Strange quark mass (m_s) dependent model of anisotropic strange quark star

In relativistic astrophysics, compact objects are the most dense objects in the universe. These objects are formed at the end of stellar evolution, when all the processes of the thermonuclear reactions stop owing to lack of fuel for sustaining them. A few such compact objects are white dwarfs (henceforth WD), neutron stars (henceforth NS), strange stars (henceforth SS), and black holes (henceforth BH), classified depending on their internal structure. White dwarfs are formed at the last state of planetary nebula and are stable against electron degeneracy pressure as proposed by S. Chandrasekhar [1,2]. On the basis of the relativistic approach, he derived the maximum possible mass $1.4\; M_\odot$ of a WD considering the electron degeneracy pressure. More massive compact objects like NS, SS, and BH are formed as remnants of supernovas. All these compact objects constitute the most important class of astronomical objects in present day research, in the field of relativistic astrophysics. For example, old WDs have been used recently to calibrate the current age of the universe. However, in the understanding of the dynamics of formation of galaxies at the time of early universe, supermassive BHs play a very important role. Coalescences of NSs and BHs are possibly the sources of intense gravitational waves travelling through the interstellar medium, detected in recent years by gravitational wave detectors. Though Chandrasekhar predicted that the maximum mass of WDs would be $1.4\; M_\odot$ , Das and Mukhopadhyay [3] have recently predicted that the upper mass limit of WD could be as high as $2.58\; M_\odot$ , considering the presence of high magnetic fields due to the smaller number of occupied Landau levels [4]. Therefore, it is very important to consider the internal composition of a compact object properly. The upper limit of mass of NSs is still an issue of debate, and it is challenging to predict the actual composition of the interior matter of a compact object. However, to distinguish a compact object from a BH, it is very crucial to predict the upper limit of the mass of a compact object, and this area draws considerable attention from researchers. In this context, treating neutrons as an ideal fermi gas, Oppenheimer and Volkoff [5] found the maximum mass of a typical Neutron Star to be $0.7\; M_\odot$ . However, in their approach, they ignored the nucleon-nucleon strong interaction at ultra high densities. As the internucleon distances are significantly small at such high densities, such nucleon-nucleon interactions cannot be ruled out. Accordingly, maximum mass should depend on EoS significantly, as such interaction may affect the EoS of matter in the compact object. In the case of highly dense stars, the suitable EoS of the stellar composition is not yet available. The exact prediction of the maximum mass of such stars is very difficult, as maximum mass is highly EoS dependent. Different compositions of matters have been taken into account to explain the maximum mass of such stars. Considering the perfect fluid matter composition inside a compact object with a density greater than the nuclear matter density, Rhoades and Ruffini [6] predicted that the maximum mass of an NS could be as high as $3.2\; M_\odot$ . Considering the Newtonian fluid of a uniform density star obeying EoS $ PV=- {\Omega}/{3} $ , where $\Omega={3}/{5}(GM^2/R)$ is the gravitational potential energy of a uniform density sphere of volumeV, Nauenberg and Chapline [7] determined the maximum mass of the compact object to be $3.6\; M_\odot$ . Assuming a perfect fluid distribution with energy density $ (\rho) $ , pressure $ (p) $ , and $ ( {\partial p}/{\partial \rho}) $ all positive, Sabbadini and Hartle [8] obtained a maximum mass of $5\; M_{\odot}$ . Considering a different form of EoS, Haensel [9] predicted that the maximum mass of a compact object may vary from 1.46 $ - $ 2.48 $ M_{\odot} $ . Many authors have used different EoS to define the observed physical properties of pulsars such as PSR J1614-2230, Vela X-1, LMC X-4, PSR J0030-451, Cen X-3, and PSR J0740-6620, but their predictions were found to be incorrect. Available neutron star models cannot explain their observed properties, such as masses and radii. These objects possess less mass and radius in comparison to an NS but higher mass to radius ratio (compactification factor) $ ( {M}/{R}) $ . All stars, showing such properties, are grouped into a new class of compact objects known as the Strange Star family after the hypothesis of Baymet al.and Alcocket al.[10,11]. Bodmer [12] and Witten [13] hypothesized that, in an absolute ground state, hadrons may form strange quark matter and not $ ^{56}{\rm Fe} $ . In the following articles [14−22], comprehensive studies on some compact objects made up of quark matter are given. Banerjeeet al.[23] derived the maximum mass of quark star to be around $1.5\; M_\odot$ . According to Annalaet al.[24] neutron stars having a mass corresponding to 1.4 $ M_{\odot} $ are inconsistent with the standard nuclear model. Their work also predicts that the nature of sound velocity may be related to the occurrence of quarks inside an NS of mass around 2 $ M_{\odot} $ . According to the work of Itoh [25], it is possible that a stable quark star may exist in hydrostatic equilibrium. It is important to study the interior composition of a stable quark star. In this context, Madsen [26] proposed that compact objects made up only with up $ (u) $ and down $ (d) $ quarks are perhaps unstable under the condition of zero external pressure. However, if strange $ (s) $ quarks are included into the system, the energy per baryon is effectively reduced, i.e., the energy per baryon of a system, which consists of three flavor quarks, $u,\;d$ , ands, is less than that of a two flavor quark (uanddonly) system. Therefore, it may be concluded that the three flavor Strange Quark Stars (henceforth SQS) are more stable than the quark stars consisting ofuanddquarks only. Therefore, the possibility of SQS cannot be ruled out. Though the existence of SQS is possible in nature, their formation process is so far quite unclear. Several attempts have been made to discuss the formation of SQS. Two well accepted possibilities that were predicted in articles [12,13,25] are as follows:

1. Strange stars may have been formed due to hadron-quark phase transitions inside compact objects, at high temperatures, at the moment of the formation of the early universe.

2. At ultra-high densities, a neutron star may be compacted into a strange star spontaneously, owing to a strong gravitational pull.

Alford [27] predicted that, inside the core of NS, the existence of a low temperature and high density region is adequate to form bulk quark matter. To explain the observed properties of strange quark stars, a suitable EoS is needed. In this context, for strange stars, one can utilize the EoS as given in the MIT bag model [28] for zero quark mass $ (m_s=0) $ assuming that the quarks form degenerated Fermi gas consisting ofu,d,s,and $ e^- $ given below:

However, in our work, we have considered a modified MIT EoS, where we have taken a non zero value for the strange quark mass. The modified EoS is given by $p_r = \dfrac{1}{3}(\rho - 4B^{\prime})$ , as discussed in Sec. II, where $B^{\prime} = B + \dfrac{1}{4}(\rho_{s} - 3p_{s})$ , $ \rho_{s} $ = density of quarks, $ p_{s} $ = quark pressure, and $ B= $ perturbative vacuum energy or bag constant.

