# Black Hole Solution of Einstein-Born-Infeld-Yang-Mills Theory.

1. IntroductionWhen considering electromagnetic field as the matter source to construct black hole solution in Einstein gravity, one usually use the standard Maxwell's theory of U(1) gauge field. However, when the field is strong enough the linear Maxwell's theory becomes invalid; the nonlinearities of electromagnetic field should be introduced as the correct electrodynamics. In 1930s, Born and Infeld proposed nonlinear electrodynamics with the aim of obtaining a finite value of the self-energy of electron [1]. Fradkin and Tseytlin reproduced Born-In-feld (BI) action in the framework of string theory [2]. The D3-brane dynamics was also noticed to be governed by BI action [3]. Hoffmann first found a solution of Einstein gravity coupled to BI electromagnetic field [4], which is devoid of essential singularity at the origin. Many black hole solutions of Einstein-Born-Infeld (EBI) theory with or without a cosmological constant have been found [5-8]. Black hole solutions of Gauss-Bonnet and three-order Lovelock gravity coupled to BI electromagnetic field have also been found in [9,10].

Since the condition for no-hair theorem in asymptotic (A)dS spacetime is much relaxed, besides the usually used matter sources such as scalar and Maxwell fields, it is natural to couple Yang-Mills (YM) field to gravity and construct black hole solutions. However, the YM equations are so complicated that early attempts of searching for black hole solutions of Einstein-Yang-Mills (EYM) theory were performed numerically. The first analytic black hole solution was found by Yasskin applying Wu-Yang ansatz [11]. This kind of solutions have also been generalized to higher dimensions and higher derivative gravity [12, 13]. Regular nonminimal magnetic black hole solutions have been investigated recently in [14]. To our knowledge, black hole solutions of Einstein gravity coupled to both BI electromagnetic field and YM field have not been studied; in this paper, we want to construct blackhole solution of Einstein-Born-Infeld-Yang-Mills (EBIYM) gravity and study some properties of the black hole.

Among the properties of black holes, thermodynamical properties have gained much attention in the past several decades. Since the early work [15] studying thermal phase transition between Schwarzchild-AdS black hole and AdS vacuum, the behaviors of phase transition of black holes have been studied intensively. In [16,17], the thermodynamics of charged AdS black hole have been studied and found that there exist phase transitions between large/small black holes at the sacrifice of viewing the electric charge as intensive variable; the phase transition behavior resembles the one of van der Waals liquid-gas system. In order to solve the problem encountered in [16, 17], KubizMk et al. extended the phase space by identifying the cosmological constant as the pressure of the gravitational system [18, 19]; then the thermodynamic volume conjugate to pressure can be defined; in this framework the phase transitions between large/small black holes are founded too. Subsequently, the study was extended to various other kinds of blackholes [20-23]. In this paper, we will also explore the phase transitions of the black hole given below in extended phase space.

The paper is organized as follows. In Section 2, we present the black hole solution of four-dimensional Einstein-BIYM gravity and discuss its several degenerated forms. In Section 3, we calculate the thermodynamical quantities, check the first law of thermodynamics, and study the phase transitions of the black hole in extended phase space. Finally, some concluding remarks are given in Section 4.

2. Black Hole Solution of Einstein-BI-YM Theory

We intend to search for a four-dimensional black hole solution of EBIYM theory; the action of the theory is given by

j = [integral] [d.sup.4] x [square root of -g][R-2[LAMBDA]/16[pi]G + l(F) - Tr ([F.sup.(a).sub.[mu]v][F.sup.(a)[mu]v])], (1)

where G is the Newton constant; we take the convention 16[pi]G =1 in the following for convenience, Tr(*) means sum over the gauge group indices, and

LF = 4[[beta].sup.2] (1 - [square root of 1 + [F.sup.[mu]v][F.sup.[mu]v]/2[[beta].sup.2]). (2)

Here [beta] is the BI parameter with dimension of mass. In the limit [beta] [right arrow] 0, L(F) [right arrow] 0. In the limit [beta] [right arrow] [infinity], L(F) reduces to the stndard Maxwell form:

