# Cosmological models in modified gravity theories with extended nonminimal derivative couplings

###### Abstract

We construct gravitational modifications that go beyond Horndeski, namely theories with extended nonminimal derivative couplings, in which the coefficient functions depend not only on the scalar field but also on its kinetic energy. Such theories prove to be ghost-free in a cosmological background. We investigate the early-time cosmology and show that a de Sitter inflationary phase can be realized as a pure result of the novel gravitational couplings. Additionally, we study the late-time evolution, where we obtain an effective dark energy sector which arises from the scalar field and its extended couplings to gravity. We extract various cosmological observables and analyse their behavior at small redshifts for three choices of potentials, namely, for the exponential, the power-law, and the Higgs potential. We show that the Universe passes from deceleration to acceleration in the recent cosmological past, while the effective dark-energy equation-of-state parameter tends to the cosmological-constant value at present. Finally, the effective dark energy can be phantom-like, although the scalar field is canonical, which is an advantage of the model.

###### pacs:

04.50.Kd, 98.80.-k, 95.36.+x## I Introduction

Horndeski’s theory Horndeski:1974wa is the most general single-scalar tensor theory that has second-order field equations, both for the metric and the scalar field in four dimensions. It was originally discovered in 1974, then rediscovered independently Deffayet:2011gz , and recently been brought back to attention fab4 ; Charmousis:2011bf ; Kobayashi:2011nu (for a review see Charmousis:2014mia ). The generality of the theory is reminiscent of Lovelock’s theorem Lovelock:1971yv and it comes as no surprise that many of its terms, especially those that involve derivative couplings of the scalar with curvature terms, come from a dimensional reduction of higher dimensional Lovelock theories VanAcoleyen:2011mj . Note that having second-order field equations is crucial, in order to avoid Ostrogradski instabilities ostro ; Woodard:2006nt ; Woodard:2015zca .

The advantage of Horndeski cosmological models is that they are able to screen the vacuum energy coming from any field theory, assuming that after this screening the space should be in a de Sitter vacuum Martin-Moruno:2015bda ; Martin-Moruno:2015eqa . These models allow us to understand the current accelerated expansion of the Universe as the result of a dynamical evolution towards a de Sitter attractor Martin-Moruno:2015lha . Thus, it was shown that Horndeski models with a de Sitter critical point for any kind of material content may provide a mechanism to alleviate the cosmological constant problem Martin-Moruno:2015kaa . The cosmological scenario that results when considering the radiation and matter content was also studied, and it was concluded that their background dynamics is compatible with the latest observational data.

Despite the huge interest in these theories, extensions of Horndeski’s theory have also been recently discussed. In Gleyzes:2014dya a new class of scalar-tensor theories was introduced, going beyond Horndeski’s theory, where despite the fact that the equations of motion contain higher derivatives, they can be cast in a way that they contain only second-order ones Zumalacarregui:2013pma . Additionally, these generalized theories were shown to be free of ghost instabilities in the unitary gauge Gleyzes:2014qga , and later on this was also verified using the Hamiltonian formalism Domenech:2015tca ; Langlois:2015cwa ; Deffayet:2015qwa ; Langlois:2015skt ; Crisostomi:2016tcp , due to the existence of a primary constraint which prevents the propagation of extra degrees of freedom Crisostomi:2016tcp (see also Gao:2014soa and Crisostomi:2016czh ; Ezquiaga:2016nqo ; BenAchour:2016fzp for additional descriptions). We mention that these extended theories can also address the cosmological constant problem Babichev:2015qma via a self-tunning mechanism, similarly to the analysis done in the original Horndeski theory for the so-called Fab Four theory fab4 ; Charmousis:2011bf (the cosmological aspects of the Fab-Four have been explored in Copeland:2012qf ). A detailed analysis of the cosmological self-tunning and local solutions in the context of beyond Horndeski theories has also been explored in Babichev:2016kdt . Recently, it was shown that the two additional Lagrangian pieces, appearing in theories beyond Horndeski, could be re-expressed in a very elegant and compact way, by allowing the potentials to also depend on the kinetic term of the scalar field Babichev:2015qma .

