Research Article  Open Access
On SU(3) Effective Models and Chiral Phase Transition
Abstract
Sensitivity of Polyakov NambuJonaLasinio (PNJL) model and Polyakov linear sigmamodel (PLSM) has been utilized in studying QCD phasediagram. From quasiparticle model (QPM) a gluonic sector is integrated into LSM. The hadron resonance gas (HRG) model is used in calculating the thermal and dense dependence of quarkantiquark condensate. We review these four models with respect to their descriptions for the chiral phase transition. We analyze the chiral order parameter, normalized netstrange condensate, and chiral phasediagram and compare the results with recent lattice calculations. We find that PLSM chiral boundary is located in upper band of the lattice QCD calculations and agree well with the freezeout results deduced from various highenergy experiments and thermal models. Also, we find that the chiral temperature calculated from HRG is larger than that from PLSM. This is also larger than the freezeout temperatures calculated in lattice QCD and deduced from experiments and thermal models. The corresponding temperature and chemical potential are very similar to that of PLSM. Although the results from PNJL and QLSM keep the same behavior, their chiral temperature is higher than that of PLSM and HRG. This might be interpreted due the very heavy quark masses implemented in both models.
1. Introduction
At large momentum scale, quantum chromodynamics (QCD) predicts asymptotic freedom [1, 2] or a remarkable weakening in the running strong coupling. Accordingly, phase transition takes place from hadrons in which quarks and gluons are conjectured to remain confined (at low temperature and density) to quarkgluon plasma (QGP) [3, 4], in which quarks and gluons become deconfined (at high temperature and density) [5]. Furthermore, at low temperature, the QCD chiral symmetry is spontaneously broken; . In this limit, the chiral condensate remains finite below the critical temperature (). The broken chiral symmetry is restored at high temperatures. The finite quark masses explicitly break QCD chiral symmetry.
NambuJonaLasinio (NJL) model [6] describes well the hadronic degrees of freedom. Polyakov NambuJonaLasinio (PNJL) model [7–9] takes into consideration the quark dynamics [10] and has been utilized to study the QCD phasediagram [11, 12]. Also, linear model (LSM) [13] can be used in mapping out the QCD phasediagram.
Many studies have been performed on LSM like LSM [13] at vanishing temperature, LSM at finite temperature [14, 15], and LSM for , and quark flavors [16–19]. In order to obtain reliable results, extended LSM to PLSM can be utilized, in which information about the confining glue sector of the theory is included in form of Polyakov loop potential. The latter can be extracted from pure YangMills lattice simulations [20–23]. Also, the Polyakov linear sigmamodel (PLSM) and Polyakov quark meson model (PQM) [24–26] deliver reliable results. Furthermore, the quasiparticle model (QPM) [27, 28] was suggested to reproduce the lattice QCD calculations [29, 30], in which two types of actions are implemented; the lattice QCD simulations utilizing the standard Wilson action and the ones with renormalization improved action.
In the present work, we integrate the gluonic sector of QPM into LSM [31] (QLSM) in order to reproduce the recent lattice QCD calculations [32]. In QLSM [31], the Polyakov contributions to the gluonic interactions and to the confinementdeconfinement phase transition are entirely excluded. Instead we just add the gluonic part of QPM. Therefore, the quark masses should be very heavy. We will comment on this, later on. In Section 3, we outline the QLSM results. They are similar to that of PNJL. This might be interpreted due the very heavy quark masses implemented in both models. Similar approach has been introduced in [33]. The authors described inclusion of gluonic Polyakov loop, which is assumed to generate a large gauge invariance and lead to a remarkable modification in hadron thermodynamics. A quite remarkable bridging between PNJL model quantum and local Polyakov loop and HRG model has been introduced [34]. A large suppression of the thermal effects has been reported and it was concluded that the center symmetry breaking becomes exponentially small with increasing the masses of constituent quarks. In other words, the chiral symmetry restoration becomes exponentially small with increasing the pion mass.
The hadron resonance gas (HRG) model gives a good description for the thermal and dense evolution of various thermodynamic quantities in the hadronic matter [35–43]. Also, it has been successfully utilized to characterize the conditions deriving the chemical freezeout at finite densities [44]. In light of this, the HRG model can be well used in calculating the thermal and dense dependence of quarkantiquark condensate [45]. The HRG grand canonical ensemble includes two important features [38]: the kinetic energies and the summation over all degrees of freedom and energies of the resonances. On the other hand, it is known that the formation of resonances can only be achieved through strong interactions [46]; resonances (fireballs) are composed of further resonances (fireballs), which in turn consist of resonances (fireballs) and so on. In other words, the contributions of the hadron resonances to the partition function are the same as that of free (noninteracting) particles with an effective mass. At temperatures comparable to the resonance halfwidth, the effective mass approaches the physical one [38]. Thus, at high temperatures, the strong interactions are conjectured to be taken into consideration through the inclusion of heavy resonances. It is found that the hadron resonances with masses up to 2 GeV are representing suitable constituents for the partition function [35–43]. In such a way, the singularity expected at the Hagedorn temperature [35, 36] can be avoided and the strong interactions are assumed to be taken into consideration. Nevertheless, validity of the HRG model is limited to the temperatures below the critical one, .
In the present paper, we review PLSM, QLSM, PNJL, and HRG with respect to their descriptions for the chiral phase transition. We analyse the chiral orderparameter , the normalized netstrange condensate , and the chiral phasediagram and compare the results with the lattice QCD [47–49]. The present work is organized as follows. In Section 2, we introduce the different approaches PLSM [50] (Section 2.1), QLSM (Section 2.2), PNJL (Section 2.3), and HRG (Section 2.4). The corresponding mean field approximations are also outlined. Section 3 is devoted to the results. The conclusions and outlook will be given in Section 4.
2. SU(3) Effective Models
2.1. Polyakov Linear SigmaModel (PLSM)
As discussed in [31, 50], the Lagrangian of LSM with quark flavors and (for quarks, only) color degrees and with quarks coupled to Polyakov loop dynamics was introduced in [26, 51]where the chiral part of the Lagrangian of the symmetric linear sigmamodel Lagrangian with is [52, 53] . The first term is fermionic part (2) with a flavorblind Yukawa coupling of the quarks. The second term is mesonic contribution (3):The summation runs over the three flavors ( for the three quarks , and ). The flavorblind Yukawa coupling should couple the quarks to the mesons. The coupling of the quarks to the Euclidean gauge field is given via the covariant derivative [20, 21]. In (3), is a complex matrix which depends on the and [53], where are Dirac matrices, are the scalar mesons, and are the pseudoscalar mesons:where with are the nine generators of the symmetry group and are the eight GellMann matrices [13]. The chiral symmetry is explicitly broken throughwhich is a matrix with nine parameters . Three finite condensates , , and are possible, because the finite values of vacuum expectation of and are conjectured to carry the vacuum quantum numbers and the diagonal components of the explicit symmetry breaking term, , where , and , and squared tree level mass of the mesonic fields , two possible coupling constants and , Yukawa coupling , and a cubic coupling constant can be estimated as follows: MeV, , and and .