L(F) = -[F.sub.[mu]v] [F.sup.[mu]v] + O ([F.sup.4]). (3)

Take variation with respect to the metric, the Maxwell field [A.sub.[mu]], and the YM field [A.sup.(a).sub.[mu]] respectively, we have the equations of motion

[G.sub.[mu]v] + [[LAMBDA].sub.g[mu]v] + [T.sup.M.sub.[mu]v] + [T.sup.YM.sub.[mu]v], (4)

[[nabla].sub.[mu]]([F.sup.[mu]v]/[square root of 1+ [F.sub.p[sigma]][F.sup.[rho][sigma]]/2[[beta].sup.2]) = 0, (5)

[mathematical expression not reproducible], (6)

where [f.sup.(a).sub.(b)(c)] are the real structure constants of the gauge group and

[T.sup.EM].sub.[mu]v] = 1/2 [g.sub.[mu]v] L] (F) + 2[F.sub.[mu][rho]][F.sup.[rho].sub.v]/[square root of 1 + [F.sub.[rho][sigma]][F.sup.[rho][sigma]]/2[[beta].sup.2], (7)

[T.sup.YM.sub.[mu]v] = - 1/2 [g.sub.[mu]v]][F.sup.(a).sub.[rho][sigma]] [F.sup.(a)[rho][sigma]] + 2[F.sup.(a).sub.[mu][rho]] [F.sup.(a)[rho]].sub.v]. (7)

In order to find a static solution of the field equations, we take a general metric ansatz

[ds.sup.2] = -f (r) [dt.sup.2] + [dr.sup.2]/f(r) + [r.sup.2] d[[OMEGA].sup.2.sub.2], (8)

where d[[OMEGA].sup.2.sub.2] is the line element of 2-sphere. Before solving (4), we need to solve equations of motion of the matter fields (5) and (6) first. Under the electrostatic potential assumption, all other components of the strength tensor [F.sup.[mu]v] vanish except [F.sup.tr]; solving (5) one obtains

[F.sup.tr] = [beta]q/[square root of [[beta].sup.2][r.sup.4] + [q.sup.2]], (9)

where q is an integration constant. Note that unlike the field strength in Maxwell electrodynamics, the one in BI electrodynamics is finite at r = 0. To solve equations of motion of the YM field (6), we take the magnetic Wu-Yang ansatz of the gauge potential [14]. Since we want to find a black hole solution with global YM charge, the gauge group is supposed to be SU(2); then the real structure constants [f.sub.(a)(b)(c)] are the complete antisymmetric symbols [[epsilon].sub.(a)(b)(c)]. We use the position dependent generators [t.sub.(r)], [t.sub.([theta])], [t.sub.([phi])] of the gauge group; the relations between the generators [t.sub.(r)], [t.sub.([theta]),] [t.sub.([phi])] and the standard SU(2) generators are

[t.sub.(r)] = cos (v[phi]) sin [theta][t.sub.(1)] + sin (v[phi]) sin [theta][t.sub.(2)] + cos [theta][t.sub.(3)],

[t.sub.([theta])] = cos (v[phi]) cos [theta][t.sub.(1)] + sin (v[phi]) cos [theta][t.sub.(2)] - sin [theta][t.sub.(3)],

[t.sub.([phi])] = - sin ([v.sub.[phi]]) [t.sub.(1)] + cos (v[phi]) [t.sub.(2)], (10)

where v is a nonvanishing integer; as will become clear later, it relates to global YM charge. Using the commutation relations [[t.sub.(a)], [t.sub.(b)]] = [S.sub.(a)(b)(c)][t.sub.(c)], where a, b, and c take values from 1 to 3 and [[epsilon].sub.(1)(2)(3)] = 1, it is straightforward to check the following commutation relations:

[[t.sub.(r)], [T.sub.([theta])]] = [t.sub.([phi])],

[[t.sub.([theta])], [T.sub.([phi])]] = [t.sub.(r)],

[[t.sub.([phi])], [T.sub.(r)]] = [t.sub.([theta])], (11)

which are satisfied. The gauge field characterized by Wu-Yang ansatz is of the form