One interesting subclass of Horndeski theory, which has been given much attention recently, includes the nonminimal (kinetic) coupling of matter to gravity by inserting derivative couplings between the geometry and the kinetic part of the scalar field Amendola:1993uh , which leads to interesting new dynamical cosmological phenomena Sushkov:2009hk ; Saridakis:2010mf , including the existence of an effective cosmological constant Capozziello:1999uwa ; Capozziello:1999xt . The nonminimal derivative coupling leads to cosmological models with rich phenomenology, such as solutions containing a Big Bang, expanding Universes with no beginning, cosmological bounces, eternally contracting Universes, a Big Crunch, and a Big Rip avoidance Saridakis:2010mf ; Granda:2010ex ; Granda:2010hb ; Sadjadi:2010bz ; Sami:2012uh ; Banijamali:2012kq ; Bruneton:2012zk ; Sheikhahmadi:2016wyz . In particular, it was shown that one is able to explain in a unique manner both a quasi-de Sitter phase and an exit from it without any fine-tuned potential Sushkov:2009hk . Furthermore, one can successfully describe the sequence of cosmological epochs without any fine-tuned potential Sushkov:2012za . Using couplings of this type, it was found that in the absence of other matter sources or in the presence of only pressureless matter, the scalar field behaves as pressureless matter and its sound speed is vanishing Gao:2010vr . These properties enable the scalar field to be a candidate of cold dark matter. It was also shown that if the kinetic term is coupled to more than one Einstein tensor, then the equation of state is always approximately equal to , independently from the potential flatness, and hence the scalar may also be considered a candidate for the inflaton. Tachyon models involving nonminimal derivative coupling have also been explored Shchigolev:2011nma ; Banijamali:2011qb , while Chaplygin gas model in this framework were studied in Granda:2011zy . Moreover, the dynamics of entropy perturbations in the two-field assisted dark energy model with mixed kinetic terms was also studied in Karwan:2010xw . Recently there has also been an investigation on how the derivative coupling can mimic cold dark matter at cosmological level and also explain the flattening of galactic rotation curves Rinaldi:2016oqp .

The inflationary context within this theory has been extensively analysed too. In the case of a power-law potential, and using the dynamical system method, all possible asymptotical regimes of the model were analysed Skugoreva:2013ooa . It was shown that for sloping potentials there exists a quasi-de Sitter asymptotic corresponding to an early inflationary Universe. In contrast to standard inflationary scenario, the kinetic-coupling inflation does not depend on a scalar field potential and is only determined by the coupling parameter. In addition to this, there is a unique nonminimal derivative coupling of the Standard Model Higgs boson to gravity which propagates no more degrees of freedom than General Relativity sourced by a scalar field, and reproduces a successful inflating background within the Standard Model Higgs parameters and, finally, does not suffer from dangerous quantum corrections Germani:2010gm . The slow-roll conditions have been found Granda:2011zk , and the reheating temperature was obtained Sadjadi:2012zp ; Sadjadi:2013na (see also recent analyses in Gumjudpai:2016ioy and Dalianis:2016wpu ). Furthermore, the cosmological perturbations originated at the inflationary stage were studied and the consistency of the results with observational constraints coming from Planck 2013 data were investigated Sadjadi:2013psa . Moreover, these scenarios exhibit a gravitationally enhanced friction during inflation, where even steep potentials with theoretically natural model parameters can drive cosmic acceleration Tsujikawa:2012mk , while being compatible with the current observational data mainly due to the suppressed tensor-to-scalar ratio. Finally, the gravitational production of heavy -particles of mass of the order of the inflaton mass, produced after the end of inflation, was also studied Koutsoumbas:2013boa , where it was found that this production is suppressed as the strength of the coupling is increased.

A combined perturbation and observational investigation of the scenario of nonminimal derivative coupling between a scalar field and curvature was performed in Dent:2013awa . Using Type Ia Supernovae (SNIa), Baryon Acoustic Oscillations (BAO), and Cosmic Microwave Background (CMB) observations, it was shown that, contrary to its significant effects on inflation, the nonminimal derivative coupling term has a negligible effect on the Universe acceleration, since it is driven solely by the usual scalar-field potential. Therefore, the scenario can provide a unified picture of early and late time cosmology, with the nonminimal derivative coupling term responsible for inflation, and the usual potential responsible for late-time acceleration.

Finally, nonminimal derivative couplings to gravity have also been explored in a variety of extended theories of gravity. For instance, one can incorporate an additional coupling to the Gauss Bonnet invariant, obtaining rich cosmological behavior, with both decelerated and accelerated phases Granda:2011eh ; Granda:2012hm . Additionally, a large class of scalar-tensor models with interactions containing the second derivatives of the scalar field but not leading to additional degrees of freedom have also been extensively investigated Deffayet:2010qz . These models exhibit peculiar features, such as an essential mixing of scalar and tensor kinetic terms, named kinetic braiding, and possess a rich cosmological phenomenology, including a late-time asymptotic de Sitter state, and a possible phantom-divide crossing, with neither ghosts nor gradient instabilities. Finally, the nonminimal derivative coupling to gravity has also been investigated in the context of the curvaton model Feng:2013pba , or in the framework of four-dimensional new-minimal supergravity Farakos:2012je .