In order to get a good analysis it is more convenient to convert the condensates and into a pure nonstrange and strange condensates [54]:
The second term in (1), , represents Polyakov loop effective potential [20], which agrees well with the nonperturbative lattice QCD simulations and should have center symmetry as pure gauge QCD Lagrangian does [8, 24]. In the present work, we use the potential as a polynomial expansion in and [8, 9, 55, 56]:where
In order to reproduce pure gauge lattice QCD thermodynamics and the behavior of the Polyakov loop as a function of temperature, we use the parameters , , and . For a much better agreement with the lattice QCD results, the deconfinement temperature in pure gauge sector is fixed at MeV.
2.1.1. Polyakov Linear SigmaModel (PLSM) in Mean Field Approximation
In thermal equilibrium the grand partition function can be defined by using a path integral over the quark, antiquark, and meson fields:where and is the volume of the system. is the chemical potential for . We consider symmetric quark matter and define a uniform blind chemical potential . Then, we evaluate the partition function in the mean field approximation [53, 57]. We can use standard methods [58] in order to calculate the integration. This gives the effective potential for the mesons.
We define the thermodynamic potential density of PLSM asAssuming degenerate light quarks, that is, , the quarks and antiquarks contribution potential is given as [51]where , and the valence quark and antiquark energy for light and strange quark are as follows: and , respectively. Also, as per [54] the light quark sector (13) decouples from the strange quark sector () and light quark mass gets simplified in this new basis to
The purely mesonic potential is given asWe notice that the sum in (7), (11), and (14) gives the thermodynamic potential density similar to (10), which has seven parameters , and , two unknown condensates and , and two order parameters for the deconfinement and . The six parameters , and are fixed in the vacuum by six experimentally known quantities [53]. In order to evaluate the unknown parameters , and , we minimize the thermodynamic potential (10) with respect to , and , respectively. Doing this, we obtain a set of four equations of motion:where min means , and are the global minimum:Accordingly, the chiral order parameter can be deduced as
2.2. Linear SigmaModel and QuasiParticle Sector (QLSM)
When the Polyakov contributions to the gluonic interactions and to the confinementdeconfinement phase transition are entirely excluded, the Lagrangian of LSM with quark flavors and (for quarks, only) color degrees of freedom, where the quarks couple to the Polyakov loop dynamics, has been introduced in [26, 51]The main original proposal of the present work is the modification of (18):where the chiral part of the Lagrangian is of symmetry [52, 53]. Instead of , the gluonic potential , which is similar to the gluonic sector of the quasiparticle model, is inserted (review (33)). The Lagrangian with consists of two parts: fermionic and mesonic contributions (2) and (3), respectively.
Some details about the quasiparticle model are in order. The model gives a good phenomenological description for lattice QCD simulation and treats the interacting massless quarks and gluons as noninteracting massive quasiparticles [59]. The corresponding degrees of freedom are treated in a similar way as the electrons in condensed matter theory [60]; that is, the interaction with the medium provides the quasiparticles with dynamical masses. Consequently, most of the interactions can be taken into account. When confronting it to the lattice QCD calculations, the free parameters can be fixed. The pressure at finite and is given as where the function stands for bag pressure at finite and which can be determined by thermodynamic selfconsistency and ; the stability of with respect to the selfenergies () and the distribution function for bosons and fermions, , respectively, is given as The quasiparticle dispersion relation can be approximated by the asymptotic mass shell expression near the light cone [27, 28]: where is the selfenergy at finite and and is a factor taking into account the mass scaling as used in the lattice QCD simulations. In other words, was useful when the lattice QCD simulations have been performed with quark masses heavier than the physical ones. In the present work, the gluon selfenergies are relevant [61]: where the effective coupling at vanishing chemical potential is given as And the twoloop effective coupling reads [27] and is a regulator at . The parameter is used to adjust the scale as found in lattice QCD simulations. These two parameters are not very crucial in the present calculations. The regulator and scale are controlled by the condensates ( and ) and the order parameters ( and ), which are given as function of temperature and baryon chemical potential. The function [62] depends on the QCD coupling , , with being the energy scale. It is obvious that the QCD coupling in (24) and (25) is given in dependence, only. In calculating at finite it is apparently needed to extend to be dependent, as well. The twoloop perturbation estimation for functions gives
2.2.1. Linear SigmaModel and QuasiParticle Sector (QLSM) in Mean Field Approximation
As in Section 2.1.1 and (9), we derive the thermodynamic potential density in the mean field approximation. This consists of three parts: mesonic and quasigluonic potentials in additional to the quark potential:(i)First, the quark potential part [53] isIt is obvious that is equivalent to . The occupation quark/antiquark numbers readand antiquarks , respectively. The number of internal quark degrees of freedom is denoted by and (for quarks and antiquarks). The energies are given aswith the quark masses which is related to and for , and , and quarks, respectively. As given, the latter are proportional to the fields:where the Yukawa coupling . The symbols for the chiral condensates, and for light and strangequarks, respectively, are kept as in the literature.(ii)Second, the purely mesonic potential part reads(iii)Third, the quasigluonic potential part is constructed from (22), (21), and (20): In (33), the degeneracy factor and two parameters and , which were given in (25), should be fixed in order to reproduce the lattice QCD calculations. Here, we find that and MeV give excellent results.
When adding the three potentials given in (33), (32), and (28), the thermodynamics and chiral phase translation can be analysed. The resulting potential can be used to determine the normalized netstrange condensate and chiral order parameter (51):where is function of and the quark masses should be very heavy. The QLSM results are similar to that of PNJL, Section 3. This might be interpreted due the very heavy quark masses implemented in both models.
2.3. Polyakov NambuJonaLasinio (PNJL) Model
The Lagrangian of PNJL reads [63, 64]where the matrices are chiral projectors, is the Polyakov loop potential (LandauGinzburg type potential), and stand for gauge field interactions. The mass of a particular flavor is denoted by , where . The two coupling constants and , , are GellMann matrices [13] and are Dirac matrices. The model is not renormalizable so that we have to use threemomentum cutoff regulator in order to keep quark loops finite.
The Polyakov loop potential is given by [65]with and being constants, and we choose the following fitting values for the potential parameters: , and MeV. These are adjusted to the pure gauge lattice data such that the equation of state and the Polyakov loop expectation values are reproduced.
2.3.1. Polyakov NambuJonaLasinio (PNJL) Model in Mean Field Approximation
The thermodynamic potential density of PNJL is defined aswhere is the single quasiparticle energy, , and from isospin symmetry, . In the above integrals, the vacuum integral has a cutoff whereas the medium dependent integrals have been extended to infinity. By the selfconsistent gap equation, the quark mass can be estimated:where denotes the chiral condensate of quark with flavor and other parameters are listed out in Table 1 [63, 64]. For isospin symmetry, we define the light and strangequark masses asHere, we notice the strong dependence on the fields.

