Review Article  Open Access
FreezeOut Parameters in HeavyIon Collisions at AGS, SPS, RHIC, and LHC Energies
Abstract
We review the chemical and kinetic freezeout conditions in high energy heavyion collisions for AGS, SPS, RHIC, and LHC energies. Chemical freezeout parameters are obtained using produced particle yields in central collisions while the corresponding kinetic freezeout parameters are obtained using transverse momentum distributions of produced particles. For chemical freezeout, different freezeout scenarios are discussed such as single and double/flavor dependent freezeout surfaces. Kinetic freezeout parameters are obtained by doing hydrodynamic inspired blast wave fit to the transverse momentum distributions. The beam energy and centrality dependence of transverse energy per charged particle multiplicity are studied to address the constant energy per particle freezeout criteria in heavyion collisions.
1. Introduction
As a result of ultrarelativistic collision between two heavy ions, a fireball is expected to form that rapidly thermalizes. The enormous amount of energy density deposited in the fireball results in large pressure gradients from the central to the peripheral region of the fireball that drives the expansion of the fireball. This expansion leads to cooling of the fireball. Further, as the interparticle distance grows with time, the particles cease to interact after sometime and free stream to the detector. The surface of last scattering is the freezeout surface. Since scattering could be both elastic (where particle identities do not change) and inelastic (where particle identities change), it is possible to have two distinct freezeouts, namely, chemical freezeout (CFO), where inelastic collisions cease, and thermal/kinetic freezeout (KFO) where elastic collisions cease and the particle mean free path becomes higher than the system size, which forbids the elastic collision of the constituents in the system [1]. While the CFO surface is determined by analysing the measured hadron yields [2–5], the KFO surface can be determined by studying the data of transverse momentum () distribution of produced particles [6–11]. In general, freezeout could be a complicated process involving duration in time and a hierarchy where different types of particles and reactions switchoff at different times. This leads to the concept of “sequential freezeout.” From kinetic arguments, it is expected that reactions with lower crosssections switchoff at higher densities/temperature or earlier in time compared to reactions with higher crosssections. Hence, the chemical freezeout, which corresponds to inelastic reactions, occurs earlier in time compared to the kinetic freezeout, which corresponds to elastic reactions. In accordance with the above discussions, one can think of strange or charmed particles decoupling from the system earlier than the lighter hadrons. A series of freezeouts could be thought of corresponding to particular reaction channels [12].
In this review, we present the detailed study of chemical and kinetic freezeout scenario in central heavyion collisions from the lower AGS energies to the largest LHC energies. The paper is organized as follows. In the next section, we discuss chemical freezeout followed by introduction to chemical freezeout models employed and then present results and discussions. Section 3 consists of discussions on transverse energy per charged particle and the freezeout criteria. In Section 4, we discuss the kinetic freezeout properties obtained using hydrodynamic inspired blast wave model fit to the experimental data. Finally, in Section 5, we give summary and conclusions.
2. Chemical FreezeOut
Quantum Chromodynamics (QCD) which is the quantum field theory that addresses the physics of strong interactions has three conserved charges, namely, baryon number , electric charge , and strangeness . Thus, the equilibrium thermodynamic state of QCD matter is completely determined by temperature and the three chemical potentials , , and corresponding to , , and , respectively. Various thermodynamic quantities like pressure, energy density, and so forth, and even different susceptibilities of conserved charges of QCD computed in lattice QCD at zero compare well with hadron resonance gas (HRG) model predictions for the same up to the quarkhadron transition region around 150–160 MeV [13–15]. Thus, HRG which is a gas of noninteracting hadrons and resonances is a good low approximation to QCD thermodynamics. These models have also been quite successful in describing the particle multiplicities measured in heavyion collision experiments across a wide range of beam energies from GeV [2–5] with a few thermal parameters to be fitted from data. Apart from heavy ion collisions, even in systems like and , statistical models have been found to successfully describe the particle multiplicities [16]. For a recent interpretation of such universal behaviour of particle production, please look at [17]. However, recent lattice QCD results on strangeness fluctuations and correlations show that strange hadrons currently unobserved but predicted by quark models and lattice computations can influence the value of the extracted freezeout temperature within a HRG model approach [18]. For a detailed estimate of the effect of the additional strange hadrons on the freezeout parameters one needs to model their decay properties. We leave such an exercise for the future. In this review, the hadronic spectrum includes only hadrons listed in the PDG [19].
