# Exact Relativistic Magnetized Haloes around Rotating Disks

Authors: Antonio C. Gutiérrez-Piñeres; Abraão J. S. Capistrano
Journal: Advances in Mathematical Physics
 (2015)

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## Abstract

The study of the dynamics of magnetic fields in galaxies is one of important problems in formation and evolution of galaxies. In this paper, we present the exact relativistic treatment of a rotating disk surrounded by a magnetized material halo. The features of the halo and disk are described by the distributional energy-momentum tensor of a general fluid in canonical form. All the relevant quantities and the metric and electromagnetic potentials are exactly determined by an arbitrary harmonic function only. For instance, the generalized Kuzmin-disk potential is used. The particular class of solutions obtained is asymptotically flat and satisfies all the energy conditions. Moreover, the motion of a charged particle on the halo is described. As far as we know, this is the first relativistic model describing analytically the magnetized halo of a rotating disk.


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## 1. Introductory Remarks

In the observational context, many ambiguities still exist about the main constituents, geometry, and dynamics (thermodynamics) of the galactic disk-haloes. However, there are several different observations which probe the galactic and surrounding galactic magnetic field. For instance, it can be measured by nonthermal radio emission from energy equipartition that results from the interaction of magnetic energy with relativistic particles which can play a role in the formation of arms in spiral galaxies (see Krause’s “Magnetic Fields and Halos in Spiral Galaxies” [1] and “Magnetic Fields in Spiral Galaxies” [2] and references therein). For nearby galaxies, other probes are used as optical polarization, polarized emission of clouds and dust grains, maser emissions, diffuse radio polarized emission, and rotation measures of background polarization sources also. Magnetic fields can be seen as a new structural quantity and added to other constituent parameters (e.g., H-alpha lines, density mass, local shocks, etc.) are important to study the formation and dynamics of galaxies. Other works propose that magnetic fields also play important role in large-structure formation [3].It is important to stress that magnetic fields are found mainly in interstellar medium and can be found in every type of galaxies but remarkably noticed in spiral galaxies (see [4] and references therein). For instance, Milky Way has been actively studied in its three regions (central bulge, halo, and accretion disk). This motivates obtaining a proper description of magnetic fields from an oriented general principle and relativistic thin disks have been revealed as one of the best ways to study them. Relativistic disks were also extensively studied in literature in several configurations. Exact solutions that have relativistic static thin disks as their sources were first studied by Bonnor and Sackfield [5] and T. Morgan and L. Morgan [6, 7]. Subsequently, several classes of exact solutions corresponding to static [8–17] and stationary [18–22] thin disks have been obtained by different authors.The superposition of a static or stationary thin disk with a black hole has been considered in [23–31]. Thin disks around static black holes in a magnetic field have been studied in [32]. Relativistic disks embedded in an expanding Friedmann-Lemaître-Robertson-Walker universe have been studied in [33] and perfect fluid disks with halos in [34]. Furthermore, the stability of thin disks models has been investigated using a first-order perturbation of the energy-momentum tensor in [35]. On the other hand, thin disks have been discussed as sources for Kerr-Newman fields [36, 37], magnetostatic axisymmetric fields [38, 39], and conformastatic and conformastationary metrics [40–42]. Also, models of electrovacuum static counterrotating dust disks were presented in [43], charged perfect fluid disks were studied in [44], and charged perfect fluid disks were presented as sources of static and Taub-NUT-type spacetimes in [45, 46]. Also, monopole and dipole layers in curved spacetimes were analyzed in [47] and electromagnetic sources distributed on shells in a Schwarzschild background in [48].The thin disks with magnetic fields studied in [36–38] were obtained by means of the well-known “displace, cut, and reflect” method. Solutions that can be interpreted as thin disks of finite extension can be obtained if an appropriate coordinate system is introduced. A coordinate system that adapts naturally to a finite source and presents the required discontinuous behavior is given by the spheroidal coordinates. Some examples of finite thin disks obtained from vacuum solutions expressed in these coordinates can be found in [5, 6, 9, 11] and from electrovacuum solutions in [42].Moreover, interestingly, magnetic fields seem to play an important role in the formation of jets (resulting from collimated bipolar outflows of relativistic particles) and the accretion disk near supermassive black holes [49]. A current revision of the status of our knowledge about the magnetic fields in our Milky Way and in nearby star-forming galaxies is summarized in [50]. Additionally, a study of the disk and halo rotation is reported in [51], whereas the possibility of magnetic fields that can be generated in the outskirts of disks is studied in [52]. Solutions for the Einstein and Einstein-Maxwell field equations which are consistently applicable to the context of astrophysics remain a topical problem. Nevertheless, the effects of magnetic fields on the physical processes in galaxies and their disk-halo interaction have been scarcely considered in the past. Similarly, the relevance of relativistic models of disks around black holes in a magnetic field is discussed in [32].The presence of the electric field on the dark matter halo models has been considered in [53], whereas the presence of electromagnetic field in the halo-disk system has been studied in [54, 55] in which the gravitational sources are statics. In [54] we provided detailed overview of the research in the relativistic disks; accordingly we will not repeat them here.In this paper, we do not focus on the whys and wherefores of the detailed discussion on the probes and relevance of magnetic fields on disks but we apply a standard galaxy modeling as a stationary thin disk and, correspondingly, we associate the halo with the region surrounding the disk. We present the conformastationary version of the static thin disk-halo systems studied in [54]. In addition, we study the features of the principal quantities characterizing the dynamic of the magnetized haloes corresponding to the disks presented in [56]. Therefore, we take the definition in [57] as standard, following the original terminology by Synge [58]: conformastationary are those stationary spacetimes with a conformally flat space of orbits.Accordingly, we show that the rotating disk-haloes with isotropic pressure, stress tensor, and heat flow generalize the static disk-haloes obtained in [54]. Our results are compatible with those presented in [53] on possible features of galactic halo. Moreover, the description of the motion of charged particles on disk is deduced and is in agreement with the results of the similar analysis discussed in [59]. As far as we know, this is the first relativistic model describing analytically the relativistic magnetized halo of a rotating disk.The paper is organized as follows. In Section2, the distributional Einstein-Maxwell equations for haloes surrounding thin disks are obtained. In Section 3 we obtain expressions, in terms of an arbitrary harmonic function, for the most important quantities characterizing the dynamic of the disk and halo. In Section 4 we first calculate quantities for harmonic function described by the generalized Kuzmin-disk potential. Then, we analyze the obtained results and calculate the constants of motion of the disk. Moreover, the description of the motion of a charged particle on the halo is shown in Section 5. Finally, we complete the paper with a discussion of the results in Section 6.