Now, we have all the PNJL model parameters except , and , which can be estimated from minimizing the thermodynamic potential (43) with respect to , and , respectively. Doing this, we obtain a set of four equations of motion:Then, the potential of the PNJL model reads Having completed the introduction of both PLSM and PNJL, it is in order now to discuss central symmetry related to the Polyakov loop. It has been shown that the colorsinglet has symmetry through the normalized character in the fundamental representation of , . This becomes equivalent to an ensemble of Polyakov loop [66]. Furthermore, it was concluded that can be taken as an order parameter for colorconfinement to colordeconfinement phase transition; that is, the center symmetry is spontaneously broken at high temperatures.
Reference [67] introduced an attempt to resolve some incongruities within NJL and PNJL. It was argued that by integrating corresponding extremum conditions, the thermodynamic potential is directly obtained, where the integration constant can be fixed from StefanBoltzmann law. Keeping the regulator finite at finite temperature and chemical potential is the main advantage of this approach.
2.4. Hadron Resonance Gas (HRG) Model
Treating hadron resonances as a free (noninteracting) gas [35–39] is conjectured to give an accurate estimation for the thermodynamic pressure below . It has been shown that thermodynamics of strongly interacting system can also be approximated as an ideal gas composed of hadron resonances with masses ≤2 GeV [38, 68]; that is, confined QCD matter (hadrons) is well modelled as a noninteracting gas of resonances. The grand canonical partition function readswhere is temperature (chemical potential). The Hamiltonian () is given as the kinetic energies of the relativistic Fermi and Bose particles.
The main motivation of using is that(i)it contains all relevant degrees of freedom of confined, strongly interacting QCD matter,(ii)it implicitly includes interactions, especially the ones leading to formation of resonances,(iii)it gives a quite satisfactory description of the particle production in heavyion collisions.
With these assumptions, the thermodynamics resulted from singleparticle partition functions where is the th particle dispersion relation, is spinisospin degeneracy factor, and stands for bosons and fermions, respectively.
For hadron resonances which are not yet measured, experimentally, a parametrization for a total spectral weight has been proposed [69] as a recent estimation for Hagedorn mass spectrum [70, 71]. In the present work, we merely include known (measured) hadron resonances with mass ≤2 GeV. This mass cutoff is assumed to define the validity of HRG in modelling the hadronic phase. Resonances with heavier masses diverge all thermodynamic quantities at the Hagedorn temperature [35, 36].
Very recently, it has been shown that indeed the viral expansion is a reliable way to include hadron resonances, because the phase shift is a directly accessible quantity in experiments [72]. For instance, for accurate isospinaveraged observables, the scalarisoscalar ( meson) resonance and scalar should not be included in the HRG model.
The HRG model has been used in calculating the higherorder moments of the particle multiplicity, in which a grand canonical partition function of an ideal gas with experimentally observed states up to a certain mass cutoff is utilized [44]. The HRG model has been successfully utilized in characterizing two different conditions generating the chemical freezeout at finite densities, namely, constant normalizedentropy density [73–76], constant product of kurtosis and variance [77], and constant traceanomaly [78]. As introduced in [76], the third freezeout conditions, which is characterized by constant is accompanied by constant .
Our HRG model was used to study the possible differences between the behavior of light and strange quarkantiquark condensates in hadron phase. The contribution to the pressure due to a particle of mass , baryon charge , isospin , strangeness , and degeneracy is given bywhere is the modified Bessel function. In hadrons, the isospin is an almost exact symmetry.
The quarkantiquark condensates are given by the derivative of (46) with respect to the constituent quark masses:where and are light and strange quarkantiquark condensates in vacuum, respectively [45]. It was found that at small chemical potential the strange quarkantiquark condensate is larger than the light one. At large chemical potential, such difference gradually diminishes.
Some authors still prefer to take into account repulsive (electromagnetic) van der Waals interactions in order to compensate the strong interactions in hadron matter [78]. Accordingly, each resonance constituent is allowed to have an eigenvolume. Thus, such total volume should be subtracted from the fireball volume or that of the heat bath. Also, considerable modifications in thermodynamics of hadron gas including energy, entropy, and number densities are likely. The hardcore radius of hadron nuclei can be related to the multiplicity fluctuations.
About ten years ago, Tawfik derived matrix for the HRG model [38], which describes the scattering processes in the thermodynamical system [79]. Accordingly, (45) can be written as an expansion of the fugacity term:where are the virial coefficients and the subscript refers to the order of multipleparticle interactions:The sum runs over the spatial waves. The phase shift of twobody inelastic interactions, for instance, depends on the resonance halfwidth and spin and mass of produced resonances:In (50), by replacing by , the antiparticles are taken into consideration. For a narrow width and/or being at low temperature, the virial term decreases so that the nonrelativistic ideal partition function of hadron resonances with effective masses is obtained. This means that the resonance contributions to the partition function are the same as that of massive free resonances. At temperatures comparable to , the effective mass approaches the physical one. Thus, we conclude that, at high temperatures, the strong interactions are taken into consideration via heavy resonances (45), that is, Hagedorn picture. We therefore utilise the grand canonical partition function (48) without any corrections.
In order to verify this picture, Tawfik checked the ability of HRG with finitevolume constituents in reproducing lattice QCD thermodynamics [78]. At radius fm, the disagreement becomes obvious and increases with increasing . At high temperatures, the resulting thermodynamics becomes nonphysical. It was concluded that the excluded volume seems to be practically irrelevant. It has a negligible effect, at fm. On the other hand, a remarkable deviation from the lattice QCD calculations appears, especially when the radius becomes large.
In the present work, the chiral parameters, and , see Section 3, are extracted from HRG assuming fully and partially chemical nonequilibrium [80]. There is no difference when and when it is allowed to have values different from unity, where and refer to nonequilibrium treatment or occupation factors for light and strange quarks, respectively. These two parameters enter (45) after raising them to exponents reflecting the light and strange quarks contents of th hadron. They are identical to the fugacity factor and therefore are multiplied to the exponential function.
3. Results
A systematic comparison between PLSM, PNJL, QLSM, and HRG is presented. It intends to calculate two chiral quantities, the orderparameter , and the normalized net strange and net nonstrange condensate . The results will be confronted to the lattice QCD simulations [47–49]. The comparison with the lattice should signal which model is close to the lattice and, on the other hand, offers differentiation between the effective models themselves.