[mathematical expression not reproducible]. (12)

One can check that the equations of motion of YM field(6) are satisfied under the choice of gauge (12). Under the gauge (12), the only nonvanishing component of the YM field strength tensor is

[F.sub.[theta][phi]] = -v sin [theta][t.sub.(r)]. (13)

With the field strength tensors (9), (13), and the metric ansatz (8), one can work out the expression of energy momentum tensor straightforwardly. Substituting (7) and (8) into (4) and solving (4) we find the following new black hole solution:

[mathematical expression not reproducible]. (14)

Here [m.sub.0] is the mass parameter and [sub.2][F.sub.1] [1/2,1/4,5/4, -[q.sup.2]/[r.sup.4][[beta].sup.2]] is the Gaussian hypergeometric function. Before further analysis of solution (14), we discuss its several limiting forms. When the parameter v in (14) vanishes, the Einstein-BI black hole in (A)dS space is reproduced [8]. When [beta] [right arrow] [infinity], BI electrodynamics reduces to the standard Maxwell form; solution (14) reduces to

[f.sub.(r)] = 1 - [m.sub.0]/r - 1/3 [LAMBDA][r.sup.2] + [q.sup.2]/[r.sup.2] + [v.sup.2]/[r.sup.2], (15)

which is a new black hole with both electric charge and magnetic YM charge. When [beta] [right arrow] 0, the electric charge vanishes automatically; one obtains a magnetic black hole with only YM charge

f(r) = 1 - [m.sub.0]/r - 1/3 [LAMBDA][r.sup.2] + [v.sup.2]/[r.sup.2], (16)

which is of the same form as the 4-dimensional (A)dSReinssner-Nordstrom (RN) black hole. When v = 0 and [beta] [right arrow] [infinity], solution (14) degenerates to RN black hole in (A)dS space.

3. Thermodynamics

In this section, we will first calculate the thermodynamic quantities of the black hole obtained in the last section, then check the first law of thermodynamics, and finally extend the phase space to explore the phase transition behaviors of the black hole.

3.1. Calculations of Thermodynamical Quantities. Since the black hole (14) is asymptotic to (A)dS, in order to calculate the mass of the black hole, one should adopt the method proposed by Abbott and Deser [24], which gives

M = 8T[pi][m.sub.0]. (17)

Note that the area of unit 2-sphere [[omega].sub.2] = 4[pi] is used. In order to calculate the temperature, one should take the Euclidean continuation (t [right arrow] -i[tau]) and demand the absence of conical singularity at the horizon; the period of the Euclidean time r is the inverse of Hawking temperature 1/T; one obtains

T = 1/4[pi][r.sub.+](1 + 2[[beta].sup.2][r.sup.2.sub.+] - [LAMBDA][r.sup.2.sub.+] - [v.sup.2][r.sup.2.sub.+] - [v.sup.2]/[r.sup.2.sub.+] - 2[beta] [square root of [q.sup.2] + [r.sup.4.sub.+][[beta].sup.2]]), (18)

where [r.sub.+] is the radius of the outmost horizon of the black hole. In model (1) we considered that entropy of the black hole (14) obeys the area law, which is

S = 16[[pi].sup.2][r.sup.2.sub.+]; (19)

note that the convention 16[pi]G =1 is adopted. The electric charge is defined as

[Q.sub.e] = 1/4[pi] [integral] * fd[[OMEGA].sup.2] = q (20)

where * F represents Hodge dual of the strength tensor and the integration is performed on the t = const and r [right arrow] [infinity] hypersurface. The electrostatic potential [PHI], measured at infinity with respect to the horizon, is defined as

[mathematical expression not reproducible]. (21)

Our calculation gives [PHI] = (q/[r.sup.+]) [sub.2][F.sub.1][1/2,1/4, 5/4, - [q.sup.2]/[r.sup.4.sub.+][[beta].sup.2]]. Since the gauge group is SU(2), we can define a global YM charge, for which we take the definition [25-27]

[Q.sub.YM] = 1/4[pi] = [integral][square root of [F.sup.(a).sub.[theta][phi]] [F.sup.(a).sub.[theta]] [phi]]d[theta]d[phi]. (22)