Many investigators have used the MIT EoS to describe the observed properties of SQS adequately [29−35]. The stability of strange quark matter in presence of magnetic fields has been studied by Isayev [36]. Using the MIT EoS, Kalamet al.[37] predicted that a larger range ofBis permissible to satisfy the observed properties of a few pulsars like 4U 1820-30, Her X-1 and SAX J 1808.4-3658. Azizet al.[38] determined the wider range ofB(41.58 − 319.31 $ \rm MeV/fm^3 $ ) that is required to predict the observed properties of NS with a quark core.

Inside a compact object, pressure may be anisotropic, if the density exceeds the nuclear matter density, as proposed by Ruderman [39] and Canuto [40]. Super-fluidity and super-conductivity also play a crucial role in describing the anisotropic behavior of highly dense stars as explained by Bowers and Liang [41]. A detailed review work has been done by Herrera and Santos [42] on the possible origin of anisotropy. Anisotropy may also develop due to pion condensation [43], phase transition [44], existence of super-fluid of type 3A [45], or the presence of a solid core. Consideration of the presence of anisotropy in pressure is important, as anisotropic stars contain more mass than isotropic stars of same radius. Assuming the anisotropic nature of matter in the context of MIT EoS, Debet al.[46] prescribed a singularity free solution for compact objects, considering the Mak and Harko density profile, which is compatible with the observed data. Using MIT EoS, Goswamiet al.[47] predicted the maximum value of mass and radius of a class of SQS in the presence of anisotropy. Recently Sahaet al.[48] obtained the EoS for different compact objects, from observational data admitting the MIT EoS having aBvalue, that is suitable for stable quark matter.

In this paper, to solve EFEs, we consider the form of $ g_{rr} $ metric component as proposed by Thirukkanesh and Maharaj, and Thirukkanesh and Ragel [49,50] , which is characterized by two parameters namelyaandb,implying that physical 3-space associated with the star has the 3-spheroid geometry immersed within the 4-dimensional Euclidean space. The parametersaandbcan be determined by applying suitable boundary conditions. In this paper, we have included the mass of strange quark $ m_s $ in the EoS of MIT bag model, and we have evaluated the maximum mass by solving TOV equation for different stability windows of 3 flavor quark matter using the modified EoS. The effects of $ m_s $ on the gross properties of SQS are studied. Some interesting results are noted. It is observed that the stability of quark matter is affected due to inclusion of $ m_s $ in EoS.

This paper is arranged in the following manner. In Sec. II, the thermodynamic properties of SQM are given in brief considering the finite value of strange quark mass $ (m_s\neq0) $ , and the possible range of the values ofBare determined for different stability windows of three flavor quarks. In Sec. III, Einstein Field Equations for anisotropic stars are solved for known metric anstaz, and the condition for the physical viability of the solution is explored. In Sec. IV, the maximum mass and radius are given. In Sec. V, physical applications of our model by taking different compact objects are given. Energy conditions are shown in Sec. VI. Stability of the model is presented in Sec. VII. We present the Tidal Love Number and Tidal de-formability, using our model, in Sec. VIII. Finally, in Sec. IX, we discuss our findings.

We consider the EoS of the interior matter corresponding to the MIT bag model [51], in which quarks are assumed to be fermions and the dynamic process of quark confinement is set out by the following set of equations [52],

and

where $ p_{i} $ and $ \rho_{i} $ represent the pressure and energy density ofith quark, respectively. In case of a strange quark star, the interior matter may be composed ofu,d, andsquarks and electrons $ (e^{-}) $ as considered by Kettneret al.[52]. The charge neutrality condition of strange quark matter can be expressed as,

whereirepresents the particle type.

From the work of Kettneret al.[52] and Penget al.[53], the mathematical expressions of quark pressure $ (p_{i}) $ , quark energy density $ (\rho_{i}) $ , and number density of quarks $ (n_{i}) $ can be approximated by the following relations when temperature of the star is significantly smaller $ (T\rightarrow 0) $ than the chemical potential of quarks,

where the degeneracy factor $ g_{i} $ = 6 for all quark flavors and 2 for electrons. The charge neutrality condition given in Eq. (4) is modified as

whereμ= $ \mu_d $ = $ \mu_s $ is the chemical potential of thedandsquarks. In case of SQS composed ofu,d,andsquarks, whereuanddare less massive thans,and the mass of strange quark is assumed to be zero $ (m_s\rightarrow 0) $ , it is noted from Eq. (8) that $ \mu_{e^-}\rightarrow0 $ . Therefore, electrons are not compulsory constituents for the charge neutrality of a gas of massless strange quarks $ (m_s\rightarrow 0) $ . In the case $ (m_s=0) $ , Eqs. (5) and (6) give $ p_i $ = $ \dfrac{1}{3} \rho_{i} $ . Consequently, from Eqs. (2) and (3), one can establish the EoS for matter composed of massless quarks and electrons. This is known as the MIT bag model equation of strange matter as given in Eq. (1). Now the EoS of strange quark matter, in its most general form, can be obtained from Eqs. (2), (3), (5), and (6) considering a non-zero mass for strange quarks $ (m_s\neq0) $ is given below:

where $ B^{\prime} = B + \dfrac{1}{4}(\rho_{s} - 3p_{s}) $ , $ \rho_{s} $ = density of the strange quark, and $ p_{s} $ = pressure exerted by the strange quark.