Out of the three chemical potentials it is a common practice to fix and from the following constraints: Thus, the usual set of free parameters that are fitted to the data are , , and an overall normalization factor which is the volume . An additional parameter called the strangeness suppression factor which accounts for any out of equilibrium production of strangeness is also often used. Such a program allows us to determine the thermodynamic state of the fireball at the time of CFO and hence sets a baseline for all hadronic thermal physics to be pitted against data to isolate signals for quark gluon plasma (QGP) as well as the QCD critical point. Thus, it is necessary to have a very detailed and vivid understanding of the physics of the CFO.
The traditional picture of CFO is where all the hadrons chemically freezeout together (1CFO). Such a picture provides a descent qualitative description of the hadron multiplicities at all the beam energies with a few exceptions where the , where is number of degrees of freedom, is significantly large.
The latest LHC data has posed a serious challenge to this 1CFO picture where the strange to nonstrange particle ratios like cannot be explained [20]. This has led to proposals for various alternate freezeout schemes. In [21], hadronization followed by hadronic afterburner within the hybrid UrQMD model was employed. PYTHIA generated initial condition was followed by hydrodynamic expansion. Then, around energy density of 700 MeV/fm^{3}, using CooperFrye prescription, hadrons were formed and the system entered a transport stage that mainly caused late stage baryonantibaryon annihilation. This resulted in successful description of all the particle yields. Such an approach has also been employed to successfully describe the centrality dependence of the hadron yields at the LHC [22]. These studies yield a hadronization temperature of MeV for vanishing baryon chemical potential. In another approach, 1CFO with nonequilibrium quark phase space factors for light and strange quarks were used [23]. This also resulted in good description of the yields.
Both the above approaches accounted for effects on particle yields due to departure from equilibrium physics. In yet another approach, it was realised that one could describe the particle yields within the ambit of equilibrium physics by proposing flavor dependent freezeout surfaces (2CFO) [24, 25]. It was argued on the basis of hadrochemistry that strange and nonstrange hadrons could freezeout at different times (2CFO). In 2CFO, all strange hadrons and those with hidden strangeness freezeout at the same surface while the rest of the non strange hadrons freezeout at a separate surface. Here, we will study the dependence of the extracted freezeout thermal parameters on (a) the choice of the thermodynamic ensemble, (b) choice of the free parameters, (c) choice of particles whose yields are used as inputs to extract the values of the thermal parameters, and (d) choice of the CFO scheme. We find that this program yields fairly robust values of the thermal parameters that show little sensitivity to the specific details of the fitting procedure. Having obtained and studied the systematics of the CFO parameters, we compute several particle ratios and compare with the available data. We find that ratios of particles of unlike flavor are particularly sensitive to the choice of the CFO scheme [26].
2.1. Model
In the most general case, different hadron species would chemically decouple from the fireball at different freezeout surfaces at different times. Thus, the grand partition function of all the hadrons that are emitted at different times from the fireball can be written as a product of the partition function at each freezeout surface as the freezeout at two different surfaces are independent processes. Thus, for a given , the relevant HRG partition function in the Grand Canonical Ensemble (GCE) is given by a summed contribution over single particle partition functions of all hadrons:where is the partition function of the hadron. and are the temperature and volume, respectively, of the fireball as well as the hadron at the time of its CFO. In terms of the corresponding fireball chemical potentials , , and , the hadron chemical potential is expressed as where , , and are the quantum numbers of the hadron. In 1CFO, there is a single CFO surface and hence for all hadrons. Similarly, , , , and are same for all hadrons. In 2CFO, there are two CFO surfaces. for all nonstrange hadrons while for all strange hadrons and those with hidden strangeness content. Volume and chemical potentials are also treated similarly. A partial derivative with respect to gives the primordial yield of the hadron :where for bosons and for fermions and is the Bessel function of the second kind. and are the mass and degeneracy factor of the hadron and its conserved charges are , , and . The total multiplicity of the hadron is given by a sum of the primordial yield as well as feeddown from heavier resonances that decay to it where taken from P.D.G. [19] is the branching ratio for the hadron to decay to the hadron.
