Zhong-Wen Feng^,1, Xia Zhou¹, Guansheng He², Shi-Qi Zhou¹, Shu-Zheng Yang¹¹Physics and Space Science College, China West Normal University, Nanchong, 637009, China
²School of Mathematics and Physics, University of South China, Hengyang, 421001, China

Received:2021-01-3Revised:2021-02-26Accepted:2021-03-9Online:2021-04-09


Abstract
In this paper, the Joule-Thomson expansion of the higher dimensional nonlinearly anti-de Sitter (AdS) black hole with power Maxwell invariant source is investigated. The results show the Joule-Thomson coefficient has a zero point and a divergent point, which coincide with the inversion temperature T_i and the zero point of the Hawking temperature, respectively. The inversion temperature increases monotonously with inversion pressure. For the high-pressure region, the inversion temperature decreases with the dimensionality D and the nonlinearity parameter s, whereas it increases with the charge Q. However, T_i for the low-pressure region increase with D and s, while it decreases with Q. The ratio $\eta$_BH between the minimum inversion temperature and the critical temperature does not depend on Q, it recovers the higher dimensional Reissner-Nördstrom AdS black hole case when s = 1. However, for s > 1, it becomes smaller and smaller as D increases and approaches a constant when D → ∞ . Finally, we found that an increase of mass M and s, or reducing the charge Q and D can enhance the isenthalpic curve, and the effect of s on the isenthalpic curve is much greater than other parameters.
Keywords： Joule-Thomson expansion;Maxwell invariant source;higher dimensional nonlinearly AdS black hole


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Zhong-Wen Feng, Xia Zhou, Guansheng He, Shi-Qi Zhou, Shu-Zheng Yang. Joule-Thomson expansion of higher dimensional nonlinearly AdS black hole with power Maxwell invariant source. Communications in Theoretical Physics, 2021, 73(6): 065401- doi:10.1088/1572-9494/abecd9

1. Introduction

By introducing the quantum mechanism into general relativity, Hawking and Bekenstein demonstrated that black holes have temperature and entropy [1-3]. After that, researchers have established the complete theories of black hole thermodynamics. According to those theories, the thermodynamic properties of a variety of complicated black holes were explored in the past few decades [4-11]. Among all, the anti-de Sitter (AdS) black holes have attracted people’s attention for their strange thermodynamic properties. Hawking and Page first pointed out the existence of a thermodynamic phase transition in Schwarzschild-AdS spacetime [12]. This heuristic work shows the deeper-seated relation between confinement and deconfinement phase transition of the gauge field in the AdS/CFT correspondence. Within this context, a series of works have been done to investigate the common properties between AdS spacetimes and the general thermodynamic system. In [13, 14], Chamblin et al proposed that the phase structures of Reissner-Nördstrom (R-N) AdS black hole are similar to that of the Van der Waals system. Furthermore, by interpreting the cosmological constant Λ and mass M as the thermodynamic pressure P and chemical enthalpy H, receptively [15-17], the implications of black hole thermodynamics have been investigated in many contexts. In the extended phase space, Kubizňák and Mann calculated the P-V critical behavior of R-N AdS black hole and demonstrate that they also coincide with those of the Van der Waals fluid [18]. In [19], Johnson showed the AdS black holes can be considered as holographic heat engines, which outputs work from a pressure-volume space. Besides, Dolan found that the black hole with the non-positive cosmological constant has no adiabatic compressibility [20, 21].

There is no doubt now that the studying of the black holes'van der Waals behavior is so important since it connects the gravity with the ordinary thermodynamical system. Recently, the black hole thermodynamics have been extended to the regime of Joule-Thomson expansion [22, 23]. In the van der Waals system, the Joule-Thomson expansion occurs when the gas from the high-pressure zone through the porous plug into the low-pressure zone. Meanwhile, the enthalpy remains the same in this process and can be used to define the non-equilibrium states of expansion. Based on the viewpoints of [16, 24, 25], Ökcü and Aydmer investigated the Joule-Thomson expansion of R-N AdS black hole for the first time. Their result shows that R-N AdS black hole has a similar Joule-Thomson expansion process with the van der Waals fluid [26]. Subsequently, the Joule-Thomson expansion of Kerr AdS black hole, D-dimensional R-N AdS spacetime, charged Gauss-Bonnet black hole, Bardeen-AdS black hole, Hayward-AdS et al were studied in [27-35, 43].