The energy per baryon $ (E_B) $ in the case of $ ^{56}{\rm Fe} $ is around 930.4 MeV. Therefore, we may conclude that the energy per baryon of matter consisting of only two flavor quarks (up and down) might be higher than this value; otherwise, it is possible that a free $ ^{56}{\rm Fe} $ nucleus could only be composed up $ (u) $ and down $ (d) $ quarks. However, this phenomenon has not been observed. Inclusion of third flavor quarks $ (s) $ into the system reduces [26] the energy per baryon, and consequently, quark matter composed of three flavors would be more stable with respect to $ ^{56}{\rm Fe} $ if the value of $ E_B<930.4 ~\rm MeV $ . In case of metastable SQM, $ E_B $ should lie in the range $ 930.4 < ~ E_B ~ < 939 ~\rm MeV $ [54], where 939 MeV is known as the mass of nucleon. For unstable SQM, $E_B > 939~\rm MeV$ . In case of three flavor quark matter (SQM), the density of baryon number is given by

InFig. 1, the plot of $ E_B $ with strange quark mass $ (m_s) $ is shown for different values ofB. Also, fromFig. 1, we summarize our observation inTable 1. FromTable 1, it is evident that energy per baryon of three quark systems depends on the value ofBand $ m_s $ . Depending on the value ofBand $ m_s $ , we note that the three flavor quark matters may be (i) stable, (ii) metastable, or (iii) unstable. Also, we observe that for a fixedB, the model predicts some constraints on the upper limit of $ m_s $ , above which strange matter should be metastable or unstable. In this paper, we consider a value of $ m_s $ below this constraint value.

Figure 1.(color online) Variation of energy per baryon $ (E_B) $ with strange quark mass $ (m_s) $ for different value of bag constant $ (B) $ .

Stability	$B=57.55 \rm\;MeV/fm^3$	$B=66.90 \rm\;MeV/fm^3$	$B=83.21 \rm\;MeV/fm^3$	$B=91.54 \rm\;MeV/fm^3$	$B=95.11 \rm\;MeV/fm^3$
Stable	$ m_s<334 $	$ m_s<200 $	$ m_s<100.5 $	···	···
( $E_{B} < 930.4\rm~ MeV$ )
Metastable	···	···	$ 100.5	$ 0	···
( $ 930.4 )			$<120.3 $	$<60.18 $
Unstable	···	···	$ m_s>120.3 $	$ m_s>60.18 $	$ m_s>0 $
( $ E_{B}>939\rm~ MeV $ )

Table 1.Values ofBand corresponding Constraints on $ m_s $ essential for different stability windows of 3-flavor SQM.

Let us consider the interior of the cold compact stars described by the static spherically symmetric space time metric:

where ${\rm e}^{\nu(r)}$ and ${\rm e}^{\lambda(r)}$ are metric functions ofr. In relativistic compact stars, the energy momentum tensor of the interior matter content with anisotropic fluid pressures is given by

whereρ, $ p_{r} $ , and $ p_{t} $ are the energy density $ (\rho) $ , radial pressure $ (p_r) $ , and tangential pressure $ (p_t) $ , respectively. The measure of the pressure anisotropy in this model is defined by $ p_{t}-p_{r} $ = Δ. As $ p_r $ and $ p_t $ depend onr, Δ is also a function ofr.

The Einstein Field Equation ( $ hence forth ~~ EFE $ ) is given by

where $ {\bf R}_{ij} $ = Ricci tensor and $ {\bf R} $ = Ricci scalar. The left hand side represents the geometry corresponding to the energy momentum tensor of matter given in the right hand side.

Using Eqs. (12) and (13) in Eq. (14), the EFEs can be represented as

where $ (^\prime) $ indicates the derivative with respect tor. We have used the conventional values $ 8\pi G $ = 1 , and $ c =1 $ . Now we consider metric anstaz as proposed in Refs. [49,50,55] for the $ g_{rr} $ component characterized by two parameters denoted byaandbas given below:

In Eq. (18), dimensions of constantsaandbare $\rm Km^{-2}$ . These two constants define the curvature of space time.

Using Eqs. (10) and (18) in Eqs. (15)–(17), we obtain the following expression for physical parameters relevant to viable stellar configurations:

and

where $ X=\dfrac{2aB^{\prime}r}{b}-\dfrac{ar}{(1+ar^2)}+\dfrac{(-2ab+3b^2-2aB^{\prime}+2bB^{\prime})r}{b(1+br^2)} $ and $ Y=\dfrac{(a-b)r}{(1+ar^2)(1+br^2)} $ . Now we can determine the mass function $ m(r) $ of the star from the following expression:

Using Eq. (19), the expression of mass function in this model can be represented as

Eq. (24) shows that for $ m(r) > 0 $ , we should have $ a > b $ . The following bounds on metric constants "a" and "b" should be followed in order to get a physically viable stellar model. The expression for central density $ (\rho_0) $ can be found from Eq. (19) by putting $ r=0 $ and is given below:

Again, from Eq. (20), we note the value of central pressure $ (p_0) $ as follows:

For physically realistic models the following conditions must be satisfied:

(i) The interior metric as given in Eq. (12) should be continuous at the surface of the star, and hence, it must be equal to the exterior metric given by Schwarzschild:

Matching the potentials at the boundary, $ r=R $ gives

and

From Eq. (30), one can establish the connection between the constants "a"and "b"through the relation

Using Eqs. (26) and (31), we can express central density $ (\rho_0) $ as a function of the compactness $ (u) $ as given below:

whereu= $ \dfrac{M}{R} $ is defined as the compactness of the star.

(ii) The radial pressure $ (p_{r}) $ must vanish at $ (r=R) $ . Then, using Eq. (20), the radius $ (R) $ of the star can be determined as

From Eq. (33), it is evident that radiusRdepends on $ m_s $ through constant $ B^{\prime} $ as well as constantsaandb.

(iii) Inside a star, physical parameters likeρ, $ p_{r} $ and $ p_{t} $ all have positive values.

For positive central pressure $ (p_0 > 0) $ , we note from Eq. (27) that a lower bound on the constant "a"exists, which is

In Eq. (34), the dimension of $ B^{\prime} $ should be $\rm Km^{-2}$ as the dimensions ofaandRare $\rm Km^{-2}$ and $\rm Km$ , respectively, anduis dimensionless. AsBis given in $\rm MeV/fm^3$ , we have to divideBby the factor $ (3\times10^4) $ to get the dimension $\rm Km^{-2}$ . Accordingly $ B^{\prime} $ can be expressed in $\rm Km^{-2}$ .

(iv) The gradient of energy-density and the pressure must be negative inside the star, i.e., $ \left(\dfrac{{\rm d}\rho}{{\rm d}r}\right)<0 $ , $\left(\dfrac{{\rm d}p_{r}}{{\rm d}r}\right) < 0$ and $ \left(\dfrac{{\rm d}p_{t}}{{\rm d}r}\right)<0 $ .