3.1. Chiral OrderParameter
The chiral orderparameter was originated in lattice techniques [81]. The latter calculates dimensionless quantities in units of lattice spacing rather than physical units. The lattice spacing can then be converted into the physical units. relates the light quark condensate to the strange quark mass:where is the strange quark physical mass which is fixed here to in order to get the ratio of light and strange quark masses . Also, we notice that the dimensionless depends on the thermal behavior of the light quark condensate . In lattice QCD, the chiral condensate remains finite. But it contains contributions which would diverge in the continuum limit. Therefore, it requires renormalization, in particular an additive and multiplicative renormalization. In order to remove, at least, the multiplicative renormalization factor, we take into consideration (51) as a definition for the order parameter. The light quark condensate itself can be calculated from the potential, PLSM (16), QLSM (34), PNJL (43), and HRG (47). Accordingly, we estimate (51) from the four models and then compare them with the lattice QCD calculations, Figure 1. We find that this chiral order parameter in the effective models and firstprinciple lattice QCD simulations [47, 48] rapidly decreases with increasing .
Comparing with the lattice QCD [47], the best agreement is found with PLSM, but PLSM underestimates the recent lattice QCD [48]. In fact, the lattice calculations [48] lay on top of all curves from the effective models. This might be originated to the specific configurations of the lattices and the actions implemented in each simulation, Section 3.1. The other effective models lay below the two sets of lattice calculations.
The four models PLSM, QLSM, PNJL, and HRG and different sets of lattice calculations have different critical temperatures. In Table 2, we list out the critical temperatures corresponding to each order parameter. In determining the pseudocritical temperatures, , different criteria are implemented. They are not only quite unorthodox but also distinguishable from each other. Further details will be elaborated in Section 3.3.
3.1.1. A Short Comparison between the Two Sets of Lattice QCD Calculations
References [47, 48] presented results for quark flavors, where all systematics are controlled, the quark masses are set to their physical values, and the continuum extrapolation is carried out. Larger lattices and a Symanzik improved gauge besides a stoutlink improved staggered fermion action are implemented. Depending on the exact definition of the observables, the remnant of the chiral transition is obtained at MeV. Extending these results, the transition temperature was also determined for small nonvanishing baryonic chemical potentials. At high temperatures, the lattice pressure is found ~30% lower than the StefanBoltzmann limit.
Reference [49] used quark flavors with physical strange quark mass and almost physical light quark masses. The calculations have been performed with two different improved staggered fermion actions, the asqtad and p4 actions. Overall, a good agreement between results obtained with these two improved staggered fermion discretization schemes is found. At high temperatures, the lattice pressure is ~14% lower than the StefanBoltzmann limit.
From this short comparison, we find the following.(i)References [47, 48] implement Symanzik improved gauge and stoutlink improved staggered fermion action. The resulting pressure is found ~30% lower than the StefanBoltzmann limit.(ii)Reference [49] uses improved staggered fermion actions: the asqtad and p4 actions. The resulting pressure is ~14% lower than the StefanBoltzmann limit.
3.1.2. Couplings in PLSM
In the effective models, the parameters, especially the couplings, are very crucial for the outcome of the calculations. One of the motivations for the present work is the failure of PLSM [50] in reproducing the lattice QCD results [47–49] even with large coupling . In [50], ranges between and . The first value was enough to reproduce the lattice QCD calculations, PRD80, 014504 (2009), and PLB730, 99 (2014). Increasing to does not enable PLSM to reproduce the other lattice simulations [47–49]. Furthermore, through fitting with lattice QCD calculations and experiments, the parameters of PLSM can be estimated. This was described in details in [50, 53].
Scope of the present script is the regeneration for the lattice QCD calculations [47–49]. In the present work, we tackle this problem through comparison with various effective models. In doing this, we have modified LSM and present systematic analysis for two order parameters. We have added to LSM the gluonic sector of the quasiparticle model. This is the essential original proposal of the present script. Thus, waiving details about PLSM itself are though as legitimated. But for a complete list of the PLSM parameters, the readers are kindly advised to consult [50, 53].
3.2. Normalized NetStrange Condensate
Another dimensionless quantity shows the difference between nonstrange and strange condensates:where are nonstrange (strange) condensates and () are nonstrange (strange) masses. Using Ward identities and GellMannOakesRenner relation, expression (52) might be given in terms of pion and kaon masses and their decay constants [82]. Accordingly, the final results might be scaled but their thermal behavior remains unchanged. The lattice QCD calculations for (solid circles) [47] and (open circles) [49] are compared with the calculations from PLSM (solid curve), QLSM (dotted curve), PNJL (doubledotted curve), and HRG (dashdoubledotted curve) in Figure 2.
It is obvious that PLSM agrees with the lattice results [49] at low and also at high temperatures. Its ability to reproduce the other set of lattice results [48] is limited to the high temperatures. This might be originated in the difference between the two sets of lattice QCD simulations, Section 3.1.1. The HRG model agrees well with these lattice calculations [48]. It is apparent that such agreement is limited to temperatures below the critical value due to the limited applicability of the HRG model. The remaining two models PNJL and QLSM show qualitative thermal behavior as that from the other effective models and lattice calculations, which can be described by large plateau at low temperatures, around the critical temperature the values of decrease rapidly, and at high temperature vanishes but very slowly. Both models are closer to [49] rather than to [48].
Both Figures 1 and 2 show that the PNJL model and HRG model describe much better the LQCD data for the magnetization and normalized netstrange condensate, respectively, than for the chiral condensate. One should bear in mind that the magnetizations have been simulated in a different lattice than the one for the netstrange condensate. Unfortunately, both quantities are not available from the same lattice simulation.
3.3. QCD Chiral PhaseDiagram
For mapping out the QCD chiral phasediagram, various approaches are available. From PLSM and PNJL, as they possess two order parameters, one for strange and one for nonstrange chiral condensates, hints about QCD chiral phase transition can be analysed. Furthermore, PLSM and PNJL possess deconfinement order parameter because of the Polyakov loop potential. Therefore, from strange and nonstrange chiral condensates, a dimensionless quantity reflecting the difference between both condensates, , can be deduced as function of temperature at fixed baryon chemical potential. Apparently, this signals the QCD chiral phase transition. At the same value of baryon chemical potential, we can also deduce the deconfinement order parameter as function of temperature. At a fixed baryon chemical potential, the thermal dependence of these two quantities intersects with each other at a characterizing point representing the phase transition. When repeating this procedure at different values of the baryon chemical potentials, we get a set of points representing the QCD phasediagram. The results are given in Figure 3, as solid curve for PLSM and dotted curve for PNJL.
For the QCD chiral phasediagram from QLSM, we implement another method. As no Polyakov loop potential is included, the QCD chiral phasediagram is characterized by the higherorder moments of particle multiplicity [31], which are assumed to highlight various types of fluctuations in and . Therefore, we utilize the possible fluctuations accompanying normalized secondorder moment [31] in mapping out the QCD chiral phase transition. The problematic of determining pseudocritical temperature from the second moment has been discussed in [83]. Accordingly, we observe that the peaks corresponding to different temperatures are conjectured to be characterized by different values of the baryon chemical potentials, where the QCD chiral phase transition is conjectured to occur. We analyse this dependence at different values of the temperature . Then, we follow the scheme to determine and , which is characterized by maximum , where is the secondorder moment of the particle multiplicity. The results are illustrated in Figure 3, as dashdotted curve.