By analyzing previous works, one finds that the in-depth analysis of Joule-Thomson expansion of higher-dimensional black holes in the complex gravity is still missing. To our knowledge, the reasons for this lie in two main aspects, one is the Joule-Thomson expansion behavior of AdS black holes are closely related to their properties of spacetimes. The change of any parameter of spacetimes would make the calculations more complicated, and even unable to obtain accurate results. Moreover, the van der Waals behavior is not valid for every AdS spacetimes [37, 38], which may leads to the absence of Joule-Thomson expansion. Despite the difficulties, it beneficial to investigate how the dimension of spacetimes and the complex gravity affect the Joule-Thomson expansion behavior since those works help people more understand the properties of black holes.

In recent years, an interest in the subject of the higher dimensional nonlinearly black hole has been growing. It is well known that, on the one hand, the black holes in the higher dimension have more physical information, which can be detected by the Large Hadron Collider and Advanced LIGO’s detection of gravitational waves [39-42]. Besides, many unified theories show that the coupling characteristics between the gravity field and the gauge field can be obtained in higher dimensions. Hence, it is believed that the related researches open a new window into gravity and quantum gravity. On the other hand, many charge AdS black holes are derived from the Einstein-Maxwell-AdS theory. However, the classical Maxwell theory has some defects, such as the central singularity of the point-like charges, vacuum polarization in quantum electrodynamics et al, those leads to the linear electrodynamics fail when the electromagnetic field is too strong. To crackdown on those problems, Born and Infeld introduced the non-linear electrodynamics (NLEDs) by eliminating the infinite self-energy. Furthermore, for generalizing NLEDs into higher dimensions and keeping the conformal symmetry of Maxwell action, one proposed the power Maxwell invariant (PMI) theory, which is an improved NLEDs model [36, 44]. As an improved NLEDs model, the Lagrangian density of PMI field can be expressed as ${L}_{\mathrm{PMI}}={\left(-F\right)}^{s}={\left(-{F}_{\mu \nu }{F}^{\mu \nu }\right)}^{s}$ with an arbitrary rational number s. It causes the properties of PMI field are more abundant than the Maxwell field. By introducing the PMI source into the astrophysical frameworks, many new results are obtained [46-49]. Moreover, the source turns out to be important in the studying on the strongly coupled dual gauge theory [49]. Recently, the black hole solutions Einstein gravity coupled to the PMI theory have attracted people’s attention since they believe the non-linear properties of the fundamental theory can be found in those spacetimes. In [50-52], the thermodynamic properties of those black holes have been analyzed in detail. In particular, in the extended phase space, the phase structure and the critical behavior of higher dimensional nonlinearly AdS black hole with PMI source are similar to those of Van der Waals fluid [53]. Due to the above discussion, it is believed that the higher dimensional nonlinearly AdS black hole with PMI source has the Joule-Thomson expansion process. Therefore, we calculate Joule-Thomson coefficient, the equation of the inversion curve and the equation of the isenthalpic curves in this paper. Meanwhile, we also use the numerical method to analyze the influence of dimensionality D, and the nonlinearity parameter s on the Joule-Thomson expansion.

The rest of the paper is organized as follows. In the next section, we review the metric of nonlinearly AdS black hole and its thermodynamic properties. Section 3 is devoted to deriving the Joule-Thomson coefficient, the ratio between the minimum of inversion temperature and the critical temperature, the equation of the inversion curve, and the equation of the isenthalpic curve. Then, we investigate the influence of various parameters (especially the dimensionality and the nonlinearity parameter) of the black hole on Joule-Thomson expansion via the numerical method. The conclusion and discussion are contained in section 4. This research takes the units G = c = k_B = 1.