(v) Both the pressures (radial and tangential) are same at the centre $ (r=0) $ , and therefore, $ \Delta = 0 $ at the centre of the star.

(vi) The square of radial $\left(v_{r}^2 = \dfrac{{\rm d}p_{r}}{{\rm d}\rho}\right)$ and tangential $\left(v_{t}^2 = \dfrac{{\rm d}p_{t}}{{\rm d}\rho}\right)$ sound velocities should lie within the range $ 0\leq v_{r}^2 \leq 1 $ and $ 0\leq v_{t}^2 \leq 1 $ .

Buchdahl predicted that the maximum value of mass to radius ratio (compactness) should obey the relation $ M/R\leq\dfrac{4}{9} $ [56]. From Eq. (19), it is noted that the central density of a star is related to the constants of the metric parameters through the relation $ \rho_0 = 3(a - b) $ . Therefore, for a given central density $ (\rho_0) $ , the mass function given in Eq. (25) can be written as

For a stellar configuration to be stable, the mass $ (M) $ of a star should increase with central density $ (\rho_0) $ , i.e., $ ({\partial{M}}/{\partial{\rho_0}}) >0 $ [57,58]. In presence of small perturbation, the condition $ (\partial{M}/\partial{\rho_0}) < 0 $ corresponds to an unstable stellar model. InFigs. 2and3, we have shown the mass-radius plot for two chosen values of the bag constant $ (B) $ , e.g., $ B = 57.55 $ and $ 91.54~\rm MeV/fm^3 $ , respectively. In both cases, the maximum mass is found to reach its maximum value when $m_s \rightarrow 0 \rm~ MeV$ . It is noted that the maximum mass may be as high as $ 2.01 M_\odot $ when $B = 57.55~\rm MeV/fm^3$ and $ 1.60~ M_\odot $ when $B = 91.54 ~ \rm MeV/fm^3$ . The corresponding radii are $ 10.96 ~\rm km $ and $ 8.69 ~\rm km $ , respectively. Again, keepingBfixed, we note that higher values of $ m_s $ admit lower maximum mass as evident fromFigs. 2and3. We note that when $ B=57.11 ~\rm MeV/fm^3 $ and $ m_s=150 ~\rm MeV $ , the maximum mass = 1.93 $ M_\odot $ , and when $ B=91.54 \rm MeV/fm^3 $ and $ m_s= $ 150 MeV, the maximum mass = 1.54 $ M_\odot $ . Dependence of maximum mass on the value of $ m_s $ can be explained from the concept of equation of state. The corresponding central densities $ (\rho_0) $ assume the values $ 1.98 \times 10^{15} ~\rm gm/cm^3 $ and $3.13 \times 10^{15} ~\rm gm/cm^3$ , respectively, as evident fromFigs. 4and5where $ B=57.55 $ and $ 91.54 ~\rm MeV/fm^3 $ , respectively. We note that though the maximum mass is less when $ B=91.54 ~\rm MeV/fm^3 $ , its compactness is slightly greater, and as a result, its central density becomes greater than when $ B=57.11~\rm MeV/fm^3 $ . This is also verified from Eq. (32).Figures 4and5also indicate that after reaching the point of maximum mass, star mass decreases with an increase in central density. Therefore, the stability criterion $({\partial{M}}/{\partial{\rho_0}}) > 0$ is valid only up to the maximum mass point. It is evident fromFig. 6that a higher value of $ m_s $ admits a softer EoS of matter, and consequently, the maximum mass becomes smaller for higher values of $ m_s $ .

Figure 2.(color online) Mass vs. radius curve for strange quark star for different strange quark mass $ (m_s) $ for a fixed bag constant $B = 57.55 ~\rm MeV/fm^3$ . The maximum mass points are filled by black points. Here, the black, red, green, orange, and blue lines represent the observed masses of PSR J1614-2230, PSR J1903+0327, 4U 1820-30, PSR J0030+0451, and GW170817, respectively.

Figure 4.Mass vs. central density curve for strange quark star for different strange quark mass $ (m_s) $ for a fixed bag constant $B = 57.55 ~\rm MeV/fm^3$ . The maximum mass points are filled by black points.

Figure 6.Variation of radial pressure $ (p_r) $ with energy density $ (\rho) $ for different values of strange quark mass $ (m_s) $ for an arbitrary bag constant $B = 60 ~\rm MeV/fm^3$ .

Figure 3.(color online) Mass vs. radius curve for strange quark star for different strange quark mass $ (m_s) $ for a fixed bag constant $B = 91.54 ~\rm MeV/fm^3$ . The maximum mass points are filled by black points. Here the black, red, green, orange, and blue lines represent the observed masses of PSR J1614-2230, PSR J1903+0327, 4U 1820-30, PSR J0030+0451, and GW170817, respectively.

Figure 5.Mass vs. central density curve for strange quark star for different strange quark mass $ (m_s) $ for a fixed bag constant $B = 91.54 ~\rm MeV/fm^3$ . The maximum mass points are filled by black points.

Case I:Now, we consider the compact object PSR J1614-2230, which is supposed to be an SQS having an observed mass 1.97 $ M_{\odot} $ [47]. We have predicted the radius of PSR J1614-2230 from our proposed model and tabulated the same inTable 2. We have noted that the radius $ (R) $ of the star depends on the mass $ (m_s) $ of the strange quark, and the value ofB. FromTable 2, it is observed that the radius of PSR J1614-2230 may be predicted for different combinations ofa,B,and $ m_s $ . It is also noted that the predicted radius decreases whenBand $ m_s $ increase. We have also determined the binding energy per baryon $ (E_B) $ for different combinations ofBand $ m_s $ and listed the same inTables 2and3. We may conclude that the stability of SQM is a function of bothBand $ m_s $ . Energy per baryon increases with the increase inBand $ m_s $ . An interesting feature is that the mass of $ m_s $ cannot be increased arbitrarily depending on the value ofB. For example, when $ B=57.55 $ , the value of $ m_s $ should lie below 290 MeV to get stable SQM. However, when $ 290 , SQM becomes metastable, and for $ m_s> $ 334 MeV, SQM is unstable. However, with increasingB,these stability windows change and occur at different values of $ m_s $ , as shown inTables 2and3. We have noted that beyond a certain value of $B\; (=91.54 ~ \rm MeV/fm^3)$ , SQM becomes unstable for any value of $ m_s $ [59]. The variations of different physical parameters, namely energy density $ (\rho) $ , radial pressure $ (p_{r}) $ , tangential pressure $ (p_{t}) $ , and pressure anisotropy $ (\Delta) $ are also shown inFigs. 7−10for different values of $ m_s $ . We note that all the physical parameters are well behaved for the chosen value of different parameters. InFigs. 11and12we have shown the variation of density and pressure gradients inside PSR J1614-2230.

