I Introduction

Cosmological perturbations in warm-tachyon inflationary universe model with viscous pressure

M. R. Setare 111E-mail: rezakord@ipm.ir   , V. Kamali 222E-mail: vkamali1362@gmail.com

Department of Science, Campus of Bijar, University of Kurdistan, Bijar, Iran

Department of Physics, Faculty of Science,

Bu-Ali Sina University, Hamedan, 65178, Iran

Abstract

We study the warm-tachyon inflationary universe model with viscous pressure in high-dissipation regime. General conditions which are required for this model to be realizable are derived in the slow-roll approximation. We present analytic expressions for density perturbation and amplitude of tensor perturbation in longitudinal gauge. Expressions of tensor-to-scalar ratio, scalar spectral index and its running are obtained. We develop our model by using exponential potential, the characteristics of this model are calculated for two specific cases in great details: 1- Dissipative parameter and bulk viscous parameter are constant parameters. 2- Dissipative parameter is a function of tachyon field and bulk viscous parameter is a function of matter-radiation mixture energy density . The parameters of the model are restricted by recent observational data from the nine-year Wilkinson microwave anisotropy probe (WMAP9), Planck and BICEP2 data.

## I Introduction

Big Bang model has many long-standing problems (monopole, horizon, flatness,…). These problems are solved in a framework of inflationary universe models 1-i (). Scalar field as a source of inflation provides a causal interpretation of the origin of the distribution of Large-Scale Structure (LSS), and also observed anisotropy of cosmological microwave background (CMB) 6 (); planck (); BICEP2 (). The standard models for inflationary universe are divided into two regimes, slow-roll and reheating regimes. In the slow-roll period, kinetic energy remains small compared to the potential term. In this period, all interactions between scalar fields (inflatons) and other fields are neglected and as a result the universe inflates. Subsequently, in reheating epoch, the kinetic energy is comparable to the potential energy that causes inflaton to begin an oscillation around the minimum of the potential while losing their energy to other fields present in the theory. After the reheating period, the universe is filled with radiation.
In warm inflation scenario the radiation production occurs during inflationary period and reheating is avoided 3 (). Thermal fluctuations may be generated during warm inflationary epoch. These fluctuations could play a dominant role to produce initial fluctuations which are necessary for Large-Scale Structure (LSS) formation. In this model, density fluctuation arises from thermal rather than quantum fluctuation 3-i (). Warm inflationary period ends when the universe stops inflating. After this period, the universe enters in the radiation phase smoothly 3 (). Finally, remaining inflatons or dominant radiation fields create matter components of the universe. Some extensions of this model are found in Ref.new ().
In the warm inflation models there has to be continuously particle production. For this to be possible, then the microscopic processes that produce these particles must occur at a timescale much faster than Hubble expansion. Thus the decay rates (not to be confused with the dissipative coefficient) must be bigger than . Also these produced particles must thermalize. Thus the scattering processes amongst these produced particles must occur at a rate bigger than . These adiabatic conditions were outlined since the early warm inflation papers, such as Ref. 1-ne (). More recently there has been considerable explicit calculation from Quantum Field Theory (QFT) that explicitly computes all these relevant decay and scattering rates in warm inflation models 4nn (); arj ().
In warm inflation models, for simplicity, particles which are created by the inflaton decay are considered as massless particles (or radiation). Existence of massive particles in the inflationary fluid model as a new model of inflation was studied in Ref.41-i (). Perturbation parameters of this model were obtained in Ref.2-ne (). In this scenario the existence of massive particles alters the dynamic of the inflationary universe models by modification of the fluid pressure. Using the random fluid hydrodynamic fluctuation theory which is generalized by Landau and Lifsitz landa (), we can describe the cosmological fluctuations in the system with radiation and tachyon scalar field. Decay of the massive particles within the fluid is an entropy-producing scalar phenomenon. In the other hand, ”bulk viscous pressure” has entropy-producing property. Therefore, the decay of particles may be considered by a bulk viscous pressure , where is Hubble parameter and is phenomenological coefficient of bulk viscosity 3-ne (). This coefficient is positive-definite by the second law of thermodynamics and in general depends on the energy density of the fluid.
The Friedmann-Robertson-Walker (FRW) cosmological models in the context of string/M-theory have been related to brane-antibrane configurations 4-i (). Tachyon fields, associated with unstable D-branes, are responsible of inflation in early time 5-i (). The tachyon inflation is a k-inflation model n-1 () for scalar field with a positive potential . Tachyon potentials have two special properties, firstly a maximum of these potential is obtained where and second property is the minimum of these potentials is obtained where . If the tachyon field starts to roll down the potential, then universe, which is dominated by a new form of matter, will smoothly evolve from inflationary universe to an era which is dominated by a non-relativistic fluid 1 (). So, we could explain the phase of acceleration expansion (inflation) in terms of tachyon field.
Cosmological perturbations of warm inflation model (with viscous pressure) have been studied in Ref.9-f () (2-ne ()). Warm tachyon inflationary universe model has been studied in Ref.1-m (), also warm inflation on the brane (with viscous pressure) has been studied in Ref 6-f () (v-2 ()). To the best of our knowledge, a model in which warm tachyon inflation with viscous pressure has not been yet considered. In the present work we will study warm-tachyon inspired inflation with viscous pressure. The paper organized as follow: In the next section, we will describe warm-tachyon inflationary universe model with viscous pressure and the perturbation parameters for our model. In section (3), we study our model using the exponential potential in high dissipative regime. Finally in section (5), we close by some concluding remarks.