2. The higher dimensional nonlinearly charged black hole with PMI source

2.1. The metric of higher dimensional nonlinearly AdS black hole with PMI source

To begin with, it is necessary to review the metric and the thermodynamic properties of nonlinearly AdS black hole with PMI source. In the D-dimensional (D ≥ 4) AdS spacetimes, the bulk action of Einstein-PMI gravity can be written in the form [43, 44]:
(1)$\begin{eqnarray}I=-\displaystyle \frac{1}{16\pi }\int {{\rm{d}}}^{D}x\sqrt{-g}\left[R-2{\rm{\Lambda }}+{\left(-{F}_{\mu \nu }{F}^{\mu \nu }\right)}^{s}\right],\end{eqnarray}$
where R is the Ricci scalar, ${\rm{\Lambda }}=-\left(D-1\right)\left(D-2\right)/2{l}^{2}$ is the cosmological constant with the radius of the AdS space l, F_$\mu$ν = ∂_$\mu$A_ν − ∂_νA_$\mu$ represents the strength of the electromagnetic field, and s is the nonlinearity parameter. Based on the equation (1), the line element of a D-dimensional nonlinearly AdS black hole with PMI source takes the form [53]
(2)$\begin{eqnarray}{\rm{d}}{s}^{2}=-f\left(r\right){\rm{d}}{t}^{2}+\displaystyle \frac{{\rm{d}}{r}^{2}}{f\left(r\right)}+{r}^{2}{\rm{d}}{{\rm{\Omega }}}_{D-2}^{2},\end{eqnarray}$
where ${\rm{d}}{{\rm{\Omega }}}_{D-2}^{2}$ denotes the line element of a $\left(D-2\right)$-dimensional space. When considering the field equations arising from the variation of the bulk action with the metric (2), the metric function $f\left(r\right)$ and gauge potential A are given by:
(3)$\begin{eqnarray}\begin{array}{rcl}f\left(r\right) & = & 1-\displaystyle \frac{m}{{r}^{D-3}}+\displaystyle \frac{{r}^{2}}{{l}^{2}}\\ & & -\,\displaystyle \frac{{\left(2s-1\right)}^{2}{\left[\tfrac{\left(D-2\right){\left(2s-D+1\right)}^{2}{q}^{2}}{\left(D-3\right){\left(2s-1\right)}^{2}}\right]}^{s}}{\left(D-2\right)\left(2s-D+1\right){r}^{2\left(\tfrac{{Ds}-4s+1}{2s-1}\right)}},\end{array}\end{eqnarray}$

(4)$\begin{eqnarray}A=-\sqrt{\displaystyle \frac{D-2}{2\left(D-3\right)}}{{qr}}^{\tfrac{2s-D+1}{2s-1}}{\rm{d}}t,\end{eqnarray}$
where the electromagnetic field 1-form is F = dA. Notably, to keep the nonlinear term of the source, the nonlinear parameter should satisfy s > 1/2 and $s\ne \left(D-1\right)/2$. The parameters m and q are related to the ADM mass M and total electric charge Q of the black hole respectively, which reads
(5)$\begin{eqnarray}\begin{array}{rcl}M & = & \displaystyle \frac{{\omega }_{D-2}\left(D-2\right)}{16\pi }m,\quad Q=\displaystyle \frac{{\omega }_{D-2}\sqrt{2}(2s-1)s}{8\pi }\\ & & \times \,{\left(\displaystyle \frac{D-2}{D-3}\right)}^{s-\tfrac{1}{2}}{\left[\displaystyle \frac{\left(D-1-2s\right)q}{2s-1}\right]}^{2s-1},\end{array}\end{eqnarray}$
with the volume of a unit $\left(D-2\right)$ sphere ${\omega }_{D-2}\,=2{\pi }^{\tfrac{D-1}{2}}/{\rm{\Gamma }}\left[\left(D-1\right)/2\right]$. According to equation (5), metric function (3) can be rewritten as follows:
(6)$\begin{eqnarray}\begin{array}{rcl}f\left(r\right) & = & 1-\displaystyle \frac{16M\pi }{\left(D-2\right){r}^{D-3}{\omega }_{D-2}}+\displaystyle \frac{16P\pi {r}^{2}}{\left(D-1\right)\left(D-2\right)}\\ & & +\,\displaystyle \frac{{\left(1-2s\right)}^{2}}{\left(D-2\right)\left(1-D+2s\right)}{r}^{\left[\tfrac{2+2s\left(D-4\right)}{1-2s}\right]}{\rm{\Theta }},\end{array}\end{eqnarray}$
where
(7)$\begin{eqnarray}{\rm{\Theta }}={\left\{\displaystyle \frac{{2}^{\tfrac{5}{2s-1}}{\pi }^{\tfrac{2}{2s-1}}\left(D-2\right)}{D-3}{\left[\displaystyle \frac{{\left(1+\tfrac{1}{D-3}\right)}^{\tfrac{1}{2}-s}Q}{s\left(2s-1\right){\omega }_{D-2}}\right]}^{\tfrac{2}{2s-1}}\right\}}^{s},\end{eqnarray}$
and P = −Λ/8π = (D − 1)(D − 2)/16πl² is a thermodynamic pressure, which is a key definition in the framework of black hole chemistry.