$B/ ( {\rm MeV}/{\rm fm^3} )$	a	$m_{s}/\rm MeV$	$E_B/\rm MeV$	Predicted radius $ (R) $	Stability
57.55	0.01	0	828.49	11.25	stable
		50	834.98	11.21	stable
		100	852.07	11.10	stable
		290	930.37	11.07	stable
		334	933.89	11.05	metastable
70	0.015	0	870.06	10.33	stable
		50	876.26	10.29	stable
		150	915.39	10.09	stable
		180	930.07	10.04	stable
		190	934.94	10.03	metastable
		199	939.25	10.02	unstable
		205	942.09	10.02	unstable
90	0.023	0	926.48	9.31	stable
		40	930.26	9.29	stable
		50	932.33	9.28	metastable
		75	939.45	9.25	unstable
		100	948.06	9.20	unstable
		150	970.07	9.11	unstable
91.54	0.023	0	930.42	9.27	metastable
		50	936.24	9.24	metastable
		100	951.92	9.16	unstable
		150	973.89	9.07	unstable

Table 2.Predicted radius for the compact object PSR J1614-2230 with mass 1.97 $ M_{\odot} $ .

$B /({\rm MeV}/{\rm fm^3})$	a	$m_{s}/\rm MeV$	$E_B /\rm MeV$	Predicted radius (R)	stability
57.55	0.008	0	828.49	11.10	stable
		50	834.98	11.05	stable
		100	852.07	10.94	stable
		150	875.14	10.82	stable
		290	930.37	10.91	stable
80	0.015	0	899.60	9.65	stable
		50	905.61	9.61	stable
		100	921.69	9.53	stable
		120	930.11	9.50	stable
		121	930.54	9.49	metastable
		140	939.25	9.45	unstable
		150	944.01	9.43	unstable
90	0.015	0	926.48	9.33	stable
		40	930.26	9.31	stable
		50	932.33	9.30	metastable
		75	939.17	9.26	unstable
		100	948.10	9.22	unstable
		150	970.10	9.13	unstable
91.54	0.015	0	930.42	9.29	metastable
		50	936.24	9.25	metastable
		100	951.92	9.18	unstable
		150	973.89	9.09	unstable

Table 3.Predicted radius for the compact object Vela X-1 with mass 1.77 $ M_{\odot} $ .

Figure 7.Variation ofρwithrin PSR J1614-2230 for different values of strange quark mass $ (m_{s}) $ andB= 70 $\rm MeV/fm^3$ .

Figure 8.Variation of $ p_{r} $ withrin PSR J1614-2230 for different values of strange quark mass $ m_{s} $ andB= 70 $\rm MeV/fm^3$ .

Figure 9.(color online) Radial variation of tangential pressure $ p_{t} $ in PSR J1614-2230 for different values of strange quark mass $ m_{s} $ andB= 70 $ MeV/fm^3 $ .

Figure 10.Radial variation of Δ in PSR J1614-2230 for different values of strange quark mass $ m_{s} $ andB= 70 $\rm MeV/fm^3$ .

Figure 11.Behavior of energy density gradient ( $ {\rm d}\rho/{\rm d}r $ ) in PSR J1614-2230 withB= $ 70 ~\rm MeV/fm^3 $ for different $ m_s $ .

Figure 12.(color online) Behavior of different pressure gradients in PSR J1614-2230 withB= $ 70 ~\rm MeV/fm^3 $ for different $ m_s $ . Here red and green colours represent ( $ {\rm d}p_r/{\rm d}r $ ) and ( $ {\rm d}p_t/{\rm d}r $ ) respectively.

Case II:Consider another low mass X-ray binary star Vela X-1 of observed mass 1.77 $ M_{\odot} $ [60]. We have calculated its radius from our proposed model and tabulated the same inTable 3. The radial variation of different physical parameters like energy density $ (\rho) $ , radial pressure $ (p_{r}) $ , tangential pressure $ (p_{t}) $ and pressure anisotropy $ (\Delta) $ are also plotted inFigs. 13−16respectively. InFigs. 17and18we have shown the variation of density and pressure gradients inside Vela X-1.

Figure 13.Radial variation of energy density $ (\rho) $ in Vela X-1 for different values of strange quark mass $ (m_{s}) $ andB= 80 $\rm MeV/fm^3$ .

Figure 14.Radial variation of radial pressure $ p_{r} $ in Vela X-1 for different values of strange quark mass $ m_{s} $ andB= 80 $\rm MeV/fm^3$ .

Figure 15.(color online) Radial variation of tangential pressure $ p_{t} $ in Vela X-1 for different values of strange quark mass $ m_{s} $ andB= 80 $ MeV/fm^3 $ .

Figure 16.Radial variation of Δ in Vela X-1 for different values of strange quark mass $ m_{s} $ andB= 80 $\rm MeV/fm^3$ .

Figure 17.Behavior of energy density gradient ( ${\rm d}\rho/{\rm d}r$ ) in Vela X-1 withB= $ 80 ~\rm MeV/fm^3 $ for different $ m_s $ .

Figure 18.(color online) Behavior of different pressure gradients in Vela X-1 withB= $ 80 ~\rm MeV/fm^3 $ for different values of $ m_s $ . Here, red and green colours represent ( $ {\rm d}p_r/{\rm d}r $ ) and ( $ {\rm d}p_t/{\rm d}r $ ) , respectively.

For any fluid sphere that is anisotropic in nature, all the energy conditions [61,62], such as the $ (i) $ weak energy condition (WEC), $ (ii) $ null energy condition (NEC), $ (iii) $ strong energy condition (SEC), and $ (iv) $ dominant energy condition (DEC), must be fulfilled throughout the interior of the fluid sphere. These are expressed mathematically as shown below.