Just as the definition of electric charge, the integration in (22) is performed on t = const and r [right arrow] [infinity] hypersurface too. Our calculation gives

[Q.sup.YM] = -v. (23)

In order to preserve the YM charge being positive, v is taken to be negative. Now with all the thermodynamic quantities above in hand, one can check that the first law of thermodynamics

dM = JdS + [PHI]d[Q.sub.e] + Ud[Q.sub.YM] (24)

is satisfied, where U defined by [mathematical expression not reproducible] is the thermodynamic potential conjugate to the YM charge [Q.sub.YM].

3.2. Phase Transition in Extended Phase Space. In extended phase space, cosmological constant is identified as pressure of the gravitational system:

P = - [LAMBDA]/8[pi]. (25)

There are some reasons to do so. First, one can suppose there exist more fundamental theories, where the cosmological constant arises as vacuum expectation value. Second, the Smarr relation becomes inconsistent with the first law of thermodynamics unless the variation of [LAMBDA] is included [18]. Now the mass of the black hole is viewed as enthalpy H [equivalent to] M rather than internal energy of the system [28]; then the Gibbs free energy of the system is G = H - TS. If the BI parameter [beta] is viewed as a free thermodynamic variable too, one can check the first law of thermodynamics in extended phase space

dH = JdS + [PHI]d[Q.sub.e] + Ud[Q.sub.YM] + VdF + Bd[beta] (26)

is satisfied, where

[mathematical expression not reproducible] (27)

is the thermodynamic volume conjugate to the pressure, and

[mathematical expression not reproducible] (28)

is the thermodynamic quantity conjugate to [beta]

Before studying the phase transitions of the black hole (14) for a general let us first discuss two limiting cases [beta] [right arrow] 0 and [beta] [infinity]. When [beta] [right arrow] 0, in terms of the temperature and horizon radius, the pressure of the system can be written as

P = T/2[r.sub.+] - 1/8[pi][r.sup.2.sub.+] + [Q.sup.2.sub.YM]/8[pi][r.sup.4.sub.+]. (24)

The critical points of the thermal phase transition are determined by the following critical equations:

[mathematical expression not reproducible]. (30)

The critical equations (30) can be solved analytically, which gives the critical horizon radius

[r.sub.c] = [square root of 6] [Q.sub.YM] (31)

and the critical temperature

[T.sub.c] = 1/3[square root of 6][pi][Q.sub.YM]. (32)

It is easy to see that the critical horizon radius and temperature and consequently the critical pressure are solely determined by the YM charge. This is because, as previously mentioned, when [beta] [right arrow] 0, the electric charge vanishes automatically and the black hole carries only YM charge as shown in (16).

When [beta] [right arrow] [infinity], this case corresponds to the black hole described by the metric (8) with f(r) given in (15). The pressure of the system is given by

P = T/2[r.sub.+] - 1/8[pi][r.sup.2.sub.+] + [Q.sup.2.sub.e] + [Q.sup.2.sub.YM]/8[pi][r.sup.4.sub.+]. (33)

Solving the critical equations (30), we obtain the critical horizon radius

[r.sup.c] = [square root of 6 ([Q.sup.2.sub.e] + [Q.sup.2.sub.YM]) (34)

and the critical temperature

[T.sub.C] = 1/2[pi][summation][square root of 6([Q.sup.2.sub.e] + [Q.sup.2.sub.YM])]. (35)

The critical horizon radius, temperature, and pressure are determined by both electric and YM charge. Now, for the black hole (15) by taking proper values of the related parameters we can plot the isobars as displayed in Figure 1. On T-[r.sub.+] plot of Figure 1, the dotted line is the isobar of P > [P.sup.c]; in this case there is only a single phase which is in analogy to the thermal behavior of "ideal gas." The dashed line is the isobar of P = [P.sub.c]. The solid line is the isobar of P < [P.sup.c]; one can see that there are two branches of black holes whose temperatures increase with the increase of horizon radius; one branch is in small radius region and the other one is in large radius region. Between the two branches, there is a region whose temperature decreases with the increase of horizon radius, which means the thermal expansion coefficient is negative; this region corresponds to an unstable phase. For appropriate value of temperature, two horizon radii are permitted; thus large/small black holes phase transition occurs. This kind of thermal behavior resembles the one of van der Waals gas/liquid system. The phase transition can also be seen in G-T plot, where "swallow tail" appears when P < [P.sup.c], just as the solid line shows us. The dashed line on G-T plot is the isobar of P = [P.sup.c], and the dotted line corresponding to P > [P.sub.c] describes "ideal gas" phase.