The publicly available code THERMUS [27] allows one to compute the hadron yields in 1CFO within the GCE as well as various other ensembles like the canonical ensemble where all the charges are conserved exactly or treat the charges in a mixed ensemble. For example in the Strangeness Canonical Ensemble (SCE), the baryon and electric charges are conserved on an average in the GCE while strangeness is treated in the canonical ensemble. We have analysed all available hadronic yields and ratios at AGS, SPS, RHIC, and LHC experiments within GCE and SCE with 1CFO as the freezeout scheme in the THERMUS code. We have also analysed the same data with 2CFO freezeout scheme [24]. The unified CFO thermal parameters in 1CFO lie intermediate to the freezeout parameters of the strange and nonstrange CFO surfaces in case of 2CFO. We also report several particle ratios, particularly strange to nonstrange particle ratios that are sensitive to the CFO mechanism chosen.
2.2. Results and Discussions
In Tables 1, 2, 3, and 4, an exhaustive compilation of multiplicity data for the central case available at various beam energies are shown. In addition to the AGS [28–37], SPS [38–46], RHIC data at , 130, and 200 GeV [55–62], and LHC [63] for which the CFO thermal parameters within 1CFO have been already well established, here we have also analysed the preliminary data from RHIC Beam Energy Scan (BES) program [47, 73–78] at , 11.5, 19.6, 27, and 39 GeV [48–54]. While data for nonstrange and strange mesons and baryons are available for all the energies from SPS onwards, data of the multistrange baryons are not available at the AGS energies (data for is only available at the top AGS energies). As we will note later, this has direct consequence on the extraction of the thermal parameters. While and seem to be mildly sensitive to the presence of the strange baryons, the extracted value of seem to lower significantly from the expected trend at the AGS energies due to the absence of the strange baryons from the fits. This is expected since at the AGS energies the fireball is baryon dominated due to large baryon stopping which results in higher values of as compared to SPS energies [79]. Thus, strange baryons like , , and are expected to play a significant role in determining as compared to which is dominant at higher energies where is small and we have a meson dominated fireball. For all the fits reported here, we always obtain from (1). and are sometimes kept as free parameters while at other times we obtain from (2) and fix to unity. , , and volume are always treated as free parameters.



Currently, at the BES energies, data for , , , , , , , , , and are available. We use the same particles for the SPS, top RHIC, and LHC energies for a uniform treatment at all energies. The extracted thermal parameters (a) , (b) (, , and ), (c) , and (d) radius, which is reflective of volume of the system, are shown in Figure 1. Results for both SCE and GCE are shown for comparison. We find that the results are quite similar in the two ensembles studied. However, as seen in Figure 5, the is consistently lower for SCE than GCE at all energies mainly because there is one less parameter to fit in case of SCE. We have also repeated the same exercise using ratios instead of yields. We found that though the extracted and parameters are consistent within errors for the two cases, in general the central values for () are higher (lower) when particle yields are used for fitting compared to the case when particle ratios are used. The is reduced in ratio case as the uncertainty over volume is irrelevant. However, it is not advisable to use ratios for fitting as the specific choice of independent ratios out of various possibilities could bias the results of the fits [80]. This will become more clear from our later discussion on particle ratios.
(a)
(b)
(c)
(d)
In the above case we had treated as a free parameter and extracted it from fits to data. One could also impose strangeness neutrality condition as in (2) and extract from it. We had also allowed to be a free parameter. However, as seen from Figure 1, does not seem to show any systematic dependence with and hovers around unity. We thus repeated the fits for two further different parameter sets. In one case we still allowed to be free while fixed from (2) while in the other case we fixed in addition to fixing . We have compared these three cases in Figure 2. While the thermal parameters extracted seem to be very robust and hence insensitive to the different fitting procedures, is least for the case where is held at unity and is solved from the constraint (2). This is mainly because this case has the least number of free parameters and hence is the largest.