## Ii The model

In this section, we will obtain the parameters of the warm tachyon inflation with viscous pressure. This model may be described by an effective tachyon fluid and matter-radiation imperfect fluid. Tachyon fluid in a spatially flat Friedmann Robertson Walker (FRW) is recognized by these parameters 1 (); v-2 ()

 Tνμ=diag(−ρϕ,Pϕ,Pϕ,Pϕ) (1) Pϕ=−V(ϕ)√1−˙ϕ2, ρϕ=V(ϕ)√1−˙ϕ2,

Important characteristics of the potential are and 2 (). The imperfect fluid is a mixture of matter and radiation of adiabatic index which has energy density ( is temperature and is entropy density of the imperfect fluid.) and pressure where, . is bulk viscous pressure 3-ne (), where is phenomenological coefficient of bulk viscosity. The dynamic of the model in background level is given by the Friedmann equation,

 3H2=ρT=V(ϕ)√1−˙ϕ2+ρ, (2)

the conservation equations of tachyon field and imperfect fluid

 ˙ρϕ+3H(Pϕ+ρϕ)=−Γ˙ϕ2⇒¨ϕ1−˙ϕ2+3H˙ϕ+V′V=−ΓV√1−˙ϕ2˙ϕ, (3)

and

 ˙ρ+3H(ρ+P+Π)=˙ρ+3H(γρ+Π)=Γ˙ϕ2, (4)

where we have used the natural units () and . is the dissipative coefficient with the dimension . Dissipation term denotes the inflaton decay into the imperfect fluid in the inflationary epoch. In the above equations dots ”.” mean derivative with respect to cosmic time, prime denotes derivative with respect to the tachyon field . The energy density of radiation and the entropy density increase by the bulk viscosity pressure (see FIG.1 and FIG.2)v-2 ().

During slow-roll inflation epoch the energy density (1) is the order of potential, i.e. and dominates over the imperfect fluid energy density, i.e. . Using slow-roll approximation when, and 3 () the dynamic equations (2) and (3) are reduced to

 3H2=V         , (5) 3H(1+r)˙ϕ=−V′V,

where . From above equations and Eq.(4), when the decay of the tachyon field to imperfect fluid is quasi-stable, i.e. and , may be written as

 ρ=1γ(rV˙ϕ2−Π)=1γ(r3(1+r)2(V′V)2−Π). (6)

In the present work, we will restrict our analysis in high dissipative regime, i.e. where the dissipation coefficient is much greater than v-2 (). Dissipation parameter may be a constant parameter or a positive function of inflaton by the second law of thermodynamics. There are some specific forms for the dissipative coefficient, with the most common which are found in the literatures being the form mm-1 (),2nn (),3nn (),4nn (). In some works and potential of the inflaton have the same forms 1-m (); v-2 (). In Ref.2-ne (), perturbation parameters for warm inflationary model with viscous pressure have been obtained where and . In this work we will study the warm-tachyon inflationary universe model with viscous pressure in this two cases.
The slow-roll parameters of the model are presented by

 ϵ=−˙HH2≃12(1+r)V(V′V)2, (7) η=−¨HH˙H≃1(1+r)V(V′′V−12(V′V)2).