Now, let us consider phase transition of the blackhole (14) for a general value of [beta]. For general [beta], the pressure of the system is

[mathematical expression not reproducible]. (36)

In this case, the critical equations (30) are too complicated to be solved analytically, we solve them numerically, the results are collected in Table 1. From the data in the table, one learns that, with the increase of [beta] or [Q.sub.YM], [T.sub.c] and [P.sub.c] decrease while [r.sub.c] and the ratio [P.sub.c][r.sup.c]/[T.sub.c] increase. Figure 2 gives the isobaric plots near the critical point of [P.sub.c]] = 0.0006631 and Figure 3 displays the effects of YM charge and BI parameter on the critical pressures. On T-[r.sub.+] plot of Figure 2, just as the case of [beta] [right arrow] [infinity], P > [P.sub.c] isobar describes the "ideal gas" phase. The isobar of P < [P.sub.c] shows that the "large black hole" region and "small black hole" region are thermodynamical stable while the medium region is thermodynamical unstable, which indicates the existence of phase transition. On G-T plot of Figure 2, the isobars show that when P < [P.sub.c] phase transition characterized by the "swallow tail" occurs. On Figure 3(b) one can see that, although corresponding to different orders of magnitude of [beta] the dotted line ([beta] = 1) and the dashed line ([beta] = 10) are almost coincident, and the deviation of the solid line ([beta] = 0.1) from the dotted or dashed one is small; it seems that the influence of the values of [beta] to critical pressure is not that large just as the authors found in [23]. This may be attributed to the parameter region we choose.

4. Conclusion

In this paper, we construct a black hole solution of Einstein gravity coupled to BI electromagnetic field and SU(2) YM field. When the parameter v =0, one reproduces the Einstein BI balck hole in (A)dS space. When the BI parameter [beta] [right arrow] [infinity], the solution degenerates to a new black hole with electrostatic charge and magnetic YM charge. When [beta] [infinity] 0, the solution reduces to a black hole with only YM charge. When the parameters v = 0 and [beta] [right arrow] [infinity], one obtains the (A)dS-RN black hole. We calculate the thermodynamical quantities such as mass, temperature, entropy, electric charge, and YM charge and check that the fist law of thermodynamics is satisfied.

We study the phase transition behaviors of the black hole in extended phase space by identifying the cosmological constant as pressure of the system. The critical equations can be solved analytically when taking [beta] [right arrow] [infinity] limit while they have to be solved numerically for general [beta]. After plotting the isobars one sees that when above the critical pressure there is only an "ideal gas" phase, when below the critical pressure, there are two stable regions corresponding, respectively, to large/small black hole phases with an unstable medium region, which implies the existence of the large/small black hole phase transition; this thermal behavior of black hole is in analogy to the one of van der Waals gas. The effects of [beta] and [Q.sub.YM] on critical pressures are also considered and displayed in the isobaric plots.

http://dx.doi.org/10.1155/2017/2038202

Competing Interests

The authors declare that they have no competing interests.

Acknowledgments

This work is supported by the National Natural Science Foundation of China (NSFC) under Grants nos. 11447153 (for Kun Meng) and 11447196 (for Da-Bao Yang).

References

[1] M. Born and L. Infeld, "Foundations of the new field theory," Proceedings of the Royal Society A: Mathematical, Physical and Engineering Sciences, vol. 144, no. 852, pp. 425-451, 1934.

[2] E. S. Fradkin and A. A. Tseytlin, "Non-linear electrodynamics from quantized strings," Physics Letters. B, vol. 163, no. 1-4, pp. 123-130, 1985.