In this work we are interested in investigating a theory that goes beyond Horndeski, based on a generalization of nonminimal derivative coupling. In particular, we consider the latter coupling and introduce an additional arbitrary coefficient-function of the field and its derivatives. We mention that this class is not included in Horndeski theory, since only specific combinations of it are allowed Deffayet:2011gz ; Gleyzes:2013ooa ; Gleyzes:2014rba . This paper is outlined in the following manner. In Section II, we present the action and deduce the gravitational field equations. In Section III, we apply the developed formalism to a spatially flat Friedmann-Robertson-Walker (FRW) background metric, and present the modified Friedmann equations. The early-time cosmology is briefly analysed in Section IV, and the late-time evolution is considered in Section V. In the latter, we study the full Friedmann equations and focus on important observables, by considering three well-known scalar potentials, such as the exponential, power-law and the Higgs potential. Finally, in Section VI we discuss our results and conclude.

## Ii Extended nonminimal derivative coupling

In this work, we consider a generalized nonminimal coupling of the scalar field derivative to gravity, by introducing an additional arbitrary coefficient-function of the field and its derivatives. The action is given by

(1) |

with the metric, , the scalar curvature, and the derivative coupling parameters, the scalar field potential, the scalar kinetic energy and an arbitrary function. Note that in principle can be absorbed inside , however we prefer to keep it separately in order to be able to reproduce at any stage the results of the simple nonminimal derivative coupling by setting to . Finally, we have included the usual matter action, corresponding to a matter fluid of energy density and pressure .

Variation of the action with respect to the metric leads to the field equations

(2) |

where is the double dual of the Riemann tensor defined as mtw

(3) |

and where . Additionally, variation of the action (1) with respect to provides the scalar field equation of motion, namely

(4) |

In this work we will consider the case where , which is adequate to capture the new features of the theories beyond Horndeski at hand. Hence the coupling constant has dimensions of inverse mass to the power of six while has dimensions of inverse mass to the power of two. Using the identity

(5) |

and the fact that apart from the potential term the rest of the action is shift symmetric, we can now write our field equations in the following elegant way

(6) |

and

(7) |

where

(8) |

## Iii Cosmological Equations

In this section we are interested in investigating the cosmological implications of theories with extended nonminimal derivative couplings. Hence, we focus on a spatially-flat Friedmann-Robertson-Walker (FRW) background metric of the form

(9) |

where is the cosmic time, are the comoving spatial coordinates, is the scale factor and is the Hubble parameter, (a dot denotes differentiation with respect to ). Additionally, we consider the scalar field to be homogeneous, that is . Finally, as usual, we consider the matter sector to correspond to a perfect fluid.

In this case, the field equations (II) provide the two Friedmann equations:

(10) |

(11) |

while equation (7) gives

(12) |

As we can easily see, despite the appearance of higher derivatives in Eq. (II), on the cosmological background they disappear Gleyzes:2014dya , and we only have to deal with up to two derivatives. From the above expressions one can see that the Friedmann equations (10) and (11) can be written in the usual form, namely

(13) | |||||

(14) |

where we have defined an effective dark energy sector with energy density and pressure:

(15) |

(16) |

respectively. Therefore, in the scenario at hand, the dark-energy equation-of-state parameter is given by

(17) |

One can straightforwardly see that, in terms of the dark energy density and pressure, the scalar field evolution equation (12) can be written in the standard form

(18) |

Furthermore, the matter energy density and pressure satisfy the standard evolution equation

(19) |

Finally, we introduce the deceleration parameter , which is an indicator of the accelerated expansion, and is defined as

(20) |

and thus negative values of correspond to accelerating evolution. Additionally, in order to allow for an easy comparison between the observational and theoretical results, instead of the time variable we can use the redshift , defined as

(21) |

where we have normalized the scale factor so that its current value is . Thus, time derivatives can be expressed as

(22) |

## Iv Early-time cosmology

In order to examine the early-time behavior of the scenario at hand we will neglect the matter content of the theory. We are interested in exponential cosmological solutions, which could describe the inflationary epoch. Note that since we desire to study the pure effects of the novel, extended nonminimal derivative couplings, we do not consider an explicit potential, since it is well known that a potential term can easily drive an exponential solution, with the best example being a simple cosmological constant.