From Eqs.(6) and (7) we find

 ρ=1γ(23r1+rϵρϕ−Π). (8)

The condition of slow-roll is , therefore from above equation, warm-tachyon inflation with viscous pressure could take place when

 ρϕ>3(1+r)2r[γρ+Π]. (9)

Inflation period ends when, which implies

 ρϕ≃3(1+r)2r[γρ+Π],[V′fVf]21Vf≃2(1+rf),

where the subscript denotes the end of inflation. The number of e-folds is given by

 N=∫ϕfϕ∗Hdt=∫ϕfϕ∗H˙ϕdϕ=−∫ϕfϕ∗V2V′(1+r)dϕ. (10)

where the subscript denotes the epoch when the cosmological scale exits the horizon.

We will study inhomogeneous perturbations of the FRW background by using the linear perturbation equation of warm inflation scenario landa (). These scalar perturbations in the longitudinal gauge, may be described by the perturbed FRW metric

 ds2=(1+2Φ)dt2−a2(t)(1−2Ψ)δijdxidxj, (11)

where and are gauge-invariant metric perturbation variables 7-f (). All perturbed quantities have a spatial sector of the form , where is the wave number. Following Ref.landa (), we introduce the stress-energy tensor as

 Tab=(ρ+P)nanb+Pgab+naqb+nbqb+Πab (12)

where the trace-free tensor and are orthogonal to the unit vector ( is the unit normal to the constant-time surface landa ()). For the linear perturbation theory and are replaced by and respectively. We also define the perturbation parameters

 qi=(ρ+P)∇iδV          δΠij=∇i∇jδΠ−13gij∇2δΠ (13)

So, the perturbed Einstein field equation equation of motion in momentum space have these forms

 Φ=Ψ,
 ˙Φ+HΦ=12[−(γρ+Π)avk+V˙ϕ√1−˙ϕ2δϕ], (14)
 ¨δϕ1−˙ϕ2+[3H+ΓV]˙δϕ+[k2a2+(lnV)′′+˙ϕ(ΓV)′]δϕ (15) −[11−˙ϕ2+3]˙ϕ˙Φ−[˙ϕΓV−2(lnV)′]Φ=0,

The fluid equations obtain from the stress-energy tensor landa ().

 (˙δρ)+3γHδρ+ka(γρ+Π)v+3(γρ+Π)˙Φ (16) −˙ϕ2Γ′δϕ−Γ˙ϕ[2(˙δϕ)+˙ϕΦ]=0,
 ˙v+4Hv+ka[Φ+δPρ+P+Γ˙ϕρ+Pδϕ]=0. (17)

where

 δP=(γ−1)δρ+δΠ,       δΠ=Π[ζ,ρζδρ+Φ+˙ΦH].

The above equations are obtained for Fourier components , where the subscript is omitted. in the above set of equations is given by the decomposition of the velocity field () 6-f (). Warm inflation model may be considered as a hybrid-like inflationary model where the inflaton field interacts with imperfect fluid 9-f (), 8-f (). Entropy perturbation may be related to dissipation term 10-f (). In slow-roll approximation the set of perturbed equations are reduced to v-2 ()

 Φ≃12H[−4(γρ+Π)avk+V˙ϕδϕ], (18)
 [3H+ΓV]˙δϕ+[(lnV)′′+˙ϕ(ΓV)′]δϕ≃[˙ϕΓV−2(lnV)′]Φ, (19)
 δρ≃˙ϕ23γH[Γ′δϕ+ΓΦ], (20)

and

 v≃−k4aH(Φ+(γ−1)δρ+δΠγρ+Π+Γ˙ϕγρ+Πδϕ). (21)

Using Eqs.(18), (20) and (21), perturbation variable is determined

 Φ≃˙ϕV2HδϕG(ϕ)[1+Γ4HV+([γ−1]+Πζ,ρζ)˙ϕΓ′12γH2V], (22)

where

 G(ϕ)=1−18H2[2γρ+3Π+γρ+Πγ(Πζ,ρζ−1)].