For the HRG model, we map out the QCD chiral phasediagram by utilizing the quarkantiquark condensate as order parameter [45]. It is assumed that the thermal dependence of the quarkantiquark condensate remains finite in the hadronic phase but vanishes at temperature higher than the critical chiral temperature. The results are given in Figure 3 as well, as doubledotted curve.
We can now shortly summarize the methods implemented to determine the pseuodcritical temperatures.(i)PLSM and PNJL: due to chiral and deconfinement phase transitions for light and strange quarks, is determined as function of temperature at a fixed baryon chemical potential, . This signals the QCD chiral phase transition. At the same value of , the deconfinement order parameter can be studied as function of temperature, as well. Then, the thermal dependence of these two quantities is conjectured to intersect with each other at a characterizing point. When repeating this procedure for different values of , a set of points of pseudocritical temperatures and can be deduced.(ii)QLSM: the normalized secondorder moment of particle multiplicity is implemented in mapping out the QCD chiral phase transition. Peaks corresponding to different temperatures are conjectured to be characterized by different values of and .(iii)HRG: the quarkantiquark condensates are implemented as order parameters. At vanishing and finite , the thermal dependence of the quarkantiquark condensate remains finite in the hadronic phase and vanishes at temperature higher than the critical chiral temperature, .
We observe that the chiral boundary from PLSM (solid curve) is positioned within the upper band of the lattice QCD calculations [84–86] and agrees well with the freezeout results deduced from the STAR BES measurements (symbols) [87]. The temperatures calculated from the HRG model by using the quarkantiquark condensate as the order parameter (doubledotted curve) [45] are higher than the chiral temperatures from the PLSM and the freezeout temperatures calculated in the lattice QCD (band) and from the STAR BES measurements (symbols). Despite this difference, the corresponding  sets are very similar to that of the PLSM. The results from PNJL and QLSM are higher than that from the HRG model.
4. Conclusions and Outlook
In the present work, we report on a systematic comparison between PLSM, PNJL, QLSM, and HRG in generating the chiral quantities, orderparameter , and normalized netstrange and nonstrange condensates . Furthermore, we confront the results deduced from the four effective models to the recent lattice QCD calculations in order to distinguish between the models and to interpret the firstprinciple lattice QCD calculations.
For the orderparameter , the best agreement is found with PLSM, while the recent lattice QCD [48] lay on top of all curves. This might be understood from the lattice configurations and the actions implemented in the simulations. The other effective models lay below the two sets of the lattice calculations. We notice that the effective PLSM, QLSM, PNJL and HRG and the different sets of the lattice calculations have different critical temperatures, Table 2.
For the normalized netstrange and nonstrange condensates , PLSM again gives an excellent agreement with the lattice results [49] at low and high temperatures. But its ability to reproduce the lattice simulations [48] is limited to high temperatures. This might be originated in the difference between the two sets of lattice QCD simulations. Furthermore, we find that the HRG model agrees well with the lattice QCD calculations [48]. It is apparent that this is restricted to temperatures below the critical value. The effective models PNJL and QLSM show the same qualitative thermal behavior. There is a large plateau at low temperatures. Around the critical temperature the values of decrease rapidly. At high temperature, vanishes but very slowly. The effective models PNJL and QLSM are closer to [49] rather than to [48].
In light of this, we conclude that the PLSM reproduces and as well. The HRG model is able to reproduce , while PNJL and QLSM seem to fail. These features and differences are present in the chiral phasediagram, Figure 3, as well.
In Section 3.3, we have introduced the various order parameters used in the different models in order to deduce and of the QCD chiral phase transition. The strange and nonstrange chiral condensates and the Polyakov loop potentials are utilized in PLSM and PNJL. The thermal dependence of these two quantities are assumed to intersect with each other at a characterizing point representing the QCD chiral phase transition. For QLSM, no Polyakov loop potential is included in, therefore, the chiral phasediagram is characterized by the higherorder moments of the particle multiplicity. The possible fluctuations accompanying the normalized secondorder moment are assumed to map out the QCD chiral phase transition. For the HRG model, we utilize the quarkantiquark condensates as order parameter.
Again, we find that the PLSM chiral boundary (solid curve) is located within the upper band of the lattice QCD calculations and agrees well with the freezeout results deduced from the experiments and the thermal models (symbols). It is obvious that the chiral temperature calculated from the HRG model is larger than that from the PLSM. This is also larger than the freezeout temperatures calculated in the lattice QCD (band) and from the experiments and the thermal models (symbols). Despite this difference, the corresponding and sets are very similar to that from the PLSM. This might be explained as follows. The and are calculated using different order parameters: In HRG vanishing quarkantiquark condensate but in PLSM crossing (equalling) chiral condensates and Polyakov loop potentials can be utilized in determining both chiral and . The latter assumes that the two phase transitions, the chiral and the deconfinement, occur at the same temperature. The earlier deals with the chiral phase transition independent on the confinementdeconfinement one.
The results from the two models PNJL and QLSM show the same qualitative behavior. The chiral temperatures are higher than that from the PLSM and HRG. This might be interpreted due to the heavy quark masses implemented in both models.
Any model comparison with lattice results should span as much as possible of the parameter space. Even with the narrow parameter space explored in the present paper, we would like to highlight that the results are limited. But, with reference to previous work [50], the parameters alone are not able to explain the diversity with the results in this study. We have to attack essential components of LSM and integrate gluonic sector taken from the quasiparticle models.
Conflict of Interests
The authors declare that there is no conflict of interests regarding the publication of this paper.
Acknowledgments
The present work was supported by the World Laboratory for Cosmology And Particle Physics (WLCAPP) http://wlcapp.net/. The authors are very grateful to the anonymous referee for his/her very constructive comments, suggestions, and even criticisms, which helped a lot in improving the paper.