Using the metric (9) we examine whether the cosmological equations (10)–(12) admit solutions in which the scale factor has an exponential dependence in time of the form

(23) |

with a constant. Inserting this in the first Friedmann equation (10), and setting as usual , we can easily see that the general solution for the scalar field has a linear time dependence, thus we depict our solution for the scalar field as

(24) |

where are integration constants, which will be determined in the following, in order for the full system of equations to be satisfied. Inserting this expression for the scalar field in the Klein-Gordon equation (12) we deduce that it is satisfied if

(25) |

Substituting back to the Friedmann equations (10) and (11), we obtain

(26) |

Hence and are both positive, namely

(27) | |||||

(28) |

In summary, we can see that the scenario at hand easily admits de-Sitter solutions, that can describe the inflationary epoch of the Universe. In particular, for a given set of coupling parameters and , one obtains the de-Sitter solution (23), with the scalar field evolving as in Eq. (24), where the solution parameters and are determined by inverting Eqs. (27) and (28). The only requirement is the obtained and to be real numbers, and this constrains the allowed parameter space. For instance, note that if one of or is zero, the system does not admit an exponential solution unless there is a bare cosmological constant. We stress that the above de-Sitter solution has been obtained without considering a potential term, i.e. it is an effect of the extended nonminimal derivative coupling terms considered in this work.

In general, at early times, where matter can be neglected, we can express the deceleration parameter (20) using the Friedmann equations (10) and (11) as

(29) |

where we have defined the “total” equation-of-state parameter of the Universe as

(30) |

Hence, the condition for accelerated expansion can then be formulated as , or equivalently

(31) |

where for generality we have kept the potential term. Hence, one can use this requirement in order to find more general inflationary solutions, beyond the de-Sitter one.

## V Late-time cosmology

In the present Section we investigate several cosmological models in the framework of gravitational theories with an extended nonminimal derivative coupling, focusing on the late-time evolution. In particular, we are interested in studying the full Friedmann equations (13) and (14), i.e., considering the matter sector as well, and we focus on important observables such as the dark-energy equation-of-state parameter defined in (17), and the dark-matter and dark-energy density parameters defined respectively as

(32) |

Additionally, concerning the scalar potential we will consider three well-known cases, namely the exponential potential Copeland:1997et ; Ferreira:1997au ; Chen:2008ft ; exsol1 ; exsol2 :

(33) |

with and constants, the power-law potential Abramo:2003cp ; Saridakis:2009pj :

(34) |

with and constants, and the Higgs potential Lyth:1995hj :

(35) |

where is a constant, while the constant may be related to the mass of the Higgs boson by the relation , where gives the minimum of the potential.

In general, in the above cases, and in the presence of matter, analytical solutions are impossible to be extracted, and thus we resort to numerical elaboration of the cosmological equations. Thus, we evolve the equations using as independent variable the redshift defined in (21).

In order to perform a numerical elaboration of the above cosmological equations, it proves convenient to re-write them in dimensionless way. In particular, we introduce the dimensionless variables , defined as

(36) | |||

(37) |

Using these new variables, the generalized Friedmann equations (10), (11), the scalar field equation (12), as well as the matter conservation equation (19), take the form

(38) |

(39) |

(40) |

(41) |

respectively. Therefore, after solving Eqs. (39) and (40) for and , the cosmological field equations take the form

(42) |

(43) |

(44) | |||||

(45) |

which must be solved together with Eq. (41) after the equation of state of matter has been imposed. The initial conditions for the system (42)-(45) are , , , and , respectively. Furthermore, in terms of the dimensionless variables the deceleration parameter (20) becomes

(46) |

while the dark-energy equation-of-state parameter reads as

(47) |

Finally, the dimensionless time-redshift relation (22) becomes

(48) |

### v.1 Exponential potential

Let us start the analysis by considering the exponential potential (33), namely

(49) |

with and the potential parameters. In terms of the dimensionless variables introduced in (36), the above exponential potential takes the form

(50) |

where

(51) |

In the following we consider the time evolution of a dust matter fluid, namely we assume that , and hence the redshift dependence of the auxiliary matter energy density is given by . In this case, the dimensionless cosmological equations (42), (44) and (45) become

(52) |

(53) | |||||

(54) |

respectively. Additionally, the parameter of the dark energy equation of state (17) reads as

(55) |

A crucial observation is that according to the above expression, could acquire values below too, and thus the phantom regime can be exhibited. This is an advantage of the scenario at hand, since such a behavior is obtained although the scalar field is canonical, that it is a pure result of the extended, gravitational couplings.

