Hadron-Quark Phase Transition in Quark-Hybrid Stars

Gustavo A. Contrera ^{1}^{1}1Home address: IFLP, CONICET - Dpto. de Física, UNLP, La Plata, Argentina;

Gravitation, Astrophysics and Cosmology Group, Facultad de Ciencias Astronómicas y Geofísicas,

Paseo del Bosque S/N (1900), Universidad Nacional de La Plata UNLP, La Plata, Argentina

Department of Physics, San Diego State
University, San Diego, CA 92182, USA

Email: guscontrera@gmail.com

William Spinella

Computational Science Research Center & Department of Physics, San Diego State University, San Diego, CA 92182, USA

Email: spinella@rohan.sdsu.edu

Milva Orsaria

CONICET, Rivadavia 1917, 1033 Buenos Aires, Argentina; Gravitation, Astrophysics and Cosmology Group, Facultad de Ciencias Astronómicas y Geofísicas, Paseo del Bosque S/N (1900), Universidad Nacional de La Plata UNLP, La Plata, Argentina

Email: morsaria@fcaglp.unlp.edu.ar

Fridolin Weber

Department of Physics, San Diego State
University, San Diego, California 92182, USA & Center for
Astrophysics and Space Sciences, University of California, San Diego,
La Jolla, California 92093, USA

Email: fweber@mail.sdsu.edu

## 1 Introduction

The recent discovery of the two-solar mass neutron stars () [1] and () [2] allows us to consider the possible existence of deconfined quarks in the cores of neutron stars [3, 4]. Nevertheless if the dense interior of a neutron star is indeed converted to quark matter, it must be three-flavor quark matter since it has lower energy than two-flavor quark matter. And just as for the hyperon content of neutron stars, strangeness is not conserved on macroscopic time scales, which allows neutron stars to convert confined hadronic matter to three-flavor quark matter until equilibrium brings this process to a halt. As first realized by Glendenning [5], the presence of quark matter in neutron stars enables the hadronic regions of the mixed phase to become more isospin symmetric than in the pure phase by transferring electric charge to the quark phase. The symmetry energy can be lowered thereby at only a small cost in rearranging the quark Fermi surfaces. The stellar implication of this charge rearrangement is that the mixed phase region of a neutron star will have positively charged regions of nuclear matter and negatively charged regions of quark matter [5]. This should have important implications for the electric and thermal properties of neutron stars. First studies of the transport properties of quark-hybrid neutron star matter have been reported in [6, 7].

It has been shown [8, 9, 10, 11] that the appearance of a mixed phase of quarks and hadrons in NSs depends on the surface tension between nuclear and quark matter, which should be around MeV/fm. Although recent studies about the nucleation process during the phase transition predict the value of the surface tension, their results vary and are strongly model dependent [12, 13, 14, 15, 16]. Thus, the discussion concerning the appearance of a mixed phase in NSs remains open.

Our study is based on NSs containing deconfined quark matter, i.e. quark-hybrid stars (QHSs). To describe the quark matter phase, we use a non-local extension of the SU(3) Nambu Jona-Lasinio (NJL) model with vector interactions, whereas to represent the hadronic phase we consider a non-linear Walecka model using parametrization NL3 [17]. A phase transition between these two phases can be constructed via the Gibbs conditions, imposing global electric charge neutrality and baryon number conservation. We find that the non-local NJL model predicts the existence of extended regions of mixed quark-hadron (quark-hybrid) matter in high-mass neutron stars with masses of 2.0 to .

## 2 Modeling of the Mixed Phase

To determine the mixed phase region of quarks and hadrons, we start from the Gibbs condition for pressure equilibrium between confined hadronic () matter and deconfined quark () matter. The Gibbs condition is given by [5]

(1) |

with for the baryon chemical potentials and for the electron chemical potentials in the hadronic () and quark () phase, respectively. By definition, the quark chemical potential is given by , where is the chemical potential of the neutron. The quantities and in Eq. (1) stand collectively for the field variables and Fermi momenta that characterize the solutions to the equations of confined hadronic matter and deconfined quark matter, respectively. In the mixed phase, the baryon number density, , and the energy density, , are given by [5]

(2) |

and

(3) |

where () and () denote the baryon number (energy) densities of the hadron and quark phase, respectively. The quantity denotes the volume proportion of quark matter, , in the unknown volume . By definition varies between 0 and 1 depending on how much confined hadronic matter has been converted to quark matter [5]. In addition to the Gibbs condition (1) for pressure, the conditions of global baryon number conservation and global electric charge neutrality need to be imposed on the field equations.

(4) |

where and denote the baryon number densities of the quark phase and hadronic phase, respectively. The condition of global electric charge neutrality is given by

(5) |

where is the electric charge of the -th specie in units of the electron charge.

For the quark sector, within the non-local NJL model, the mean-field thermodynamic potential at zero temperature is [4]

(6) | |||

where , , and . The constituent quark masses are treated as momentum-dependent quantities and are given by

(7) |

where is the form factor, which we take to be Gaussian .