References
 D. J. Gross and F. Wilczek, “Ultraviolet behavior of nonAbelian gauge theories,” Physical Review Letters, vol. 30, no. 26, pp. 1343–1346, 1973. View at: Publisher Site  Google Scholar
 H. D. Politzer, “Reliable perturbative results for strong interactions?” Physical Review Letters, vol. 30, no. 26, article 1346, 1973. View at: Publisher Site  Google Scholar
 N. Cabibbo and G. Parisi, “Exponential hadronic spectrum and quark liberation,” Physics Letters B, vol. 59, no. 1, pp. 67–69, 1975. View at: Publisher Site  Google Scholar
 J. C. Collins and M. J. Perry, “Superdense matter: neutrons or asymptotically free quarks?” Physical Review Letters, vol. 34, no. 21, pp. 1353–1356, 1975. View at: Publisher Site  Google Scholar
 D. H. Rischke, “The quark gluon plasma in equilibrium,” Nuclear Physics, vol. 52, pp. 197–296, 2004. View at: Publisher Site  Google Scholar
 Y. Nambu and G. JonaLasinio, “Dynamical model of elementary particles based on an analogy with superconductivity. I,” Physical Review, vol. 122, no. 1, pp. 345–358, 1961. View at: Publisher Site  Google Scholar
 K. Fukushima, “Chiral effective model with the Polyakov loop,” Physics Letters B, vol. 591, no. 34, pp. 277–284, 2004. View at: Publisher Site  Google Scholar
 C. Ratti, M. A. Thaler, and W. Weise, “Phases of QCD: lattice thermodynamics and a field theoretical model,” Physical Review D, vol. 73, Article ID 014019, 2006. View at: Publisher Site  Google Scholar
 K. Fukushima, “Phase diagrams in the threeflavor NambuJonaLasinio model with the Polyakov loop,” Physical Review D, vol. 77, Article ID 114028, 2008. View at: Publisher Site  Google Scholar
 T. Hatsuda and T. Kunihiro, “QCD phenomenology based on a chiral effective Lagrangian,” Physics Report, vol. 247, no. 56, pp. 221–367, 1994. View at: Publisher Site  Google Scholar
 A. Masayuki and Y. Koichi, “Chiral restoration at finite density and temperature,” Nuclear Physics A, vol. 504, no. 4, pp. 668–684, 1989. View at: Publisher Site  Google Scholar
 H. Fujii, “Scalar density fluctuation at the critical end point in the Nambu–JonaLasinio model,” Physical Review D, vol. 67, no. 9, Article ID 094018, 2003. View at: Publisher Site  Google Scholar
 M. GellMann and M. Lévy, “The axial vector current in beta decay,” Il Nuovo Cimento, vol. 16, pp. 705–726, 1960. View at: Publisher Site  Google Scholar  MathSciNet
 J. T. Lenaghan and D. H. Rischke, “The O(N) model at nonzero temperature: renormalization of the gap equations in Hartree and largeN approximations,” Journal of Physics G: Nuclear and Particle Physics, vol. 26, no. 4, pp. 431–450, 2000. View at: Publisher Site  Google Scholar
 N. Petropoulos, “Linear sigma model and chiral symmetry at finite temperature,” Journal of Physics G, vol. 25, no. 11, pp. 2225–2241, 1999. View at: Publisher Site  Google Scholar
 M. Lévy, “Currents and symmetry breaking,” Il Nuovo Cimento A, vol. 52, no. 1, pp. 23–49, 1967. View at: Publisher Site  Google Scholar
 B. Hu, “Chiral ${\text{SU}}_{4}\times {\text{SU}}_{4}$ and scale invariance,” Physical Review D, vol. 9, no. 6, pp. 1825–1834, 1974. View at: Publisher Site  Google Scholar
 J. Schechter and M. Singer, “SU(4) σ model,” Physical Review D, vol. 12, no. 9, pp. 2781–2790, 1975. View at: Publisher Site  Google Scholar
 H. B. Geddes, “Spinzero mass spectrum in the oneloop approximation in a linear SU(4) sigma model,” Physical Review D, vol. 21, no. 1, pp. 278–289, 1980. View at: Publisher Site  Google Scholar
 A. M. Polyakov, “Thermal properties of gauge fields and quark liberation,” Physics Letters B, vol. 72, no. 4, pp. 477–480, 1978. View at: Publisher Site  Google Scholar
 L. Susskind, “Lattice models of quark confinement at high temperature,” Physical Review D, vol. 20, no. 10, pp. 2610–2618, 1979. View at: Publisher Site  Google Scholar
 B. Svetitsky and L. G. Yaffe, “Critical behavior at finitetemperature confinement transitions,” Nuclear Physics B, vol. 210, no. 4, pp. 423–447, 1982. View at: Publisher Site  Google Scholar
 B. Svetitsky, “Symmetry aspects of finite temperature confinement transitions,” Physics Reports, vol. 132, no. 1, pp. 1–53, 1986. View at: Publisher Site  Google Scholar  MathSciNet
 B.J. Schaefer, J. M. Pawlowski, and J. Wambach, “Phase structure of the Polyakovquarkmeson model,” Physical Review D, vol. 76, no. 7, Article ID 074023, 2007. View at: Publisher Site  Google Scholar
 T. Kahara and K. Tuominen, “Degrees of freedom and the phase transitions of two flavor QCD,” Physical Review D, vol. 78, Article ID 034015, 2008. View at: Publisher Site  Google Scholar
 B.J. Schaefer and M. Wagner, “On the QCD phase structure from effective models,” Nuclear Physics, vol. 62, no. 2, pp. 381–385, 2009. View at: Publisher Site  Google Scholar
 M. Bluhm, B. Kämpfer, and G. Soff, “The QCD equation of state near T_{c} within a quasiparticle model,” Physics Letters B, vol. 620, no. 34, pp. 131–136, 2005. View at: Publisher Site  Google Scholar
 M. A. Thaler, R. A. Schneider, and W. Weise, “Quasiparticle description of hot QCD at finite quark chemical potential,” Physical Review C, vol. 69, no. 3, Article ID 035210, 2004. View at: Publisher Site  Google Scholar
 G. Boyd, J. Engels, F. Karsch et al., “Thermodynamics of SU(3) lattice gauge theory,” Nuclear Physics B, vol. 469, no. 3, pp. 419–444, 1996. View at: Publisher Site  Google Scholar
 M. Okamoto, A. A. Khan, S. Aoki et al., “Equation of state for pure SU(3) gauge theory with renormalization group improved action,” Physical Review D, vol. 60, Article ID 094510, 1999. View at: Publisher Site  Google Scholar
 A. N. Tawfik and N. Magdy, “Thermodynamics and higher order moments in SU(3) linear σmodel with gluonic quasiparticles,” Journal of Physics G: Nuclear and Particle Physics, vol. 42, no. 1, Article ID 015004, 2015. View at: Publisher Site  Google Scholar
 S. Borsanyi, Z. Fodor, C. Hoelbling, S. D. Katz, S. Krieg, and K. K. Szabo, “Full result for the QCD equation of state with 2+1 flavors,” Physics Letters B, vol. 370, pp. 99–104, 2014. View at: Publisher Site  Google Scholar