(a)
(b)
(c)
(d)
So far we have been working with only , , , , , , , , , and for uniform treatment. Having studied the dependence on the choice of ensembles and fitting procedures with the above uniform particle set at all available energies, we now extend our input particle yield database to all available particles like and at all energies. In Figure 3, we have presented the above comparison within the GCE with and and fixed from the constraints given by (1) and (2). Overall, the thermal parameters show mild dependence on the inclusion of and . At AGS energies, the extracted and fall short of the expected value from the SPS trend due to the absence of the strange baryons from the input database.
(a)
(b)
(c)
Thus, in general, the extracted thermal parameters are quite robust and insensitive to details like choice of ensembles, fitting procedures and whether or not particles like and are included in the fits. All the above fits were done within 1CFO. As seen from Figure 5, which is a measure of the goodness of fits is quite large at few energies. This has led to efforts to develop new freezeout schemes which can describe the yields better. One such development which we will discuss here is the 2CFO scheme of CFO. We have already discussed the 2CFO scheme in detail in Section 2.1. In Figure 4, we have presented the thermal parameters extracted in the 2CFO scheme and compared with those of 1CFO in the SCE with and solved from (1). At all the energies we find that the nonstrange freezeout temperature is consistently lower than the strange freezeout temperature . While at the LHC, , and differ by about 5%, at the top SPS energy they differ by about 15%. This can be interpreted as an early freezeout for the strange hadrons [24, 83]. The 1CFO thermal parameters lie intermediate to the corresponding 2CFO values for the nonstrange and strange CFO surfaces. There is substantial improvement in for 2CFO as compared to 1CFO.
(a)
(b)
Now we will look at how well we can describe the different particle ratios within 1CFO and 2CFO freezeout schemes. As argued in [26], strange to nonstrange particle ratios are particularly sensitive to the choice of CFO scheme. This is easily understood from the following expression for the particle ratios in HRGThe above equation is obtained from (5) by taking the asymptotic limit . It is clearly evident from (7) that for ratios of particles of unlike flavors, the thermal factor coefficient does not cancel off while in 1CFO this additional factor does not arise at all. Thus, ratios of particles of unlike flavor are good probes to distinguish different freezeout schemes. In Figure 6, we have compared the particle ratios as obtained in 1CFO and 2CFO models of CFO and compared them with data. The data for ratios are obtained from the ratios of the data of corresponding yields while the errors are computed in quadratures. As argued above, we see that particle ratios of unlike flavor like and discriminate between different CFO schemes while those of same flavor like and appear similar in both the schemes. We also find 2CFO to describe all the ratios better as compared to 1CFO.
(a)
(b)
(c)
(d)
We have also plotted a triple ratio in Figure 6. Since the total , and charges carried by are same as those carried by and together, the fugacity factors cancel off and this ratio is to a very good approximation unity in 1CFO [84]. However, in 2CFO there is no such constraint. We find in data appreciable deviation from unity below GeV which can not be described in 1CFO. Currently the errors are very large and hence it is difficult to conclude anything definite. The main reason behind this is that the errors have been computed in quadratures. This might have led to an overestimate of the errors. A proper estimate of the errors of these quantities by taking into account correlations among various sources of errors is highly desired from experimental side.
With the availability of experimental data on light nuclei yields, we can also test the CFO (2CFO and 1CFO/THERMUS) model calculations for the light nuclei production. Figure 7 shows the ratio of light nuclei as a function of energy . Figure 7(a) is for ratio and Figure 7(b) is for . The solid circles denote the experimental data and bands are used to represent model calculations. In case of THERMUS calculation, the chemical freezeout temperature () and baryon chemical potential () are obtained corresponding to a given energy using relation as in [81]. For a given and , one can predict nuclei yields and hence ratios at a given energy. As discussed above, the being a like flavor ratio does not discriminate between the different freezeout schemes (1CFO or 2CFO) while being representing strange to nonstrange ratio shows the difference between two schemes. For the latter, the well known discrepancy between data and thermal model with 1CFO at = 200 GeV [85, 86] goes away in 2CFO [26]. The grand canonical approach in THERMUS explains the ratio very well; however, ratio at = 200 GeV is quite high in data compared to the expected value in THERMUS for both the GCE as well as the SCE approach.