1. NEC: $ \rho+p_{r} \geq 0 $ and $ \rho+p_{t} \geq 0 $ .

2. WEC: $ \rho \geq 0 $ , $ \rho+p_{r} \geq 0 $ , and $ \rho+p_{t} \geq 0 $ .

3. SEC: $ \rho+p_{r} \geq 0 $ , $ \rho+p_{t} \geq 0 $ and $ (\rho+p_{r}+2p_{t}) \geq 0 $ .

4. DEC: $ \rho \geq 0 $ , $ (\rho-p_{r}) \geq 0 $ and $ (\rho-p_{t}) \geq 0 $ .

FromFigs. 19−23, it is found that all the necessary energy conditions are valid in this approach.

Figure 19.Radial variation of $ (\rho + p_r) $ in PSR J1614-2230 for different values of strange quark mass $ (m_{s}) $ andB= 70 $\rm MeV/fm^3$ .

Figure 20.Radial variation of $ (\rho - p_r) $ in PSR J1614-2230 for different values of strange quark mass $ m_{s} $ andB= 70 $\rm MeV/fm^3 $ .

Figure 21.Radial variation of $ (\rho + p_t) $ in PSR J1614-2230 for different values of strange quark mass $ m_{s} $ andB= 70 $\rm MeV/fm^3$ .

Figure 22.Radial variation of $ (\rho - p_t) $ in PSR J1614-2230 for different values of strange quark mass $ m_{s} $ andB= 70 $\rm MeV/fm^3$ .

Figure 23.Radial variation of $ (\rho + p_r + 2p_t) $ in PSR J1614-2230 for different values of strange quark mass $ m_{s} $ andB= 70 $\rm MeV/fm^3$ .

For any stellar model to be viable it, must satisfy the stability criterion of the configuration within the parameter space used to define the model. We have discussed stability in light of the following analyses:

1. Verification of Tolman-Oppenheimer and Volkoff equation.

2. Fulfillment of cracking condition proposed by Herrera.

3. Value of adiabatic index $(\Gamma) > {4}/{3}$ (Newtonian limit).

According to Tolman [63] as well as Oppenheimer and Volkoff [5], the sum of the three forces, namely the gravitational $ (F_g) $ , hydrostatic $ (F_h) $ , and anisotropic $ (F_a) $ , should be equal to zero, in stable equilibrium, throughout the interior of the compact object, i.e.,

The generalized form of the TOV equation [64,65] is

where $ M_g $ denotes the effective gravitational mass within the radiusrof a stellar configuration expressed as

where $\nu^{\prime}= {{\rm d}\nu}/{{\rm d}r}$ , and at any pointrinside a stellar structure, gravitational force $ F_g $ comes from the effective mass $ (M_g) $ of the spherical region of radiusrfollowing the relation given in Eq. (38). For the present model,

In this paper, the units used forρ, $ p_r $ and $ p_t $ are $\rm MeV/fm^3$ . Now, as the metric potentialνis unitless, its derivative $\nu^{\prime}= {{\rm d}\nu}/{{\rm d}r}$ has the unit $\rm Km^{-1}$ . Againρ, $ p_r $ , and $ p_t $ can be expressed in the units $\rm Km^{-2}$ using the transformation $1~\rm Km^{-2}=3\times10^4 ~\rm MeV/fm^3$ [66]. Therefore, in view of Eqs. (39)−(41), the forces ( $ F_g $ , $ F_h $ , and $ F_a $ ) can be expressed in the unit of $\rm Km^{-3}$ . InFig. 24, we have presented the variation of $ F_g $ , $ F_h $ , and $ F_a $ with radial distance obtained from Eqs. (39)−(41), respectively, with $ m_s = $ 0, 100, 150 MeV for PSR J1614-2230. From these plots, it is ovious that inside the stellar configuration, static equilibrium is established under the combined effect of the above three forces. We note that combined effects of hydrostatic $ (F_h) $ and anisotropic $ (F_a) $ forces jointly balance the gravitational force $ F_g $ , to make the resultant of these forces equal to zero in the interior, as well as on the surface, of the compact objects. We have also noted that the anisotropic force $ (F_a) $ increases from centre to surface monotonically. In contrast, both the gravitational $ (F_g) $ and hydrostatic $ (F_h) $ forces increase from the centre, assume a maximum value between the centre and surface, and then decrease up to the surface. A similar type of variation is also reported by Mauryaet al.[67] for different compact objects in four dimensional space-time geometry.

Figure 24.(color online) Radial variation of different forces of PSR J1614-2230 for $B = 70 ~\rm MeV/fm^3$ . Here, the dotted line represents $ m_s = 0 $ , dashed line represents $ m_s = 100 $ , and solid line represents $ m_s = 150 $ .

To satisfy the causality conditions, the squares of the radial $ (v_r^2) $ and the tangential sound velocities $ (v_t^2) $ should lie within the ranges $ 0 \leq v_r^2 \leq 1 $ and $ 0 \leq v_t^2 \leq 1 $ , respectively. Fulfillment of causality conditions is evident fromFig. 25inside PSR J1614-2230. To check the stability criterion of anisotropic matter distribution inside a compact object, Herrera [68] first suggested the "Cracking condition" concept. Based on Herrera's concept, Abreuet al. [69] gave a criterion that states that, for any stellar model, the following inequility should be satisfied:

Figure 25.(color online) Radial variation of square of the radial $ (v_r^2) $ and tangential $ (v_t^2) $ sound velocities in PSR J1614-2230 for $B = 70 ~\rm MeV/fm^3$ . Plot in red represents $ v_r^2 $ and black represents $ v_t^2 $ for different values of $ m_s $ .

Eq. (42) is also known as the Abreu inequality. We have plotted the value of $ |v_t^2 - v_r^2| $ withrfor PSR J1614-2230 and shown inFig. 26that the Abreu inequality is satisfied at all points inside the star PSR J1614-2230.

Figure 26.Radial variation of $ |v_t^2 - v_r^2| $ in PSR J1614-2230 for different values of $ m_s $ for $B = 70 ~\rm MeV/fm^3$ .

An isotropic star adiabatic index $ (\Gamma) $ is defined by the following relation:

where $ p_r $ is the radial pressure.