In order to study the cosmological evolution of the dust Universe in the presence of the exponential potential we integrate the system of Eqs. (52)-(54) numerically. We choose the potential parameters as , and , while for the initial conditions we set , , and . We are interested in studying the effect of the parameters and , that determine the novel, extended nonminimal derivative coupling, on the cosmological evolution, restricting the analysis at late times, i.e., at the redshift range .

In Fig. 1, we depict the evolution of the Hubble function, of the scalar field, of the deceleration parameter, and of the dark-energy equation-of-state parameter, in terms of the redshift, for various values of and .

As we can see, the Hubble function, represented in the top left figure, is a monotonically increasing function of the redshift, indicating an expansionary cosmological evolution, while in the redshift range it remains almost constant. Its variation is not affected significantly by the change of the numerical values of the coupling parameters. Moreover, the dimensionless scalar field, depicted in the top right figure, is a monotonically decreasing function of the redshift, and therefore an increasing function of the cosmological time. Note that the scalar field behavior is strongly affected by variations of the numerical values of and . The deceleration parameter, shown in the bottom left figure, starts with high positive values, however acceleration arises quickly, with crossing zero at a redshift . The variations of the coupling parameters have a small influence on the deceleration parameter behavior. Finally, the parameter of the dark energy equation of state, presented in the bottom right figure, starts with values of the order of at , it reaches zero at , and tends to at , indicating that the dark energy sector behaves like a cosmological constant at present. Similarly to the case of the dimensionless Hubble parameter, the changes in the numerical values of the parameters and have small influence on evolution.

### v.2 Power-law potential

Let us now investigate the cosmological evolution in the extended nonminimal derivative coupling gravitational theory in the presence of a simple power-law potential of the form (34), namely

(56) |

where and are constants. Hence, using the dimensionless variables introduced in (36), the dimensionless form of the power-law potential writes as

(57) |

where

(58) |

In the case of the dust Universe, namely imposing that , the dimensionless cosmological equations (42), (44) and (45) become

(59) |

(60) | |||||

(61) |

respectively. Additionally, the dark-energy equation-of-state parameter (17) writes as

(62) |

Similarly to the exponential potential case, we can see that can acquire values of the phantom regime, which is an advantage of the scenario at hand.

In order to study the cosmological evolution of the dust Universe in the presence of the power-law potential we integrate the system of Eqs. (59)-(61) numerically. We choose the potential parameters as and , and for the initial conditions we set , , and , and similarly to the exponential potential of the previous subsection we restrict our analysis at late times, namely, at the redshift range .

As in the previous case, in Fig. 2 we depict the evolution of the Hubble function, of the scalar field, of the deceleration parameter, and of the dark-energy equation-of-state parameter, in terms of the redshift, for various values of the coupling parameters and .

The evolution of the Hubble function, presented in the top left graph, shows that the Universe is expanding, with the Hubble function monotonically increasing with the redshift, while at and below the Hubble function becomes almost a constant. The behavior of the Hubble function is relatively strongly affected by changes in the values of the coupling parameters and , with the effect being stronger at higher redshifts. The dimensionless scalar field , depicted in the top right graph, is a monotonically decreasing function of the redshift, and at high redshifts it also presents a strong dependence on the numerical values of and . The deceleration parameter, presented in the bottom left graph, has positive values of the order of at , however acceleration is obtained at a redhift . Finally, the dark-energy equation-of-state parameter, presented in the bottom right graph, has values of the order of at , it reaches zero at redshifts , and it tends to at , implying that the dark energy sector behaves like a cosmological constant at present. We mention that both and exhibit a relatively strong dependence on the numerical values of and .

### v.3 Higgs potential

As a final case we investigate the cosmological implications of theories with extended nonminimal derivative coupling, in the presence of the Higgs potential (35), namely

(63) |

where is a constant, and where the constant can be related to the Higgs mass by the relation , with the minimum of the potential. Moreover, based on the determination of from accelerator experiments one can infer for the Higgs self-coupling constant a value of the order of Higgs . In terms of the dimensionless variables (36) the above Higgs-like potential becomes

(64) |

where

(65) |

In the following paragraphs we study separately the cases of dust and radiation, respectively.