2.2. The thermodynamics of higher dimensional nonlinearly charged AdS black hole with PMI source

On the event horizon r₊, one can rewrite the ADM mass in terms of the P with the condition ${{\left.f\left(r\right)\right|}_{r=r}}_{{}_{+}}=0$, which reads as follows:
(8)$\begin{eqnarray}\begin{array}{rcl}M & = & -\displaystyle \frac{{r}_{+}^{D-3}{\omega }_{D-2}}{8\pi }\\ & & \times \,\left[1-\displaystyle \frac{D}{2}-\displaystyle \frac{8P\pi {r}_{+}^{2}}{D-1}\right.\left.+\displaystyle \frac{{\left(1-2s\right)}^{2}{\rm{\Theta }}}{2\left(1-D+2s\right)}{r}_{+}^{\tfrac{2+2s\left(D-4\right)}{1-2s}}\right].\end{array}\end{eqnarray}$
The Hawking temperature of the black hole can be easily obtained as
(9)$\begin{eqnarray}\begin{array}{rcl}T & = & \displaystyle \frac{f^{\prime} \left({r}_{+}\right)}{4\pi }=\displaystyle \frac{1}{4\pi }\\ & & \times \,\left[\displaystyle \frac{D-3}{r}+\displaystyle \frac{16P\pi r}{D-2}\right.\left.-\displaystyle \frac{\left(2s-1\right){\rm{\Theta }}}{D-2}{r}^{\tfrac{1+2s\left(D-3\right)}{1-2s}}\right],\end{array}\end{eqnarray}$
and the entropy is
(10)$\begin{eqnarray}S={\int }_{0}^{{r}_{+}}\displaystyle \frac{1}{T}{\left(\displaystyle \frac{\partial M}{\partial r}\right)}_{Q,P}{\rm{d}}{r}=\displaystyle \frac{{\omega }_{D-2}}{4}{r}_{+}^{D-2}.\end{eqnarray}$
It is clear that the entropy of the black hole obeys the area formula $S={ \mathcal A }/4$ with the area of the black hole ${ \mathcal A }$. Based on the above thermodynamics quantities, the first law of black hole thermodynamics in the extended phase space is given by
(11)$\begin{eqnarray}{\rm{d}}M=T{\rm{d}}S+V{\rm{d}}P+{\rm{\Phi }}{\rm{d}}Q,\end{eqnarray}$
where ${\rm{\Phi }}={\left(\partial M/\partial Q\right)}_{S,P}=\tfrac{{2}^{\tfrac{3-s}{2s-1}}{\pi }^{\tfrac{1}{2s-1}}\left(1-2s\right)}{1-D\ +\ 2s}$ ${{\rm{\Theta }}}^{\tfrac{1}{s}}{r}_{+}^{\tfrac{1-D+2s}{2D-1}}\sqrt{\tfrac{D-2}{D-3}}$ is the electric potential, and $V={\left(\partial M/\partial P\right)}_{S,P}\,={\omega }_{D-2}{r}_{+}^{D-1}/\left(D-1\right)$ is the thermodynamic volume, which corresponding conjugate quantity is the thermodynamic pressure P [54]. The connected Smarr relation becomes
(12)$\begin{eqnarray}\left(D-3\right)M=\left(D-2\right){TS}-2{PV}+\left(D-3\right){\rm{\Phi }}Q.\end{eqnarray}$
Next, substituting equation (8) into (9), the equation of state is
(13)$\begin{eqnarray}\begin{array}{rcl}P & = & -\displaystyle \frac{\left(D-2\right)\left(D-3\right)}{16\pi {r}_{+}^{2}}+\displaystyle \frac{\left(D-2\right)T}{4{r}_{+}}\\ & & +\,\displaystyle \frac{\left(2s-1\right){\rm{\Theta }}}{16\pi }{r}_{+}^{-\tfrac{2s\left(D-2\right)}{2s-1}}.\end{array}\end{eqnarray}$
According to the viewpoints in [18], the critical points of this thermodynamic system can be obtained by the conditions ${\left(\partial P/\partial {r}_{+}\right)}_{T={T}_{{\rm{cr}}}}={\left({\partial }^{2}P/\partial {r}_{+}^{2}\right)}_{T={T}_{{\rm{cr}}}}=0$, and the critical temperature is given by
(14)$\begin{eqnarray}\begin{array}{rcl}{T}_{{\rm{cr}}} & = & \displaystyle \frac{4\left(D-3\right)\left({Ds}-4s+1\right)}{\pi \left(D-2\right)\left(2{Ds}-6s+1\right)}\\ & & \times \,{\left[\displaystyle \frac{{ks}{\left(D-2\right)}^{2}\left(2{Ds}-6s+1\right){q}^{2s}}{16\left(D-3\right){\left(2s-1\right)}^{2}}\right]}^{\tfrac{1-2s}{2({Ds}-4s+1)}},\end{array}\end{eqnarray}$
where
(15)$\begin{eqnarray}k=\displaystyle \frac{{16}^{\tfrac{s\left(D-2\right)}{2s-1}}\left(2s-1\right){\left[\tfrac{\left(D-2\right){\left(2s-D+1\right)}^{2}}{\left(D-3\right){\left(2s-1\right)}^{2}}\right]}^{s}}{{\left(D-2\right)}^{\tfrac{2s\left(D-2\right)}{2s-1}}}.\end{eqnarray}$
Here we only express the critical temperature since it will be used to analyze the Joule-Thomson expansion of the black hole in the next section. The expressions critical pressure and the critical radius can be found in [53] if needed. From equations (9)-(15), one can see that the thermodynamic quantities of the higher dimensional nonlinearly AdS black hole with PMI source sensitively depend on the event horizon radius r₊, the dimensionality D, the ADM mass M, the total electric charge Q and the nonlinearity parameter s. Remarkably, those thermodynamic quantities can easily go back to the higher dimensional R-N AdS case when s = 1.