In Eq.(22), for and case, we may obtain the perturbation variable of warm tachyon inflation model without viscous pressure effect 1-m () (In this case, we find because of the inequality .). Using Eq.(5), we find

 (3H+ΓV)ddt=(3H+ΓV)˙ϕddϕ=−V′Vddϕ. (23)

From above equation, Eq.(19) and Eq.(22), the expression is obtained

 (δϕ)′δϕ=1(lnV)′[(lnV)′′+˙ϕ(ΓV)′+(2(lnV)′−˙ϕΓV)(V˙ϕ2GH) (24) ×(1+Γ4HV+[(γ−1)+Πζ,ρζ]˙ϕΓ′12γH2V)].

We will return to the above relation soon. Following Refs.1-m (), 6-f (), v-2 () and 10-f (), we introduce auxiliary function as

 χ=δϕ(lnV)′exp[∫13H+ΓV(ΓV)′dϕ]. (25)

From above definition we have

 χ′χ=(δϕ)′δϕ−(lnV)′′(lnV)′+(ΓV)′3H+ΓV. (26)

Using above equation, Eqs.(24) (5) and (5)

 χ′χ=−98G2H+ΓV(3H+ΓV)2[Γ+4HV−([γ−1]+Πζ,ρζ)Γ′(lnV)′3γH(3H+ΓV)](lnV)′V. (27)

A solution for the above equation is

 χ(ϕ)=Cexp(−∫{−98G2H+ΓV(3H+ΓV)2 (28) ×[Γ+4HV−([γ−1]+Πζ,ρζ)Γ′(lnV)′3γH(3H+ΓV)](lnV)′V}dϕ),

where is integration constant. From above equation and Eq.(26) we find small change of variable

 δϕ=C(lnV)′exp(I(ϕ)), (29)

where

 I(ϕ)=−∫[(ΓV)′3H+ΓV+98G2H+ΓV(3H+ΓV)2 (30) ×[Γ+4HV−([γ−1]+Πζ,ρζ)Γ′(lnV)′3γH(3H+ΓV)](lnV)′V]dϕ

Finally the density perturbation is given by 12-f ()

 δH=16π5exp(−I(ϕ))(lnV)′δϕ=16π15exp(−I(ϕ))Hr˙ϕδϕ. (31)

By inserting and , the above equation reduces to which agrees with the density perturbation in cool inflation model 1-i (). In warm inflation model the fluctuations of the scalar field in high dissipative regime () may be generated by thermal fluctuation instead of quantum fluctuations 5 () as

 (δϕ)2≃kFTr2π2, (32)

where in this limit freeze-out wave number corresponds to the freeze-out scale at the point when, dissipation damps out to thermally excited fluctuations () 5 (). With the help of the above equation and Eq.(31) in high dissipative regime () we find

 δ2H=64225√3exp(−2I(ϕ))r12~ϵTrH, (33)

where

 ~I(ϕ)=−∫[13Hr(ΓV)′+98G(1−[(γ−1)+Πζ,ρζ](lnΓ)′(lnV)′9γrH2)(lnV)′]dϕ, (34)

and

 ~ϵ=12rV′2V3. (35)

An important perturbation parameter is scalar index which in high dissipative regime is given by

 ns=1+dlnδ2Hdlnk≈1−52~ϵ−32~η+~ϵ(2VV′)(r′4r−2~I(ϕ)′), (36)

where

 ~η=1rV[V′′V−12(V′V)2]. (37)

In Eq.(36) we have used a relation between small change of the number of e-folds and interval in wave number (). The Planck measurement constraints the spectral index as planck ():

 ns=0.96±0.0073 (38)

Running of the scalar spectral index may be found as

 αs=dnsdlnk=−dnsdN=−dϕdNdnsdϕ=1rV(V′V)n′s. (39)

This parameter is one of the interesting cosmological perturbation parameters which is approximately , by using Planck observational results planck ().
During inflation epoch, there are two independent components of gravitational waves () with action of massless scalar field are produced by the generation of tensor perturbations. The amplitude of tensor perturbation is given by

 A2g=2(H2π)2coth[k2T]=V26π2coth[k2T], (40)

where, the temperature in extra factor denotes, the temperature of the thermal background of gravitational wave 7 (). Spectral index may be found as

 ng=ddlnk(ln[A2gcoth(k2T)])≃−2~ϵ, (41)

where 7 (). Using Eqs.(33) and (40) we write the tensor-scalar ratio in high dissipative regime

 R(k)=A2gPR|k=k0=54√35r12~ϵH3Trexp(2I(ϕ))coth[k2T]|k=k0, (42)

where is referred to pivot point 7 () and . An upper bound for this parameter is obtained by using Planck data, 6 (). Non-Gaussianity of the warm-tachyon inflation model is presented in Ref.1-m () as

 fNL=−53˙ϕH[1Hln(kFH)(V′′′+2k2FV′Γ)]. (43)

In high dissipative regime (), parameter has the following form

 fNL=59(V′V)2(lnrr). (44)

In the above equation, we have used Eq.(5) and definition .