According to Heintzmann and Hillebrandt [70], for any isotropic stellar structure to be stable, the adiabatic index must be within the Newtonian limit, i.e., $\Gamma > {4}/{3}$ . Chanet al. [71] modified this condition for an anisotropic star, where radial pressure $ (p_r) $ and tangential pressure $ (p_t) $ exist. For such a star, $\Gamma > \Gamma_{\max}^{\prime}$ , where

The necessary and sufficient condition for anisotropic stellar structure stability is that the adiabatic index $ (\Gamma) $ be greater then $\Gamma_{\max}^{\prime}$ . The adiabatic index Γ for PSR J1614-2230 inFig. 27shows that the value of the adiabatic index satisfies the stability criterion.

Figure 27.(color online) Radial variation of adiabatic index $ (\Gamma) $ in PSR J1614-2230 for different values of $ m_s $ at $B = 70 ~\rm MeV/fm^3$ . Here, the red line represents the value $\Gamma = {4}/{3}$ (Newtonian limit).

We have also studied the stability criterion of a stellar structure with respect to small radial oscillation. The absolute value of Lagrangian perturbation $ |\Delta p_r (R)| $ of radial pressure at $ r=R $ of the star against frequency ( $ \omega^2 $ ) is plotted inFigs. 28and29for PSR J1614-2230 and Vela X-1, respectively. We have adopted the technique proposed by Pretel [72]. The infinitesimal radial mode of oscillation can be expressed by two coupled equations:

Figure 28.(color online) Variation of absolute value of the Lagrangian change in radial pressure at the surface $ |\Delta p_r(R)| $ vs. $ \omega^2 $ for different combinations of $ m_s $ for the compact object PSR J1614-2230.

Figure 29.(color online) Variation of absolute value of the Lagrangian change in radial pressure at the surface $ |\Delta p_r(R)| $ vs. $ \omega^2 $ for different combinations of $ m_s $ for the compact object Vela X-1.

and

The eigenfunction represented byχis associated with the radial segment of the Lagrangian displacement and is denoted by $ \chi=\dfrac{\delta(r)}{r} $ . Here, we have adopted normalized eigenfunctionsχsuch that $ \chi(0)=1 $ at the centre. Owing to the term ( ${1}/{r}$ ) in Eq. (45), there is a singularity at $ r=0 $ . To avoid the singularity, the coefficient of ( ${1}/{r}$ ) in the right hand side of Eq. (45) should vanish, giving

Again, as the radial pressure goes to zero at the stellar surface ( $ r=R $ ), the corresponding Lagrangian change in radial pressure should also be zero, i.e.,

In this work, the variations of Lagrangian change in radial pressure at the stellar surface of PSR J1614-2230 and Vela X-1 are plotted as a function of $ \omega^2 $ . The minima of these plots represent the exact normal mode frequencies. It is observed that, for the lowest normal mode, $ \omega_0^2 > 0 $ ; thus, our model stays in static equilibrium against small radial perturbations too.

The distortion of the spherical shape of the surface of a compact object due to external perturbing gravity field is measured by a parameter known as the Tidal Love Number denoted by $ k_2 $ . Tidal de-formability (Λ) is also a measure of surface distortion, which is associated with the Tidal Love Number $ k_2 $ by the relation given below:

whereMis the mass of compact object, andRits radius. The expression for the even parity $ (l=2) $ Tidal Love Number (TLN) evaluated by Hindereret al.[73] is given below:

here,uis known as compactness $ \left(= \dfrac{M}{R}\right )$ and $ g=\dfrac{bH^{'}(R)}{H(R)} $ . $ H(R) $ is the value of $ H(r) $ at $ r=R $ (surface). The dash represents the derivative with respect tor. The expression of $ H(r) $ [74] is given below

The binary neutron star merger event GW170817 has placed some constraints on Λ and has been predicted by Abbott and Abbott [75]. For a star of $ 1.4 M_{\odot} $ , the Tidal de-formability should be $ \Lambda<800 $ as shown in the article [76]. InTable 5, the Tidal Love Number and Tidal de-formability of the companion star in the GW170817 event of mass $ 1.4\; M_{\odot} $ for $ m_s=90 $ and 100 MeV are listed. It is noted that the Tidal de-formability (Λ) lies with in the range $ 70<\Lambda_{1.4}<580 $ .

Star	Observed mass ( $ M_\odot $ )	$m_s/\rm MeV$	B $/\rm(MeV/fm^3)$	Predicted radius $(R)/\rm Km$	u	$ k_2 $	Λ
GW170817 [80]	1.4	90	57.55	11.53	0.1790	0.1013	367.065
			91.54	9.91	0.2083	0.0838	142.417
		100	57.55	11.50	0.1796	0.1022	365.118
			91.54	9.89	0.2088	0.0836	140.456

Table 5.Value of Tidal de-formability in our model within the parameter space used.