3. Joule-Thomson expansion of higher dimensional nonlinearly AdS black hole with PMI source

In this section, the Joule-Thomson expansion of higher dimensional nonlinearly AdS black hole with PMI source in the extended phase space is investigated. In the Joule-Thomson expansion, the enthalpy H of the van der Waals system can be used to define the non-equilibrium states. Meanwhile, the enthalpy is related to the temperature and pressure of the system [22, 23]. Hence, one can find a slope of an isenthlpic curve in the T-P plane, that is, the Joule-Thomson coefficient. According to [26], the Joule-Thomson coefficient is denoted as follows:
(16)$\begin{eqnarray}\mu ={\left(\displaystyle \frac{\partial T}{\partial P}\right)}_{H}=\displaystyle \frac{1}{{C}_{p}}\left[T{\left(\displaystyle \frac{\partial V}{\partial T}\right)}_{P}-V\right],\end{eqnarray}$
where ${C}_{p}=T{\left(\partial S/\partial T\right)}_{P}$ is the heat capacity at constant pressure. For $\mu$ > 0, one has a cooling region in the T-P plane, whereas a heating region appears for $\mu$ < 0. Moreover, when the Joule-Thomson coefficient vanishes, one can obtain the inversion temperature ${T}_{i}=V{\left(\partial T/\partial V\right)}_{P}$. In [53], the phase structure of higher dimensional nonlinearly AdS black hole with PMI source is analogous to that of Van der Waals system. Thus, it is interesting to investigate the throttling process of the higher dimensional nonlinearly AdS black hole with PMI source. Now, substituting the thermodynamic quantities of the black hole into equation (16), one yields
(17)$\begin{eqnarray}{\mu }_{\mathrm{BH}}=\displaystyle \frac{4{r}_{+}\left[16P\pi {r}_{+}^{2}+\left(D-3\right)D-{\rm{\Theta }}\left(4s-1\right){r}_{+}^{\tfrac{2+2s\left(D-4\right)}{1-2s}}\right]}{\left(D-1\right)\left[6+\left(D-5\right)D+16P\pi {r}_{+}^{2}-{\rm{\Theta }}\left(1-2s\right){r}_{+}^{\tfrac{2+2s\left(D-4\right)}{1-2s}}\right]}.\end{eqnarray}$
It is obvious that the Joule-Thomson coefficient (17) is sensitive to the properties of spacetime of the black hole. By fixing the pressure P and the charge Q, one can see how the dimensionality D and the nonlinearity parameter s affect the behaviors of the Joule-Thomson coefficient $\mu$_BH and Hawking temperature T in figure 1.