[3] A. A. Tseytlin, "Vector field effective action in the open superstring theory," Nuclear Physics. B, vol. 276, no. 2, pp. 391-428, 1986.

[4] B. Hoffmann, "Gravitational and electromagnetic mass in the born-infeld electrodynamics," Physical Review, vol. 47, no. 11, pp. 877-880, 1935.

[5] H. P. de Oliveira, "Non-linear charged blackholes," Classical and Quantum Gravity, vol. 11, no. 6, pp. 1469-1482, 1994.

[6] S. Fernando and D. Krug, "Charged black hole solutions in Einstein-Born-Infeld gravity with a cosmological constant," General Relativity and Gravitation, vol. 35, no. 1, pp. 129-137, 2003.

[7] T. Kumar Dey, "Born-Infeld black holes in the presence of a cosmological constant," Physics Letters B, vol. 595, no. 1-4, pp. 484-490, 2004.

[8] R.-G. Cai, D.-W. Pang, and A. Wang, "Born-Infeld black holes in (A)dS spaces," Physical Review. D. Third Series, vol. 70, no. 12, article 124034, Article ID 124034, 2004.

[9] D. L. Wiltshire, "Spherically symmetric solutions of Einstein-Maxwell theory with a Gauss-Bonnet term," Physics Letters. B, vol. 169, no. 1, pp. 36-40, 1986.

[10] M. H. Dehghani, N. Alinejadi, and S. H. Hendi, "Topological black holes in Lovelock-Born-Infeld gravity," Physical Review D. Particles, Fields, Gravitation, and Cosmology, vol. 77, no. 10, Article ID 104025, 2008.

[11] P. B. Yasskin, "Solutions for gravity coupled to massless gauge fields," Physical Review D, vol. 12, no. 8, pp. 2212-2217, 1975.

[12] S. H. Mazharimousavi and M. Halilsoy, "5D black hole solution in Einstein-Yang-Mills-Gauss-Bonnet theory," Physical Review D, vol. 76, no. 8, Article ID 087501, 2007.

[13] S. H. Mazharimousavi and M. Halilsoy, "Black hole solutions in Einstein-Maxwell-Yang-Mills-Gauss-Bonnet theory," Journal of Cosmology and Astroparticle Physics, vol. 2008, no. 12, 2008.

[14] A. B. Balakin, J. P. Lemos, and A. E. Zayats, "Regular non-minimal magnetic black holes in spacetimes with a cosmological constant," Physical Review D, vol. 93, no. 2, Article ID 024008, 2016.

[15] S. W. Hawking and D. N. Page, "Thermodynamics of-black-holes in anti-de Sitter space," Communications in Mathematical Physics, vol. 87, no. 4, pp. 577-588, 1983.

[16] A. Chamblin, R. Emparan, C. V. Johnson, and R. C. Myers, "Charged AdS black holes and catastrophic holography," Physical Review. D. Third Series, vol. 60, no. 6, article 064018, 1999.

[17] A. Chamblin, R. Emparan, C. V. Johnson, and R. C. Myers, "Holography, thermodynamics, and fluctuations of charged AdS black holes," Physical Review D, vol. 60, no. 10, Article ID 104026, 1999.

[18] D. Kubiznak and R. B. Mann, "P-V criticality of charged AdS black holes," JHEP, vol. 2012, article 33, 2033.

[19] S. Gunasekaran, D. Kubiznak, and R. B. Mann, "Extended phase space thermodynamics for charged and rotating black holes and Born-Infeld vacuum polarization," Journal of High Energy Physics, vol. 2012, no. 11, article 110, 2012.

[20] R.-G. Cai, L.-M. Cao, L. Li, and R.-Q. Yang, "P-V criticality in the extended phase space of Gauss-Bonnet black holes in AdS space," Journal of High Energy Physics, vol. 2013, no. 9, article 005, 2013.

[21] W. Xu, H. Xu, and L. Zhao, "Gauss-Bonnet coupling constant as a free thermodynamical variable and the associated criticality," European Physical Journal C, vol. 74, article 2970, 2014.