In this article, we have analyzed a class of strange stars described by the generalised MIT bag model EoS of the type $ \rho = 3p+4B+\rho_s-3p_s $ and included the effect of the strange quark mass $ (m_s) $ . Employing the Vaidya-Tikekar [49,50] type metric ansatz, we have solved the EFE for perfect fluids having an anisotropic pressure distribution. The $ g_{rr} $ component of the Vaidya-Tikekar metric is characterised by two parametersaandb,which define the curvature of spacetime attached to a compact object. The allowed values of bag constantBare restricted to the range 57.55− $ 91.54 ~\rm MeV/fm^3 $ , in which quark matter composed of three quarks (u,d, ands) is absolutely stable with respect to neutrons [59]. In this model, the expressions for various physical parameters are found to be explicitly dependent on the bag constantBand strange quark mass $ m_s $ . In our study, some constraints on the maximum value ofBand $ m_s $ were noted. For example, when $ B=57.55~\rm MeV/fm^3 $ , the maximum allowed value of $ m_s $ is $ 334 ~\rm MeV $ . Above this value, strange quark matter will be metastable or unstable. In contrast, when $ m_s $ = 0,Bshould lie below or at $ 91.54 ~\rm MeV/fm^3 $ to get stable strange quark matter. We have evaluated $ E_B $ to study the stability of strange quark matter inside an SQS for different values of $ m_s $ . The $ E_B $ vs. $ m_s $ plot for a givenBis shown inFig. 1, and the results are compared to the binding energy of $ ^{56}{\rm Fe} $ ( $ E_{B} = 930.4~\rm MeV $ ) and nucleons ( $ E_{B} = 939~\rm MeV $ ). We have explored three distinct windows in view of stability of strange quark matter depending on the value of $ m_s $ andBviz. $ (i) $ stable $ (ii) $ metastable, and $ (iii) $ unstable SQM. Corresponding values of $ m_s $ andBare listed inTable 1. It is evident that a lower value of $ m_s $ indicates better stability of SQM inside an SQS. Therefore, for strange quark stars having a maximum mass with stable SQM, a smaller value of $ m_s $ is preferred. Using the generalized EoS, we have obtained the M-R plot as shown inFigs. 2and4. From the M-R plots, we have observed that the maximum mass obtained from our model is $ m_s $ dependent and picks up maximum values of $ 2.01 ~~ M_\odot $ and $ 1.60 ~~ M_\odot $ when $ B=57.55 $ and $ 91.54 \rm~ MeV/fm^3 $ , respectively, for $ m_s = 0 \rm~ MeV $ , which corresponds to stable SQM. Again, keepingBfixed, we noted that a higher value of $ m_s $ admits a lower maximum mass of the quark star, as evident fromFigs. 2and4. It is noted that when $ B=57.55~\rm MeV/fm^3 $ and $ m_s=150\rm\; MeV $ , the maximum mass is $ 1.93 \; M_\odot $ , and when $ B=91.54 \rm\; MeV/fm^3 $ and $ m_s= $ 150 MeV, the maximum mass is $1.54 \; M_\odot$ . It is observed that $ m_s $ has some effect on the maximum mass and radius of an SQS, and both the maximum mass ( $ M_{\max} $ ) and radius ( $R_\rm{max}$ ) decrease with increasing $ m_s $ . Such behavior may be explained as follows: as the maximum mass of a compact object depends strictly on the EoS of interior matter, the higher the value of $ m_s $ , the softer the EoS, as evident fromFig. 6, and hence, the lower the maximum mass and radius. Such types of variation have also been reported by Liet al.[82] from a different aspect. From an article of the Particle Data Group [83], we have also evaluated the values of maximum mass as 1.97 $ M_\odot $ and 1.57 $ M_\odot $ for $ B= $ 57.55 and 91.54 $ \rm MeV/fm^3 $ , respectively, for a reasonable value of $ m_s=90\rm~ MeV $ . InTables 2and3, we have presented the energy per baryon of SQM for PSR J1614-2230 and Vela X-1, respectively. It is evident that the stability, in view of energy per baryon, is affected by the vale ofBand $ m_s $ . For physical analysis, we considered the compact objects PSR J1614-2230 and Vela X-1. The radii of PSR J1614-2230 and Vela X-1 predicted by this model are shown inTables 2and3. From our analysis, it may be concluded that 3-flavor quark matter may be stable inside these stars for lower bag constants (B) at different values of $ m_s $ . The plots of the energy density (ρ), radial pressure ( $ p_r $ ), tangential pressure ( $ p_t $ ) are shown inFigs. 7−9, respectively, for PSR J1614-2230 and inFigs. 13−15for Vela X-1. It is evident from these figures that the variation of the physical parameters satisfies the relevant properties for a viable stellar model. FromFigs. 19−23, it is also evident that the necessary energy conditions related to a stellar configuration are satisfied. We have noted that our model is stable in view of $ (i) $ validity of TOV equation, $ (ii) $ fulfillment of cracking condition of Herrera, and $ (iii) $ verification of the value of the adiabatic index ( $ \Gamma>\frac{4}{3} $ ). InFigs. 28and29, we have plotted the absolute value of Lagrangian perturbation in radial pressure at $ r=R $ of PSR J1614-2230 and Vela X-1, respectively, against normal mode frequencies $ (\omega^2) $ . The minimum values of $ |\Delta p_r (R)| $ correspond to eigen frequencies of different normal modes. It is evident from the plots that all normal mode frequencies are real ( $ \omega_n^2>0 $ ). From recent observations, the radius of a few pulsars and secondary objects in gravitational wave events were also predicted by the present model and listed inTable 4. The radius of the secondary object in the gravitational wave event GW190814 predicted by our model was in the range of $ 11.60 - 11.98 ~\rm Km $ , whenB= $ 91.54 ~\rm MeV/fm^3 $ and $ m_s $ lies in the range $ 0-200 ~\rm MeV $ . Very recently, Mauryaet al.[84] also predicted the radius of secondary object in GW190814 as $ 11.76_{-0.19}^{+0.14} ~\rm Km $ in the context of gravitational decoupling in Einstein-Gauss-Bonnet gravity. Our prediction is consistent with the result of Mauryaet al.[84]. InTable 4, we have also listed our predicted radius of PSR J0952-0607 of massM= $ 2.35\pm0.17 ~ M_\odot $ measured recently, which is supposed to be the heaviest and fastest pulsar found in the disk of our Milky Way galaxy, supporting the possible existence of SQM, and it is noted that the radius of this pulsar from our model may lie within the range of $ 11.25 - 13.45 ~\rm Km $ whenBand $ m_s $ lie in the range of $ 57.55-91.54\rm\; MeV/fm^3 $ and $ 0-200\rm\; MeV $ , respectively. Tidal Love Number and Tidal de-formability are also evaluated in this model for the companion star of GW170817 events and are listed inTable 5. The values of Tidal de-formability lie within the range $ 70<\Lambda_{1.4}< 580 $ for the parameters used here. Thus, a broad range of masses and radii of SQSs may be predicted from our proposed model admitting stable SQM.

Star	Observed mass ( $ M_\odot $ )	Observed radius $\rm{/Km}$	$m_s \rm{/MeV}$	Predicted radius $\rm (Km)$
				$B=57.55\;\rm{/(MeV/fm^3)}$	$B=91.54\; \rm{/(MeV/fm^3)}$
PSR J0030+0451 [77]	1.44	13.02	0	11.81	10.12
			100	11.61	9.98
			200	11.39	9.78
PSR J0740+6620 [78]	2.072	12.39	0	12.92	11.16
			100	12.73	11.02
			200	12.50	10.81
GW190814 [79]	2.59	····	0	13.87	11.98
			100	13.65	11.83
			200	13.40	11.60
GW170817 [80]	1.4	····	0	11.70	10.03
			100	11.50	9.89
			200	11.28	9.69
PSR J0952-0607 [81]	2.35	····	0	13.45	11.62
			100	13.24	11.47
			200	13.00	11.25

Table 4.Predicted radius $ (R) $ of some compact objects.

We are thankful to the anonymous referees for the important suggestions made to improve our article.