Figure 1.

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Figure 1.(a)-(c) The influence of D, Q and s on $\mu$_BH, respectively. (d)-(f) The influence of D, Q and s on T, respectively.


From figures 1(a)-(c), one can see that the general behavior of $\mu$_BH changes with r₊ as follows: when the event horizon enough large, $\mu$_BH is larger than zero. However, by decreasing the event horizon of the black hole, the Joule-Thomson coefficient gradually decreases to zero (i.e. T_i), and then goes to negative. Finally, the $\mu$_BH changes its sign at the divergent point. By comparing figures 1(a)-(c) with 1(d)-(f), it is found that the Joule-Thomson coefficient diverges at the points where the Hawking temperature becomes zero, and the $\mu$_BH decreases to zero as r₊ → 0. On the other hand, the curves of the Joule-Thomson coefficient move to the right as the D and Q increase, while those curves move to the left as s increases.

Next, by setting $\mu$_BH = 0, one can the inversion pressure _Pi, and then, substituting _Pi into equation (9), the parameter equation of the inversion curve can be expressed follows [55]
(18)$\begin{eqnarray}\left\{\begin{array}{l}{T}_{i}=\tfrac{1}{2\pi \left(D-2\right){r}_{+}}\left[3-D+{{sr}}_{+}^{\tfrac{2+2s\left(D-4\right)}{1-2s}}{\rm{\Theta }}\right],\\ {P}_{i}=\tfrac{1}{16\pi {r}_{+}^{2}}\left[\left(3-D\right)D+{r}_{+}^{\tfrac{2+2s\left(D-4\right)}{1-2s}}\left(4s-1\right){\rm{\Theta }}\right].\end{array}\right.\end{eqnarray}$
For further investigation of the inversion curve of the higher dimensional nonlinearly charged AdS black hole with PMI source, we plot figure 2 in the T-P plane.

Figure 2.

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Figure 2.The inversion curves for various combinations of D, Q and s.


Figure 2 illustrates the inversion temperature T_i associated with inversion pressure _Pi for various combinations of D, Q and s. It is worth noting that T_i increases monotonously with _Pi, this leads to each curve in the diagrams only exist one minimum value of inversion temperature ${T}_{i}^{\min }$, and the cooling region and the heating region are located above and below these curves, respectively, which are different from that of van der Waals fluids. By comparing the subgraphs of each row (e.g. figures 2(a)-(c)) and those of each column (e.g. figures 2(a), (d) and (g)), respectively, it can be also found that, for high pressure, the T_i decreases with the dimensionality D and the nonlinearity parameter s, whereas it increases with charge Q. However, as seen from the small box in each subgraph, the behaviors of inversion curves at low pressure are reverse to those at high pressures. In other word, D and s can enhance the curves of inversion temperature, while those curves decrease with Q.