(a)
(b)
3. Transverse Energy per Charged Particle and FreezeOut Criteria
The transverse energy is one of the important global observables used to characterize the system formed in heavyion collisions at extreme conditions of temperature and energy density, where the formation of QGP is expected. The transverse energy () is the energy produced transverse to the beam direction and is closely related to the collision geometry. is an eventbyevent variable defined asThe sum is taken over all particles produced in an event into a fixed but large solid angle. and are the energy and polar angle that a final state particle makes with the detector. The energy of the individual particles can be measured by knowing their momenta and particle identification and/or the total energy deposited in a calorimeter. To probe the early stages of the produced fireball, it is ideal to take transverse observables such as and . This is because, before the collision of two nuclei, the longitudinal phase space is filled by the beam particles whereas the transverse phase space is empty. The is produced due to the initial scattering of the partonic constituents of the incoming nuclei and also by the rescattering among the produced partons and hadrons [87, 88]. The production tells about the explosiveness of the interaction. In addition, the collision centrality can be estimated by using the distribution [89]. The ratio of pseudorapidity densities of transverse energy and number of charged particles at midrapidity, that is, , has been studied both experimentally [65, 69, 90] and phenomenologically [91–93] to understand the underlying particle production mechanism. This observable is known as global barometric measure of the internal pressure in the ultradense matter produced in heavyion collisions [94]. This quantity depends on the initial state of the collision and the viscosity of the matter as it expands to its final state, when it is observed by the detectors [95].
This observable when studied as a function of collision energy (as shown in Figure 8), shows three regions of interest. The first one from the lower SIS energies to SPS energies shows a steep increase of values, thereby indicating that the mean energy of the system increases. In the second region, from SPS to top RHIC energy, shows a very weak collision energy dependence, that is, like a saturation behaviour (Table 5 and Figure 8). In this region the mean energy does not increase, whereas the collision energy increases. This may indicate that the increase in collision energy results in new particle production in this energy domain, which is consistent with higher particle multiplicity observed at these energies. This behaviour has been well described in the context of a Statistical Hadron Gas Model (SHGM) [91, 92]. In the framework of SHGM, it has been predicted that would saturate at energies higher to that of top RHIC energy with a limiting value of 0.83 GeV [91, 92]. Here, a static fireball is assumed at the freezeout. However, a value of GeV is observed at the LHC 2.76 TeV center of mass energy recently, by the CMS collaboration [69]. This creates a third region in the excitation function of , showing a jump from top RHIC to LHC energies. In this region, along with particle multiplicity, the mean energy per particle also increases, which needs to be understood from theoretical models taking the dynamics of the time evolution of the created fireball. It is however, observed that models based on final state gluon saturation (CGC like) seem to explain this behaviour in the excitation function of [96]. The RHIC BES data seem to follow the overall trend of the collision energy dependence of . It has been seen in one of the previous works [92] that various freezeout criteria like constant energy per particle ( GeV) [97], fixed baryon + antibaryon density () [98], fixed entropy density per ) [79, 99] seem to describe the qualitative energy dependent behaviour of quite consistently.

The behavior ) as a function of energy can naively be related to first order phase transition as discussed below. If we assume the system to be following thermodynamic behavior, then may be interpreted as temperature at freezeout (volume considered to be constant at freezeout) while the collision energy may be interpreted as entropy. This figure, then could be considered as temperature versus entropy diagram, where an observed plateau represents a first order phase transition [100]. Therefore, one can say that temperature increases at very lower energies with an increase of collision energy, then remains almost constant from collision energy of about 20 GeV up to the top RHIC energies. Then, it shows an increase again from top RHIC to LHC energies. This observation of constant temperature from 20 to 200 GeV can be interpreted as the first order phase transition turning on around 20 GeV. Similar behavior is observed for the versus collision energy, being the transverse mass [53].