We note that, the factor (30) which is found in perturbation parameters (33), (36), (39) and (42) in high energy limit (), for tachyonic warm-viscous inflation model has an important difference with the same factor which was obtained for non-viscous tachyonic warm inflation model 1-m ()

 I(ϕ)=−∫[(ΓV)′3H+ΓV+98G2H+ΓV(3H+ΓV)2 ×[Γ+4HV−Γ′(lnV)′36H(3H+ΓV)](lnV)′V]dϕ.

The bulk viscous pressure effect leads to this difference. Therefore, the perturbation parameters , , and which may be found by WMAP and Planck observational data, for our model with viscous pressure, are modified due to the effect of this additional pressure.

## Iii Exponential potential

In this section we consider our model with the tachyonic effective potential

 V(ϕ)=V0exp(−αϕ), (45)

where parameter (with unit ) is related to mass of the tachyon field 8 (). The exponential form of potential have characteristics of tachyon field ( and ). We develop our model in high dissipative regime, i.e. for two cases: 1- and are constant parameters, 2- as a function of tachyon field and as a function of energy density of imperfect fluid.

### iii.1 Γ=Γ0, ζ=ζ0 case

From Eq.(35), the slow-roll parameter in the present case has the form

 ~ϵ=√32α2√V0Γ0exp(−αϕ2). (46)

Dissipation parameter in this case is given by

 r=Γ0√3V320exp(32αϕ)≫1. (47)

We find the evolution of tachyon field with the help of Eq.(5)

 ϕ(t)=1αln[α2V0Γ0t+eαϕi], (48)

where . Hubble parameter for our model has the form

 H=√V03exp(−αϕ2). (49)

At the end of inflation () the tachyon field becomes

 ϕf=2αln[√3V0α22Γ0], (50)

so, by using the above equation and Eq.(48) we may find time at which inflation ends

 tf=34α2Γ0−Γ0α2V0eαϕi. (51)

Using Eqs.(8) and (46), the energy density of the radiation-matter fluid in high dissipative limit becomes

 ρ=√V03γ2exp(−αϕ2)[α2Γ0V0exp(−αϕ)+3ζ0], (52)

and, in terms of tachyon field energy density becomes

 ρ=ρ12ϕ√3γ(α2Γ0ρϕ+3ζ0). (53)

For this example, the entropy density in terms of energy density of inflaton may be obtained from above equation

 Ts=ρ12ϕ√3γ(α2Γ0ρϕ+3ζ0). (54)

In FIG.1, we plot the entropy density in terms of inflaton energy density. It may be seen that the entropy density increases by the bulk viscous effect mm-1 ().

From Eq.(10), the number of e-fold at the end of inflation, by using the potential (45), for our inflation model is given by

 Ntotal=2Γ0α2√3V0[exp(αϕf2)−exp(αϕi2)]. (55)

where . Using Eqs.(33) and (42), we could find the scalar spectrum and scalar-tensor ratio

 δ2H=128√Γ02254√3α2[V2(ϕ0)(√V(ϕ0)+A)92]Tr4√V(ϕ0), (56)

where and

 R=94√35√Γ0(√V(ϕ0)+A)92V2(ϕ0)V(ϕ0)54Trcoth[k2T], (57)

respectively, where the subscript zero denotes the time, when the perturbation was leaving the horizon. In the above equation we have used the Eq.(34) where

 ~I(ϕ)=ln([√V(ϕ0)+A]94V(ϕ0)). (58)

These parameters may by restricted by WMAP9 and Planck data 6 (); planck (). Based on these data, an upper bound for may be found

 V(ϕ0)<2.28×10−4.

In the above equation we have used these data: , 6 (); planck (). From Eqs.(44) and (47), non-Gaussianity for our model is presented as

 fNL=5√39α2V320Γ0ln(Γ0√3V320)+32αϕ(tF)exp(32αϕ(tF)), (59)

where the freeze-out time is the time when the last three wave-vectors thermalize 1-m ().