Now, by demanding _Pi of equation (18) equals to zero, the roots are given by
(19)$\begin{eqnarray}\begin{array}{rcl}{r}_{\min } & = & {\left[\displaystyle \frac{\left(4s-1\right){\rm{\Theta }}}{D\left(D-3\right)}\right]}^{\tfrac{2s-1}{1+\left(D-4\right)s}},\\ {r}_{\min }^{{\prime} } & = & -{\left[\displaystyle \frac{\left(4s-1\right){\rm{\Theta }}}{D\left(D-3\right)}\right]}^{\tfrac{2s-1}{1+\left(D-4\right)s}}.\end{array}\end{eqnarray}$
It is worth noting ${r}_{\min }^{{\prime} }$ should be neglected since it always negative. Substituting ${r}_{\min }$ into T_i of equation (18), the minimum of inversion temperature can be obtained as
(20)$\begin{eqnarray}\begin{array}{rcl}{T}_{i}^{\min } & = & -\displaystyle \frac{\left(D-3\right)}{2\pi \left(D-2\right)}{\left[\displaystyle \frac{\left(4s-1\right){\rm{\Theta }}}{D\left(D-3\right)}\right]}^{\tfrac{1-2s}{\left[1+s\left(D-4\right)\right]}}\\ & & +\,\displaystyle \frac{s{\rm{\Theta }}}{2\pi \left(D-2\right)}{\left[\displaystyle \frac{\left(4s-1\right){\rm{\Theta }}}{D\left(D-3\right)}\right]}^{-\tfrac{1+2s\left(D-3\right)}{\left[1+s\left(D-4\right)\right]}}.\end{array}\end{eqnarray}$
Utilizing equation (14), the ratio between the minimum of inversion temperature and the critical temperature is
(21)$\begin{eqnarray}\begin{array}{rcl}{\eta }_{\mathrm{BH}} & = & \displaystyle \frac{{T}_{i}^{\min }}{{T}_{{\rm{cr}}}}=\displaystyle \frac{{\left({Ds}\right)}^{\tfrac{2s-1}{2+2s\left(D-4\right)}}}{2\left(D-2\right)}{\left(4s-1\right)}^{-\tfrac{1+2s\left(D-3\right)}{2+2s\left(D-4\right)}}\\ & & \times \,{\left(2s-1\right)}^{\tfrac{1-2s}{2+2s\left(D-4\right)}}{\left[1+2s\left(D-3\right)\right]}^{\tfrac{1+2s\left(D-3\right)}{2+2s\left(D-4\right)}}.\end{array}\end{eqnarray}$


In previous work, it is found that the ratio of R-N AdS black hole equals 1/2, which indicates that the changing trend of ${T}_{i}^{\min }$ and T_cr does not affect by the Q [26]. However, this finding is not universal. Specific to our work, one can see that the ratio $\eta$_BH depends on the dimensionality D and the nonlinearity parameter s. When s = 1, the ratio recovers the characteristic of the higher R-N AdS black hole system [28]. For the sake of simplicity, we present the ratio with s = 1, 3, 5, 7 and D = 4, 5, 6, 7, ∞ in table 1.


Table 1.
Table 1.The ratio $\eta$_BH for various nonlinearity parameter s and dimensions D.

Nonlinearity parameter	Dimensions	$\eta$BH
s = 1	D = 4	0.500 000
	D = 5	0.471 957
	D = 6	0.452 802
	D = 7	0.438 933
	D → ∞	0.333 333
s = 3	D = 4	0.458 603
	D = 5	0.434 455
	D = 6	0.414 689
	D = 7	0.399 481
	D → ∞	0.272 727
s = 5	D = 4	0.449 778
	D = 5	0.427 255
	D = 6	0.407 755
	D = 7	0.392 523
	D → ∞	0.263 158
s = 7	D = 4	0.445 956
	D = 5	0.424 204
	D = 6	0.404 849
	D = 7	0.389 624
	D → ∞	0.259 259

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In table 1, the ratio between the minimum of inversion temperature and the critical temperature decrease with s and D, which means that the denominator T_cr is grows faster than the numerator ${T}_{\min }$. When D → ∞ , the curve of $\eta$_BH approaches a constant. Interestingly, according to figure 3, one can find that the two adjacent curves get closer and closer with the increase of s, which never appear in the previous works.

Figure 3.

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Figure 3.Relationship between the ratio $\eta$_BH and the dimension D for different s.