Figure 9 shows the plotted versus , which is a measure of centrality. Table 6 shows the corresponding values for different centralities at various energies. Within the systematic errors, for all energies show a weak centrality dependence with a modest increase from most peripheral collisions to , reaching a roughly constant value towards central collisions. This centrality dependence of is shown to be equivalent to the behaviour of as a function of centrality for top RHIC energy [90] and for TeV [101] at LHC. The value of GeV/c for TeV, which is almost 37% higher as compared to the (0.5 GeV/c) at top RHIC energy [90]. This shows that not only particle multiplicity increases while going from top RHIC energy to LHC energy, the also increases, making a third region in the excitation function of . The near centrality independent behaviour of is explained by SHGM with a static fireball approximation at freezeout [91]. If the freezeout is assumed to occur at all collision energies and impact parameters in heavyion collisions on a fixed decoupling isotherm, then the energy per particle will always be the same. This possibly is the fact up to top RHIC energy within experimental uncertainties. However, the LHC measure of a higher value of needs to be understood in the above context keeping in mind that there is hardly any change of while going from top RHIC energy to LHC energy at 2.76 TeV [102]

At higher energies, when , the transverse energy production is mainly due to the meson content of the system. The experimental observations go in line with the above fact, when we observe the ratio of at higher energies. The intersection points of lines of constant and the freezeout line give the values of at the chemical freezeout.
4. Kinetic FreezeOut
At chemical freezeout, the inelastic interactions among the produced particles stop. However, these particles can still interact elastically which could affect their momentum distributions. A point in time after the collision, when the elastic interactions among the particles also stop is called the kinetic freezeout. At that time, the transverse momentum distributions of the particles get fixed and do not change thereafter. The transverse momentum distribution of particles contains two components—random and the collective. The random component depends on the temperature of the system at kinetic freezeout (). The collective component is generated by collective flow in the transverse direction given by the transverse flow velocity .
The and average transverse flow velocity of the system can be obtained using the hydrodynamicsmotivated Blast Wave model [6–11], assuming thermal equilibrium. The model assumes that the particles are locally thermalized at kinetic freezeout temperature and are moving with a common transverse collective flow velocity. Assuming a radially boosted thermal source, with a kinetic freezeout temperature and transverse radial flow velocity , the transverse momentum distribution of the particles can be given by where , , and and are the modified Bessel functions. We use the flow velocity profile of the form , where is the surface velocity, is the relative radial position in the thermal source, and is the exponent of flow velocity profile. Average transverse radial flow velocity can then be obtained as .
Usually, the spectra of the six particles (, and ) are fitted simultaneously with the blast wave model to extract the parameters such as , , and . Figure 10 shows the spectra for , , and in central collisions at different energies. For clarity, the spectra for positively charged particles are not shown. These spectra are used to extract the kinetic freezeout parameters using blast wave model. The curves in the figure represent the blast wave model fits to the data and can be seen to reasonably describe the spectra of , and at all energies. The results compiled here are taken from [42, 53, 55, 70–72]. All these results use same particles (, and ) for blastwave fitting except the 10.8 GeV ( = 4.8 GeV) energy corresponding to AGS, which use , , , and spectra; and = 17.3 GeV, where , , and are used. The ranges used for fitting of these spectra are given in Table 7. The low part of pion spectra is affected by resonance decays due to which the pion spectra is fitted above 0.5 GeV/c or ( 0.4 GeV/c^{2} for = 4.8 GeV.

Figure 11(a) shows the energy dependence of kinetic and chemical freezeout temperatures and Figure 11(b) shows and plotted versus . For chemical freezeout temperature and/or , we have taken the values obtained using 1CFO GCE fit to the particle yields as discussed in previous sections. We observe that the values of kinetic and chemical freezeout temperatures are similar around 45 GeV. If the collision energy is increased, the chemical freezeout temperature increases and becomes constant after the 11.5 GeV. However, the is almost constant around the 7.7–39 GeV and then decreases up to LHC energies. The separation between and increases with increasing energy (or decreasing ). This might suggest the effect of increasing hadronic interactions between chemical and kinetic freezeout towards higher energies.