[22] H. Xu, W. Xu, and L. Zhao, "Extended phase space thermodynamics for third order Lovelock black holes in diverse dimensions," The European Physical Journal C, vol. 74, article 3074, 2014.

[23] J.-X. Mo andW.-B. Liu, "P-V criticality of topological black holes in Lovelock-BornInfeld gravity," The European Physical Journal C, vol. 74, p. 2836, 2014.

[24] L. E Abbott and S. Deser, "Stability of gravity with a cosmological constant," Nuclear Physics, Section B, vol. 195, no. 1, pp. 76-96, 1982.

[25] A. Corichi, U. Nucamendi, and D. Sudarsky, "Emstem-Yang-Mills isolated horizons: phase space, mechanics, hair, and conjectures," Physical Review D, vol. 62, no. 4, Article ID 044046, 2000.

[26] B. Kleihaus, J. Kunz, and E Navarro-Larida, "Rotating Emstem-Yang-Mills black holes," Physical Review. D. Third Series, vol. 66, no. 10-15, 2002.

[27] Z.-Y. Fan and H. Lu, "SU(2)-colored (A)dS black holes in conformal gravity," Journal of High Energy Physics, vol. 2015, no. 2, article 013, 2015.

[28] D. Kastor, S. Ray, and J. Traschen, "Enthalpy and the mechanics of AdS black holes," Classical and Quantum Gravity, vol. 26, no. 19, Article ID 195011, 16 pages, 2009.

Kun Meng, Da-Bao Yang, and Zhan-Ning Hu

School of Science, Tianjin Polytechnic University, Tianjin 300387, China

Correspondence should be addressed to Kun Meng; mengkun@tjpu.edu.cn

Received 22 October 2016; Accepted 19 December 2016; Published 31 January 2017

Academic Editor: George Siopsis

Caption: FIGURE 1: Isobaric plots for [Q.sub.YM] = 2, [Q.sub.e] = 1. The isobars on T - [r.sub.+]s plot correspond one- to-one with the G-T plot. On both (a) and (b), from top to bottom, the pressures are, respectively, P = 1.2[P.sub.c] (dotted), P = [P.sub.c] (dashed), and P = 0.8[P.sub.c] (solid).

Caption: FIGURE 2: Isobaric plots for [Q.sub.YM] =2, [Q.sub.e] = 1, and [beta] = 10. The isobars on T - [r.sub.+] plot and G-T plot are in one-to-one correspondence with each other. On both (a) and (b), from top to bottom, the pressures are, respectively, P = 1.2 [P.sub.c] (dotted), P = [P.sub.c] (dashed), and P = 0.8 [P.sub.c] (solid).

Caption: FIGURE 3: Isobaric plots that reflect the effects of YM charge (a) and BI parameter (b). On (a), the parameters of all the isobars are taken as [Q.sub.e] = 1,[beta] = 10, and P = 0.7 [P.sub.c] ; the difference is that the solid, dashed, and dotted lines correspond to [Q.sub.YM] = 1,2,3, respectively. On (b), the parameters of all the isobars are taken as [Q.sub.e] = 1, [Q.sub.YM] = 2, and P = 0.7 [P.sub.c]; the solid, dotted, and dashed lines correspond to [beta] = 0.1,1,10, respectively.

TABLE 1: Critical values for [Q.sub.e] = 1. [beta] [Q.sub.YM] [r.sub.c] [T.sub.c] 10 3 7.7459654 0.0136979 10 2 5.4772185 0.0193717 10 1 3.4640315 0.0306296 1 2 5.4765161 0.0193728 0.1 2 5.4113483 0.0194752 [beta] [P.sub.c] [P.sub.c][r.sub.c]/[T.sub.c] 10 0.0003316 0.1875150 10 0.0006631 0.1875024 10 0.0016579 0.1874989 1 0.0006632 0.1874807 0.1 0.0006714 0.1865541

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Title Annotation: | Research Article |
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Author: | Meng, Kun; Yang, Da-Bao; Hu, Zhan-Ning |

Publication: | Advances in High Energy Physics |

Date: | Jan 1, 2017 |

Words: | 4544 |

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