Finally, considering the Joule-Thomson expansion is an isenthalpic process, it is interesting to investigate the isenthalpic curves in T-P plane. According to equations (8) and (13), the equation of the isenthalpic curves is given by
(22)$\begin{eqnarray}\left\{\begin{array}{l}T=-\tfrac{1}{2\pi {r}_{+}}+\tfrac{4M\left(D-1\right)}{\left(D-2\right){\omega }_{D-2}{r}_{+}^{D-2}}+\tfrac{{{sr}}_{+}^{\tfrac{1+2\left(D-3\right)s}{1-2s}}{\left(2s-1\right)}^{s}}{2\pi \left(1-D+2s\right)}{\rm{\Theta }},\\ P=-\tfrac{\left(D-1\right)\left(D-2\right)}{16\pi {r}_{+}^{2}}+\tfrac{\left(D-1\right)M}{{\omega }_{D-2}{r}_{+}^{D-1}}-\tfrac{\left(D-1\right){\left(1-2s\right)}^{2}{r}_{+}^{-\tfrac{2s(D-2)}{2s-1}}}{16\pi \left(D-2s-1\right)}{\rm{\Theta }}.\end{array}\right.\end{eqnarray}$
By using equation (21) and considering the ADM mass of the black hole is equals to its enthalpy in the extended phase space, that is H = M, the isenthalpic curves for various combinations of D, s, and Q are represented in figure 4.

Figure 4.

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Figure 4.The isenthalpic curves for various combinations of D, s and Q.


In figure 4, each graphics has three isenthalpic curves for different mass, the black solid curve, red dashed curve, and blue dotted curve are M = 3, M = 4, and M = 5, respectively. The gray dot-dash curve represents the inversion curve, which is consistent with that in figure 2. The inversion curves intersect the maximum point of the isenthalpic curves, it naturally leads to the left-hand side of the isenthalpic curve has a positive slope, while the slope of the isenthalpic curve becomes negative at the right-hand side. Therefore, in the throttling process, the inversion curve is regarded as the dividing line between the heating region and the cooling region. Meanwhile, by analyzing and comparing, it is easy to see that increase the mass M and s, or reduce the charge Q and D can enhance the isenthalpic curve. Furthermore, comparing figure 4(a) with (e), one can find that the isenthalpic curve still expands rightward when increasing the D, Q, and s at the same time. This indicates that the effect of s on the isenthalpic curve is much greater than other parameters.

4. Conclusion and discussion

In this paper, by considering cosmological constant as the pressure, we investigated Joule-Thomson expansion of the higher dimensional nonlinearly charged AdS black hole with PMI source. Firstly, according to the thermodynamic quantities of the higher dimensional nonlinearly charged AdS black hole with PMI source, we calculated the Joule-Thomson coefficient $\mu$_BH. The results showed that the $\mu$_BH is related to the dimensionality D, charge Q and nonlinearity parameter s. Meanwhile, it has a zero point and a divergent point, which are coincide the inversion temperature T_i and the zero point of Hawking temperature, respectively. The curve of the Joule-Thomson coefficient moves to the right as the spacetimes D or Q increases, while it moves to the left as s increases. Secondly, we analyzed inversion curve via equation (18) and figure 2. It is found that T_i increases monotonously with _Pi and leads to only one minimum value of inversion temperature ${T}_{i}^{\min }$ in the black hole system. At the high pressure area, the inversion curves increase as the dimensionality and the nonlinearity parameter decrease, or the charge increase. However, at the low pressure area, T_i increase as the D and s increase, or Q decrease. Next, we derived the expression of ${T}_{i}^{\min }$, and calculate the ratio between the minimum inversion temperature and the critical temperature $\eta$_BH. Both ${T}_{i}^{\min }$ and T_cr all contain the charge, whereas the ratio $\eta$_BH between them has nothing to do with Q. For s = 1, $\eta$_BH recovers the characteristic of the higher R-N AdS black hole system. If s > 1, it becomes smaller and smaller as D increases, which means that the denominator T_cr grows faster than the numerator ${T}_{\min }$. According to figure 3, it is obvious that the two adjacent curves get closer and closer with the increase of s, which never appear in the previous works. Finally, according to equation (21) and considering M = H in the extended phase space, we plot the isenthalpic curves for various combinations of D, M, Q and s in figure 4. It is easy to see that increase the mass M and s, or reduce the charge Q and D can enhance the isenthalpic curve, and the effect of s on the isenthalpic curve is much greater than other parameters.

Acknowledgments

The authors thank the anonymous referees for helpful suggestions and enlightening comments, which helped to improve the quality of this paper. This work is supported in part by the National Natural Science Foundation of China (Grant Nos. 11 847 048, 11 947 128 and 11 947 018) and the Fundamental Research Funds of China West Normal University (Grant Nos. 20B009, 17E093 and 18Q067).

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