The inclusion of vector interactions shifts the quark chemical potential as

(8) |

where represents the vector mean fields related to the vector current interaction. The inclusion of the form factor in Eq. (8) is a particular feature of the non-local model, which renders the shifted chemical potential momentum dependent. Accordingly, the four momenta in the dressed part of the thermodynamic potential are modified as

(9) |

Note that the quark chemical potential shift does not affect the non-local form factor , as discussed in [18, 19, 20], avoiding a recursive problem. In this work we use for the NJL model the parameters listed in Refs. [3, 4].

Within the stationary phase approximation, the mean-field values of the auxiliary fields turn out to be related to the mean-field values of the scalar fields [21]. They are given by

(10) |

Due to the charge neutrality constraint, for the quark phase we consider the three mean-field flavors , and , which can be obtained by solving the “gap” equations given by [21]

(11) | |||||

and are obtained via minimizing the thermodynamic potential, .

## 3 Results and Conclusions

Depending on the strength of quark vector repulsion, we find that an extended region made of a mixed phase of quarks and hadrons may exist in high-mass neutron stars with masses up to as can be seen in Fig 1. The radii of these objects are between 12 and 13 km, as expected for neutron stars. Table 1 lists the strength of the vector interaction, the maximum mass stars, the corresponding fraction of quark matter, and the range of the mixed phase.

() | at | Mixed phase () | |
---|---|---|---|

For the non-local NJL model and the NL3 parametrization for the hadronic phase, we find that pure quark matter could not exist in stable neutron stars. Only neutron stars that lie on the left of the mass peak are dense enough to contain quark matter. However, these stars are unstable against radial oscillations and thus could not exist stably in the universe. According to what is shown on Fig. 2, with increasing stellar mass, all the stellar cores are composed of either nucleons, nucleons and hyperons, or a mixed phase of nucleons, hyperons, and quark matter.

## Acknowledgments

G.C. and M.O. thank CONICET (Argentina) for financial support and are thankful for hospitality extended to them at the San Diego State University, where much of this work was performed. F.W. acknowledges supported by the National Science Foundation (USA) under Grant PHY-0854699. This work has been partially supported by a CONICET-NSF joint project.

## References

- [1] P. B. Demorest, T. Pennucci, S. M. Ranson, M. S. E. Roberts and J. W. T. Hessels, Nature 467, 1081 (2010).
- [2] Lynch et al. Astrophys. J 763, 81 (2013); J. Antoniadis et al., Science 340, no. 6131 (2013).
- [3] M. Orsaria, H. Rodrigues, F. Weber and G. A. Contrera, Phys. Rev. D 87, 023001 (2013).
- [4] M. Orsaria, H. Rodrigues, F. Weber and G. A. Contrera, Phys. Rev. C 89, 015806 (2014).
- [5] N. K. Glendenning, Compact Stars, Nuclear Physics, Particle Physics, and General Relativity, 2nd ed. (Springer-Verlag, New York, 2000); N. K. Glendenning, Phys. Rev. D 46, 1274 (1992); N. K. Glendenning, Phys. Rep. 342, 393 (2001).
- [6] S. Reddy, G. Bertsch and M. Prakash, Phys. Lett. B 475, 1 (2000).
- [7] X. Na, R. Xu, F. Weber and R. Negreiros, Phys. Rev. D 86, 123016 (2012).
- [8] M. G. Alford, K. Rajagopal, S. Reddy and F. Wilczek, Phys. Rev. D 64, 074017 (2001).
- [9] D. N. Voskresensky, M. Yasuhira and T. Tatsumi, Nucl. Phys. A 723, 291 (2003).
- [10] T. Tatsumi, M. Yasuhira and D. N. Voskresensky, Nucl. Phys. A 718, 359 (2003).
- [11] T. Endo, Phys. Rev. C 83, 068801 (2011); T. Endo, arXiv:1310.0913 [astro-ph.HE].
- [12] L. F. Palhares and E. S. Fraga, Phys. Rev. D 82, 125018 (2010).
- [13] M. B. Pinto, V. Koch and J. Randrup, Phys. Rev. C 86, 025203 (2012).
- [14] W. Ke and Y. Liu, arXiv:1312.2295 [hep-ph].
- [15] T. A. S. d. Carmo, G. Lugones and A. G. Grunfeld, J. Phys. G 40, 035201 (2013).
- [16] G. Lugones, A. G. Grunfeld and M. Al Ajmi, Phys. Rev. C 88, 045803 (2013).
- [17] G. A. Lalazissis, J. Konig and P. Ring, Phys. Rev. C 55, 540 (1997).
- [18] D. B. Blaschke, D. Gomez Dumm, A. G. Grunfeld, T. Klähn, and N. N. Scoccola, Phys. Rev. C 75, 065804 (2007).
- [19] K. Kashiwa, T. Hell, and W. Weise, Phys. Rev. D 84, 056010 (2011).
- [20] G. A. Contrera, A. G. Grunfeld, and D. B. Blaschke, arXiv:1207.4890 [hep-ph].
- [21] A. Scarpettini, D. Gomez Dumm, and N. N. Scoccola, Phys. Rev. D 69, 114018 (2004).