### iii.2 Γ=Γ(ϕ), ζ=ζ(ρ) case

Now we assume and , where and are positive constants. By using exponential potential (45), Hubble parameter, parameter and slow-roll parameter have these forms

 H(ϕ)=√V03exp(−αϕ2),            r=α1√3V0exp(αϕ2), (60) ~ϵ=√3V0α22α1exp(αϕ2),

respectively. Using Eq.(5), we find the scalar field in term of cosmic time

 ϕ(t)=−αα1t+ϕi. (61)

The energy density of imperfect fluid in terms of the inflaton energy density is given by the expression

 ρ=α2α1ρ12ϕ√3(γ−√3ξ1ρ12ϕ)−1. (62)

We can find the entropy density in terms of energy density

 Ts=α2α1ρ12ϕ√3(γ−√3ξ1ρ12ϕ)−1. (63)

The entropy density and matter-radiation energy density of our model in this case increase by the bulk viscosity effect (see FIG.2).

From Eq.(61) the scalar field and effective potential at the end of inflation where , becomes

 ϕf=1αln[V03(2α1α2)2],       Vf=34α4α21. (64)

By using the above equation and Eq.(61) we may find time at which inflation ends

 tf=34α2Γ0−Γ0α2V0eαϕi. (65)

Number of e-folds in this case is related to and by using Eq.(10)

 Vi=(2N−1)2Vf. (66)

At the begining of the inflation parameter is given by

 r=ri=23α21(2N−1)α2. (67)

High dissipative condition(), leads to which is agree with the warm-tachyon inflation model without viscous pressure 1-m (). From Eqs.(44) and (60), the non-Gaussianity for our model in this case (, ) is given by

 fNL=5√39α2√V0α1ln(α√3V0)+αϕ2exp(αϕ2). (68)

By using Eqs.(33) and (42) scalar power spectrum and tensor-scalar ratio result to be

 δ2H=128√α12254√3α2[√V(ϕ0)+B]−92(1+ζ1α2γα1) (69) ×exp(98[γ−1]α2√3γα1V(ϕ0)12)4√V(ϕ0)Tr,

and

 R=94√3α25√α1[√V(ϕ0)+B]92(1+ζ1α2γα1) (70) ×exp(−98[γ−1]α2√3γα1V(ϕ0)12)V(ϕ0)34Tr,

respectively, where . In the above equations we have used the Eq.(34) where

 ~I(ϕ0)=916(1−γ)(α2√3γα1)V−12(ϕ0)+94[1+ζ1α2γα1]ln(V12(ϕ0)+B). (71)

These parameters may be restricted, using WMAP9, Planck and BICEP2 data 6 (); planck (); BICEP2 (). Using WMAP9 (BICEP2) data, , () and the characteristic of warm inflation, 3 (), we may restrict the values of temperature (), using Eqs.(33), (42), or the corresponding equations (56), (57), (69), (70), in our coupled examples, (see FIG.3). We have chosen and . Using BICEP2 data, we have found the new minimum of (See for example end ()).

## Iv Conclusion

Warm-tachyon inflation model with viscous pressure, using overlasting form of potential which agrees with the tachyon potential properties, has been studied. The main problem of the inflation theory is how to attach the universe to the end of the inflation period. One of the solutions of this problem is the study of inflationary epoch in the context of warm inflation scenario 3 (). In this model radiation is produced during inflation period where its energy density is kept nearly constant. This is phenomenologically fulfilled by introducing the dissipation term . Warm inflation model with viscous pressure is an extension of warm inflation model where instead of radiation field we have radiation-matter fluid. The study of warm inflation model with viscous pressure as a mechanism that gives an end for tachyon inflation are motivated us to consider the warm tachyon inflation model with viscous pressure. In the slow-roll approximation the general relation between energy density of radiation-matter fluid and energy density of tachyon field is found. In longitudinal gauge and slow-roll limit the explicit expressions for the tensor-scalar ratio scalar spectrum index, and its running have been obtained. We have developed our specific model by exponential potential for two cases: 1- Constant dissipation coefficient and constant bulk viscous pressure coefficient . 2- as a function of tachyon field and as a function of imperfect fluid energy density . In these two cases we have found perturbation parameters and constrained these parameters by WMAP9 and Planck data.

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