [20] D. Carturan and F. Finelli: Cosmological effects of a class of fluid dark energy models. Phys. Rev. D 68, 103501 (2003)
 [21] M.–N. Célérier, K. Bolejko, A. Krasiński, C. Hellaby: A (giant) void is not mandatory to explain away dark energy with a Lemaître–Tolman model. arXiv:0906.0905 (2009)
 [22] L. P. Chimento, A. S. Jakubi and D. Pavo: dark energy, dissipation, and the coincidence problem. Phys. Rev. D 67, 087302 (2003)
 [23] L. P. Chimento: Extended tachyon field, Chaplygin gas, and solvable kessence cosmologies. Phys. Rev. D 69, 123517 (2004)
 [24] J. V. Cunha, J. S. Alcaniz and J. A. S. Lima: Cosmological constraints on Chaplygin gas dark energy from galaxy clusters X–ray and supernova data. Phys. Rev. D 69, 083501 (2004)
 [25] A. Dev, J. S. Alcaniz and D. Jain: Cosmological consequences of a Chaplygin gas dark energy. Phys. Rev. D 67, 023515 (2003)
 [26] G.F.R. Ellis: Relativistic cosmology: its nature, aims and problems. In General Relativity and Gravitation (D. Reidel Publishing Company, Dordrecht, 1984), pp. 215–288
 [27] G.F.R. Ellis and T. Buchert: The universe seen at different scales. Phys. Lett. A. (Einstein Special Issue) 347, 38 (2005)
 [28] K. Enqvist: Lemaître Tolman Bondi model and accelerating expansion. Gen. Rel. Grav. 40, 451 (2008)
 [29] J. C. Fabris, S. V. B. Goncalves and P. E. de Souza: Density perturbations in a universe dominated by the Chaplygin gas. Gen. Rel. Grav. 34, 53 (2002)
 [30] J. C. Fabris, S. V. B. Goncalves and P. E. de Souza: Mass power spectrum in a universe dominated by the Chaplygin gas. Gen. Rel. Grav. 34, 2111 (2002)
 [31] V. Gorini, A. Kamenshchik and U. Moschella: Can the Chaplygin gas be a plausible model for dark energy? Phys. Rev. D 67, 063509 (2003)
 [32] V. Gorini, A. Kamenshchik, U. Moschella and V. Pasquier: The Chaplygin gas as a model for dark energy. In: Proc. MG10, Rio de Janeiro, Brazil, 2026 July 2003, M. Novello, S. Perez Bergliaffa, R. Ruffini (eds.). World Scientific, p. 840 (2005)
 [33] R. Jackiw and A. P. Polychronakos: Supersymmetric fluid mechanics. Phys. Rev. D 62, 085019 (2000)
 [34] A. Kamenshchik, U. Moschella and V. Pasquier: An alternative to quintessence. Phys. Lett. B 511, 265 (2001)
 [35] E.W. Kolb, V. Marra and S. Matarrese: Description of our cosmological spacetime as a perturbed conformal Newtonian metric and implications for the backreaction proposal for the accelerating universe. Phys. Rev. D 78 103002 (2008)
 [36] E.W. Kolb, V. Marra and S. Matarrese: Cosmological background solutions and cosmological backreactions. arXiv:0901.4566 (2009)
 [37] E. W. Kolb and C. R. Lamb: Light–cone observations and cosmological models: implications for inhomogeneous models mimicking dark energy. arXiv:0911.3852 (2009)
 [38] J. Larena, J.–M. Alimi, T. Buchert, M. Kunz and P.–S. Corasaniti: Testing backreaction effects with observations. Phys. Rev. D 79, 083011 (2009)
 [39] N. Li and D. J. Schwarz: On the onset of cosmological backreaction. Phys. Rev. D 76, 083011 (2007)
 [40] A. Paranjape and T. P. Singh: The possibility of cosmic acceleration via spatial averaging in Lemaître–Tolman–Bondi models. Class. Quant. Grav. 23, 6955 (2006)
 [41] S. Räsänen: Accelerated expansion from structure formation. JCAP 0611, 003 (2006)
 [42] M.R. Setare: Interacting generalized Chaplygin gas model in nonflat universe. Eur. Phys. J. C 52, 689 (2007)
 [43] R.A. Sussman: Quasi–local variables, non–linear perturbations and backreaction in spherically symmetric spacetimes. arXiv:0809.3314 (2008)
 [44] R.A. Sussman: Quasi–local variables and inhomogeneous cosmological sources with spherical symmetry. AIP Conf. Proc. 1083, pp. 228235 (2008)
 [45] R.A. Sussman: Quasi–local variables in spherical symmetry: numerical applications to dark matter and dark energy sources. Phys. Rev. D 79, 025009 (2009)
 [46] A. Wiegand and T. Buchert: Multiscale cosmology and structure–emerging dark energy: a plausibility analysis. Phys. Rev. D 82, 023523 (2010)
Appendix A. Study of the model in the case
Setting to 0 allows to compare our model to the concordance model (we also suppose here that for any domain). In this situation equation (49) becomes
(A.1) 
Since and are both positive under the Chaplygin fluid constraints (see equation (50)), one also needs
(A.2) 
A.1. Evolution of the Hubble functional
Equation (55) becomes
(A.3) 
For always decreases, and for it increases in the interval and decreases in with
(A.4) 
A.2. Evolution of and
The derivatives of equations (51) and (52) show that, for , increases and decreases. For , decreases in and increases in , and increases in and decreases in , with
(A.5)  
(A.6) 
A.3. Evolution of the deceleration parameter
We define the quantities
(A.7)  
(A.8)  
(A.9)  
(A.10)  
(A.11)  
(A.12) 
and the situations