Services on Demand
- Cited by SciELO
- Access statistics
Print version ISSN 0103-9733
On-line version ISSN 1678-4448
Braz. J. Phys. vol.37 no.1a São Paulo Mar. 2007
Color flavor locked phase transition in strange quark matter
Milva OrsariaI; H. RodriguesII; S. B. DuarteI
ICentro Brasileiro de Pesquisas Físicas, Rua Dr. Xavier Sigaud 150 CEP 22290-180, Rio de Janeiro, Brazil
IICentro Federal de Educação Tecnológica CEFET/RJ, CEP 20271-110, Rio de Janeiro, Brazil
We discuss macroscopic aspects of quark matter phase transition in cold dense stellar matter, considering global charge neutrality and baryonic charge conservation. We determine the critical condition for the phase transition between the strange quark matter, SQM, and the color-flavor locked, CFL, superconducting phase. We also discuss the sensitivity of our results to variations in the gap energy, D, and in the current strange quark mass, ms0. The phase transition is calculated taking into account the baryonic density dependence of the quark masses in dense baryonic medium.
Keywords: Cold dense stellar matter; Phase transition; Color superconductivity
The strange quark matter (SQM) is supposed to be the most stable quantum state of the hadronic matter ,. The SQM can be originated by a first-order hadron-quark phase transition occurring in the core of a massive star at the end of its evolutionary path when a gravitational collapse of the structure takes place. This hadron-quark phase transition leads to a deconfined quark gas at densities presumably near to 2-3 times the normal nuclear matter density. At sufficiently large baryon chemical potential, the more stable configuration of SQM is the color flavor locked (CFL) superconducting phase in which Cooper pairs of quarks of different flavors and colors are coupled with total zero momentum. For very high density, the mass of the strange quark is negligible compared to the baryonic chemical potential, leading to the same density of the three flavors of u, d and s quarks. Consequently, the CFL phase is naturally electrically neutral.
In the present work we study the phase transition between the SQM and CFL phases, determining the critical value of the baryonic chemical potential,µ, for different baryonic densities. A phenomenological model taking into account the dependence of the quark mass with the baryonic density is employed: the dynamical density quark mass DDQM model. The sensitivity of the calculated values for the critical chemical potential for the SQM-CFL phase transition is analyzed in respect to the parameter of DDQM model used. We also discuss some results obtained when the values of the color superconducting gap and the current strange quark mass are both changed.
II. THE DDQM MODEL IN THE SQM PHASE
According to the low-density regime of QCD, the quark masses are not merely originated from the explicit breaking of chiral symmetry. So, in the study of stability of quark matter, we can not neglect the dynamical mass induced by the strong quark interaction with the medium. For low and moderate density regime, we model the dynamical mass by the density dependent quark mass given by, 
where nB denotes the baryon density and C is a free parameter that in the zero density limit (nB ® 0) correspond to the constant energy density in the DDQM model. For null current masses of quarks u and d and for the current strange quark mass, ms0, we have
The DDQM model establish the effective quark mass values in pertubative and nonperturbative regime through the dependence with the dynamical mass MD. With this model two characteristic situations for quark matter (the confinement of quarks and asymptotic freedom regime)is reproduced when the corresponing densities regime is considered.
We consider the quark matter in stellar medium, that can be treated as a degenerate Fermi gas of u,d, s quarks and electrons with chemical equilibrium maintained by the weak interaction processes
If neutrinos freely scape from the medium, playing no role on the beta equilibrium conditions, the processes displayed above imply the following relation between the chemical potentials:
leaving only two independent chemical potentials for the thermodynamical description of the system.
When the temperature is small enough, the antiquarks are statistically negligible and the density of fermions in the absence of interactions may be approximated by
where, q = u, d, s. The same expression is valid for the electrons with a factor in the right hand side.
The electromagnetic charge neutrality and the baryonic density are
respectivelly. To solve the nonlinear system of Eqs. (5) and (6) we replace the quark densities nq by its corresponding expressions in terms of chemical potentials of (3).
The pressure of the SQM in the DDQM model aplying to the SQM case is given by the thermodynamic relation
where W is the thermodynamical potential of the system. Notice that the first term on the right hand side is necessary to make the pressure expression thermodynamically consistent with the energy density given by
with the quark density defined by
At T = 0,the expressions for the quarks pressure and energy density are
where xq = .
In the above equations the auxiliary functions F, G and H, are defined as
The contributions of free electrons to the thermodynamic potential is given by
From Eq.(10) we can see that there is a given value of baryonic density for which the pressure is null. At this density the null pressure can be interpreted as a consequence of the attractive internal interaction among the constituents of the system, simulated by the change of MD in the model. This null pressure situation represents the quark matter confinement. On other hand in Eq.(10), the increase of density leads to a pressure expression of a free fermionic gas, characterizing the asymptotic freedom.
III. THE CFL PHASE
In the CFL phase the Cooper pairs occup the same lowest energy quantum state at zero temperature, leading to a Bose condensate. In this configuration, the ground state of quark matter becomes a color superconductor, , . The main consequence of color superconductivity is the appearance of a nonzero energy gap in the one-particle energy, ei = , with D being the CFL superconducting gap.
The CFL phase is characterized by same density of quarks u, d and s, so the charge neutrality is automatically satisfied. The gap D can be calculated with perturbative QCD with quark-gluon exchange[ref.], but in this work we consider it like a free parameter whit characteristic values for the transition.
The pressure in the CFL reads
where the first term gives the pressure of free quarks, with equal number densities nu = nd = ns = (n3+2D2µ)/p2, where n is the common Fermi momentum, given by
n = 2m - ,
and µ = (µu+µd+µs)/3. The second term in Eq. (16) is the contribution from the formation of the condensate to the pressure.
IV. RESULTS AND CONCLUSIONS
We have applied the Gibbs conditions for construct the phase transition between the two phases described in the last section. The critical chemical potential is defined as the value for which the pressure of the pure SQM phase equals the pressure of the pure CFL phase. Besides the Gibbs conditions, the local (neutral) electromagnetic charge of each phase and the global baryonic charge conservation are simultaneously required. In Fig.(1) we can see the difference of pressures PSQM-PCFL as a function of the baryonic chemical potential, for a given value of the gap and current strange quark mass, ms0, showing the critical potential value.
The main result of this work consists in discuss the sensitivity of the critical chemical potential of the phase transition in the DDQM model parameter, C. In Fig.(2) we display the critical chemical potential as a function of the parameter C, for different values of the superconducting gap and ms0. The results show that the critical chemical potential is less sensitive to the model parameter C than the gap and the current strange quark mass. Consequently, it is very important to have a satisfactory values for these last two external parameters in order to obtain a more accurate discution for the SQM-CFL phase transition.
 A. R. Bodmer, Phys. Rev. D 4, 1601 (1971). [ Links ]
 E. Witten, Phys. Rev. D 30, 272 (1984). [ Links ]
 G.N. Fowler, S. Raha, and R.M. Weiner, Z. Phys. C 9, 271 (1981). [ Links ]
 O. G. Benvenuto and G. Lugones, Phys. Rev. D 51, 1989 (1995). [ Links ]
 J. A. Bowers and K. Rajagopal, Phys. Rev. D 66, 065002 (2002). [ Links ]
 K. Rajagopal and F. Wilczek, Phys. Rev. Lett. 86, 3492 (2001). [ Links ]
 M. Alford and S. Reddy, Phys. Rev. D 67, 074024 (2003). [ Links ]
Received on 29 September, 2006