(a)
(b)
Figure 12 shows the average flow velocity plotted as a function of . Value of is about 0.4 times the speed of light at around 500 MeV. For 200–400 MeV, the remains almost constant and then increases when the decreases to lower values corresponding to LHC energies. The SPS (NA49) data at 220 MeV (corresponding to 17.3 GeV) has mean value little higher although consistent within error bars with BES results at nearby energies. This slight difference between BES and SPS data is may be due to different particle species and rapidity regions (as given in Table 7) used in blast wave fitting. Since reflects the expansion in the transverse direction, it is interesting to note that expansion is constant around 200–400 MeV corresponding to beam energies 7.7, 11.5, and 19.6 GeV.
It may be noted that the blastwave results are sensitive to the particle species as well as ranges and rapidity regions used for fits. However, it is difficult to satisfy consistent conditions for above mentioned properties across different experiments due to different technicality of detectors as well as due to different energy regimes where these experiments operate. In addition, the spectra also become harder and harder when we go towards higher energy. The results presented here though use common ranges but not exact same ranges as can be seen from Table 7. It will be interesting to see how the energy or dependence of and looks like if similar kinematic ranges and particle species are used. To demonstrate effect of ranges on the blast wave fitting, as an example, for ALICE experiment at LHC energy, we have tested to use same ranges as used in BES energies at RHIC (see Table 7). The mean values of the results obtained are 104 MeV, = 0.639, and 0.710. Similarly, using fit ranges: 0.5–1.0 GeV/c for pions, 0.2–1.5 GeV/c for kaons, and 0.3–3 GeV/c for protons, lead to the following mean values of fit parameters: 95 MeV, = 0.651, and 0.712 [72]. Clearly, the fit parameters are sensitive to fitting ranges and hence one needs to be careful interpreting results when kinematic conditions are different.
5. Summary
We have presented the systematic study of chemical and kinetic freezeout conditions obtained at different energies from AGS, SPS, RHIC, and LHC.
The dependence of chemical freezeout parameters on various factors like choice of thermodynamic ensemble, choice of free parameters and fitting procedures, choice of particles whose yields and/or particle ratios are used as inputs in the fits, and choice of chemical freezeout schemes have been studied in detail. While we find weak dependence of the extracted thermodynamic parameters on most of the factors listed above, choice of chemical freezeout scheme seems to influence the fitted thermal parameters significantly. Particularly, strange to nonstrange particle ratios are most sensitive to the chosen chemical freezeout scheme.
The barometric observable, transverse energy per charged particle, is related to the chemical freezeout. Various freezeout criteria seem to describe the energy dependent behavior of starting from few GeV to top RHIC energies. A static fireball approximation at freezeout, however, fails to reproduce the corresponding data at LHC and necessitates the inclusion of fireball evolution dynamics in space and time in order to describe the behavior for the whole range of energies. The similarity in the centrality dependence up to top RHIC energy indicates that irrespective of the collision species and center of mass energies, the system evolves to a similar final state at freezeout.
The kinetic freezeout temperature suggests a decrease from lower to higher energies. The separation between chemical and kinetic freezeout temperatures increases while going towards lower (or higher energies) indicating increasing hadronic interactions between chemical and kinetic freezeout at higher energies. The average transverse radial flow velocity is around 40% of speed of light at 500 MeV. The expansion in the radial direction remains similar around 200–400 MeV and then increases towards lower or higher energies reflecting higher pressure or higher initial energy density produced in these collisions.
Conflict of Interests
The authors declare that there is no conflict of interests regarding the publication of this paper.
Acknowledgment
Bedangadas Mohanty is supported by the DAESRC project fellowship for this work.
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Copyright
Copyright © 2015 Sandeep Chatterjee et al. 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}.