 E. Megías, E. R. Arriola, and L. L. Salcedo, “Polyakov loop in chiral quark models at finite temperature,” Physical Review D, vol. 74, Article ID 065005, 2006. View at: Publisher Site  Google Scholar
 E. Ruiz Arriola, L. L. Salcedo, and E. Megías, “Quark properties from the Hadron resonance gas,” Acta Physica Polonica B Proceedings Suplement, vol. 8, no. 2, pp. 439–444, 2015. View at: Publisher Site  Google Scholar
 F. Karsch, K. Redlich, and A. Tawfik, “Hadron resonance mass spectrum and lattice QCD thermodynamics,” European Physical Journal C, vol. 29, no. 4, pp. 549–556, 2003. View at: Publisher Site  Google Scholar  Zentralblatt MATH
 F. Karsch, K. Redlich, and A. Tawfik, “Thermodynamics at nonzero baryon number density: a comparison of lattice and hadron resonance gas model calculations,” Physics Letters, Section B: Nuclear, Elementary Particle and HighEnergy Physics, vol. 571, no. 12, pp. 67–74, 2003. View at: Publisher Site  Google Scholar
 K. Redlich, F. Karsch, and A. Tawfik, “Heavyion collisions and lattice QCD at finite baryon density,” Journal of Physics G: Nuclear and Particle Physics, vol. 30, no. 8, pp. S1271–S1274, 2004. View at: Publisher Site  Google Scholar
 A. Tawfik, “QCD phase diagram: a comparison of lattice and hadron resonance gas model calculations,” Physical Review D, vol. 71, Article ID 054502, 2005. View at: Publisher Site  Google Scholar
 A. Tawfik, “Influence of strange quarks on the QCD phase diagram and chemical freezeout,” Journal of Physics G, vol. 31, no. 6, pp. S1105–S1110, 2005. View at: Publisher Site  Google Scholar
 A. Tawfik, “Inmedium modifications of hadron properties,” Indian Journal of Physics, vol. 85, no. 5, pp. 755–766, 2011. View at: Publisher Site  Google Scholar
 A. Tawfik, “Phase space and dynamical fluctuations of kaontopion ratios,” Progress of Theoretical Physics, vol. 126, no. 2, pp. 279–292, 2011. View at: Publisher Site  Google Scholar
 A. Tawfik, “Antiprotontoproton ratios for ALICE heavyion collisions,” Nuclear Physics A, vol. 859, no. 1, pp. 63–72, 2011. View at: Publisher Site  Google Scholar
 A. Tawfik, “Matter–antimatter asymmetry in heavyion collisions,” International Journal of Theoretical Physics, vol. 51, no. 5, pp. 1396–1407, 2012. View at: Publisher Site  Google Scholar
 A. Tawfik, “On the higher moments of particle multiplicity, chemical freezeout, and QCD critical endpoint,” Advances in High Energy Physics, vol. 2013, Article ID 574871, 22 pages, 2013. View at: Publisher Site  Google Scholar
 A. Tawfik and D. Toublan, “Quarkantiquark condensates in the hadronic phase,” Physics Letters B, vol. 623, no. 12, pp. 48–54, 2005. View at: Publisher Site  Google Scholar
 R. Hagedorn, “Statistical thermodynamics of strong interactions at high energies,” Nuovo Cimento. Supplemento, vol. 3, pp. 147–186, 1965. View at: Google Scholar
 A. Bazavov, T. Bhattacharya, M. Cheng et al., “Chiral and deconfinement aspects of the QCD transition,” Physical Review D, vol. 85, no. 5, Article ID 054503, 2012. View at: Publisher Site  Google Scholar
 C. Schmidt, “Universal critical behavior and the transition temperature in (2+1)‐flavor QCD,” AIP Conference Proceedings, vol. 1343, p. 513, 2011. View at: Publisher Site  Google Scholar
 S. Borsanyi, Z. Fodor, C. Hoelbling et al., “QCD transition temperature: full staggered result,” in Proceedings of the 28th International Symposium on Lattice Field Theory (LATTICE '10), Villasimius, Italy, June 2010. View at: Google Scholar
 A. Tawfik, N. Magdy, and A. Diab, “Polyakov linear SU(3) $\sigma $ model: features of higherorder moments in a dense and thermal hadronic medium,” Physical Review C, vol. 89, no. 5, Article ID 055210, 2014. View at: Publisher Site  Google Scholar
 H. Mao, J. Jin, and M. Huang, “Phase diagram and thermodynamics of the polyakov linear sigma model with three quark flavors,” Journal of Physics G, vol. 37, no. 3, Article ID 035001, 2010. View at: Publisher Site  Google Scholar
 J. T. Lenaghan, D. H. Rischke, and J. SchaffnerBielich, “Chiral symmetry restoration at nonzero temperature in the $\text{SU}{(3)}_{r}\times \text{SU}{(3)}_{l}$ linear sigma model,” Physical Review D, vol. 62, Article ID 085008, 2000. View at: Publisher Site  Google Scholar
 B.J. Schaefer and M. Wagner, “Threeflavor chiral phase structure in hot and dense QCD matter,” Physical Review D: Particles, Fields, Gravitation and Cosmology, vol. 79, no. 1, Article ID 014018, 2009. View at: Publisher Site  Google Scholar
 P. Kovács and Z. Szép, “Critical surface of the $SU{(3)}_{L}\times SU{(3)}_{R}$ chiral quark model at nonzero baryon density,” Physical Review D, vol. 75, Article ID 025015, 2007. View at: Publisher Site  Google Scholar
 S. Rößner, C. Ratti, and W. Weise, “Polyakov loop, diquarks, and the twoflavor phase diagram,” Physical Review D, vol. 75, Article ID 034007, 2007. View at: Publisher Site  Google Scholar
 B.J. Schaefer, J. M. Pawlowski, and J. Wambach, “Phase structure of the Polyakovquarkmeson model,” Physical Review D, vol. 76, Article ID 074023, 2007. View at: Publisher Site  Google Scholar
 O. Scavenius, Á. Mócsy, I. N. Mishustin, and D. H. Rischke, “Chiral phase transition within effective models with constituent quarks,” Physical Review C, vol. 64, no. 4, Article ID 045202, 2001. View at: Google Scholar
 J. I. Kapusta and C. Gale, FiniteTemperature Field Theory: Principles and Applications, Cambridge University Press, Cambridge, UK, 2006. View at: Publisher Site  MathSciNet
 P. Lévai and U. Heinz, “Massive gluons and quarks and the equation of state obtained from SU(3) lattice QCD,” Physical Review C: Nuclear Physics, vol. 57, no. 4, pp. 1879–1890, 1998. View at: Publisher Site  Google Scholar
 P. Romatschke, “Quasiparticle description of the hot and dense quarkgluon plasma,” http://arxiv.org/abs/hepph/0312152. View at: Google Scholar
 M. Bluhm, B. Kämpfer, R. Schulze, D. Seipt, and U. Heinz, “A Family of equations of state based on lattice QCD: impact on flow in ultrarelativistic heavyion collisions,” Physical Review C, vol. 76, no. 3, Article ID 034901, 2007. View at: Publisher Site  Google Scholar
 J. ZinnJustin, Quantum Field Theory and Critical Phenomena, vol. 113 of International Series of Monographs on Physics, 2002.
 A. A. Osipov, B. Hiller, and J. da Providência, “Multiquark interactions with a globally stable vacuum,” Physics Letters B, vol. 634, no. 1, pp. 48–54, 2006. View at: Publisher Site  Google Scholar
 A. Bhattacharyya, P. Deb, S. K. Ghosh, and R. Ray, “Investigation of the phase diagram and bulk thermodynamic properties using the PolyakovNambuJonaLasinio model with eightquark interactions,” Physical Review D, vol. 82, no. 1, Article ID 014021, 2010. View at: Publisher Site  Google Scholar
 C. Ratti, M. A. Thaler, and W. Weise, “Phases of QCD: lattice thermodynamics and a field theoretical model,” Physical Review D: Particles, Fields, Gravitation and Cosmology, vol. 73, no. 1, 2006. View at: Publisher Site  Google Scholar
 C. A. Islam, R. Abir, M. G. Mustafa, R. Ray, and S. K. Ghosh, “The consequences of SU (3) colorsingletness, Polyakov Loop and Z (3) symmetry on a quarkgluon gas,” Journal of Physics G: Nuclear and Particle Physics, vol. 41, no. 2, Article ID 025001, 2014. View at: Publisher Site  Google Scholar
 J. Moreira, B. Hiller, A. A. Osipov, and A. H. Blin, “Thermodynamic potential with correct asymptotics for PNJL model,” International Journal of Modern Physics A, vol. 27, no. 11, Article ID 1250060, 2012. View at: Publisher Site  Google Scholar
 R. Venugopalan and M. Prakash, “Thermal properties of interacting hadrons,” Nuclear Physics A, vol. 546, no. 4, pp. 718–760, 1992. View at: Publisher Site  Google Scholar
 A. Majumder and B. Müller, “Hadron mass spectrum from lattice QCD,” Physical Review Letters, vol. 105, no. 25, Article ID 252002, 4 pages, 2010. View at: Publisher Site  Google Scholar
 R. Hagedorn, “Statistical thermodynamics of strong interactions at high energies,” Nuovo Cimento Supplemento, vol. 3, pp. 147–186, 1965. View at: Google Scholar
 R. Hagedorn, “Largeangle crosssections $\text{p}+\text{p}\to \text{A}+\text{B}$ and $\pi +\text{p}\to \text{A}+\text{B}$ at high energies predicted by the statistical model,” Il Nuovo Cimento, vol. 35, no. 1, pp. 216–226, 1965. View at: Publisher Site  Google Scholar
 W. Broniowski, F. Giacosa, and V. Begun, “Why the sigma meson should not be included in thermal models,” http://arxiv.org/abs/1506.01260. View at: Google Scholar
 M. A. Stankiewicz, “Entropy in the thermal model,” http://arxiv.org/abs/nuclth/0509058. View at: Google Scholar
 J. Cleymans, H. Oeschler, K. Redlich, and S. Wheaton, “Transition from baryonic to mesonic freezeout,” Physics Letters B, vol. 615, no. 12, pp. 50–54, 2005. View at: Publisher Site  Google Scholar
 A. Tawfik, “A universal description for the freezeout parameters in heavyion collisions,” Nuclear Physics A, vol. 764, no. 1–4, pp. 387–392, 2006. View at: Publisher Site  Google Scholar
 A. Tawfik, “Condition driving chemical freezeout,” Europhysics Letters, vol. 75, no. 3, pp. 420–426, 2006. View at: Publisher Site  Google Scholar
 A. Tawfik, “Chemical freezeout and higher order multiplicity moments,” Nuclear Physics A, vol. 922, pp. 225–236, 2014. View at: Publisher Site  Google Scholar
 A. Tawfik, “Constanttrace anomaly as a universal condition for the chemical freezeout,” Physical Review C, vol. 88, no. 3, Article ID 035203, 2013. View at: Publisher Site  Google Scholar
 R. Dashen, S.K. Ma, and H. J. Bernstein, “Smatrix formulation of statistical mechanics,” Physical Review, vol. 187, no. 1, pp. 345–370, 1969. View at: Publisher Site  Google Scholar
 A. Tawfik, M. Y. ElBakry, D. M. Habashy, M. T. Mohamed, and E. Abbas, “Degree of chemical nonequilibrium in central AuAu collisions at RHIC energies,” International Journal of Modern Physics E, vol. 25, no. 8, 2015. View at: Publisher Site  Google Scholar
 C. Schmidt, “Universal critical behavior and the transition temperature in (2+1)flavor QCD,” AIP Conference Proceedings, vol. 1343, pp. 513–515, 2011. View at: Publisher Site  Google Scholar
 J. Gasser and H. Leutwyler, “Chiral perturbation theory: expansions in the mass of the strange quark,” Nuclear Physics B, vol. 250, no. 1–4, pp. 465–516, 1985. View at: Publisher Site  Google Scholar
 M. Cheng, S. Ejiri, P. Hegde et al., “Equation of state for physical quark masses,” Physical Review D, vol. 81, no. 5, Article ID 054504, 8 pages, 2010. View at: Publisher Site  Google Scholar
 F. Karsch, “The last word(s) on CPOD 2013,” in Proceedings of the 8th International Workshop on Critical Point and Onset of Deconfinement (CPOD '13), p. 46, Napa, Calif, USA, March 2013. View at: Google Scholar
 Y. Aoki, S. Borsányi, S. Dürr et al., “The QCD transition temperature: results with physical masses in the continuum limit II,” Journal of High Energy Physics, vol. 2009, no. 6, article 088, 2009. View at: Publisher Site  Google Scholar
 A. Bazazov, T. Bhattacharya, M. Cheng et al., “Chiral and deconfinement aspects of the QCD transition,” Physical Review D, vol. 85, no. 5, Article ID 065503, 37 pages, 2012. View at: Publisher Site  Google Scholar
 A. Tawfik and E. Abbas, “Thermal description of particle production in AuAu collisions at RHIC energies (STAR),” Physics of Particles and Nuclei Letters, vol. 12, no. 4, pp. 521–531, 2015. View at: Publisher Site  Google Scholar
 F. Becattini, M. Bleicher, T. Kollegger, T. Schuster, J. Steinheimer, and R. Stock, “Hadron formation in relativistic nuclear collisions and the QCD phase diagram,” Physical Review Letters, vol. 111, Article ID 082302, 2013. View at: Publisher Site  Google Scholar
 R. Stock, F. Becattini, M. Bleicher, T. Kollegger, T. Schuster, and J. Steinheimer, “Hadronic freezeout in A+A collisions meets the lattice QCD PartonHadron transition line,” in Proceedings of the 8th International Workshop on Critical Point and Onset of Deconfinement (CPOD '13), p. 11, Napa, Calif, USA, March 2013. View at: Google Scholar
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Copyright © 2015 Abdel Nasser Tawfik and Niseem Magdy. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited. The publication of this article was funded by SCOAP^{3}.