## 2. Exact Solutions for Relativistic Magnetized Haloes Surrounding Thin Disks

In this section we consider the conventional treatment of rotating galaxies modelled as a stationary thin disk and, correspondingly, we associate the magnetized halo with the region surrounding the disk. This is motivated from the fact that the magnetic field is remarkably noticed on spiral galaxies and can play a fundamental role in formation of arms. To do so, we formulate the distributional Einstein-Maxwell field equations assuming axial symmetry [60]. We also suppose that the derivatives of the metric and electromagnetic potential across the disk space-like hypersurface are discontinuous. To formulate the corresponding distributional form of the Einstein-Maxwell field equations, we introduce the usual cylindrical coordinates xα=(t,r,z,φ) and assume that there exists an infinitesimally thin disk located at the hypersurface z=0. Accordingly, we identify the halo surrounding the disk with the positive (z≥0) and negative (z≤0) regions around the equatorial plane z=0, denoted here by the superscripts “±,” so that the metric and the electromagnetic potential can be written, respectively, as gαβ=gαβ+θ(z)+gαβ-{1-θ(z)} and Aα=Aα+θ(z)+Aα-{1-θ(z)}. Here θ(z) denotes the Heaviside distribution. As a consequence, the Ricci tensor reads(1)Rαβ=Rαβ+θz+Rαβ-1-θz+Hαβδz,where δ(z) is the Dirac distribution and(2)Hαβ=12γαzδβz+γβzδαz-γμμδαzδβz-gzzγαβ, with γαβ=2gαβ,z and all the quantities are evaluated at z=0+. In agreement with (1) the energy-momentum tensor and the electric current density acquire the form(3a)Tαβ=Tαβ+θz+Tαβ-1-θz+Qαβδz,(3b)Jα=Jα+θz+Jα-1-θz+Iαδz,where Tαβ± and Jα± are, respectively, the energy-momentum tensors and electric current density of halo. Moreover, Qαβ and Iα represent the part of the energy-momentum tensor and the electric current density of disk. The energy-momentum tensor Tαβ± in (3a) is taken to be the sum of two distributional components, the purely electromagnetic (trace-free) part and a “material” (trace) part:(4)Tαβ±=Eαβ±+Mαβ±,where Eαβ± is the electromagnetic energy-momentum tensor(5)Eαβ=FανFβν-14gαβFμνFμν,with Fαβ=Aβ,α-Aα,β and Mαβ± is an unknown “material” energy-momentum tensor to be obtained. Accordingly, the Einstein-Maxwell equations, in geometrized units such that c=8πG=μ0=ϵ0=1, are equivalent to the system of equations(6a)Gαβ±=Rαβ±-12gαβR±=Eαβ±+Mαβ±,(6b)Hαβ-12gαβH=Qαβ,(6c)F±αβ;β=J±α,(6d)Fαβnβ=Iα,where H≡gαβHαβ, and semicolon “;” in the index indicates the covariant derivative with respect to the metric. The square brackets in expressions such as [Fαβ] denote the jump of Fαβ across the surface z=0 and nβ denotes a unitary vector in the direction normal to it. To obtain a solution of the Einstein-Maxwell equations describing a system composed of a magnetized halo surrounding a rotating thin disk we will restrict ourselves to the case where the electric potential At=0.To solve the Einstein-Maxwell equations (6a), (6b), (6c), and (6d) we assume the conformastationary spacetime given by the line element(7)ds2=-e2ϕdt+ωdφ2+e-2βϕdr2+dz2+r2dφ2, where ϕ depends only on r and z and β is an arbitrary real constant. We also assume that the magnetic potential Aφ is time independent. Accordingly, by computing the Einstein tensor Gαβ explicitly from line element (7) and electromagnetic energy-momentum tensor (5), we obtain for the nonzero components of the energy-momentum tensor of the halo (EMTH) Mαβ±=Eαβ±-Gαβ±:(8a)Mtt±=-e21+βϕβ2∇ϕ·∇ϕ-2β∇2ϕ+12r-2e2βϕ∇Aφ·∇Aφ-34r-2e21+βϕ∇ω·∇ω,(8b)Mtφ±=e21+βϕβ2∇ω·∇ϕ+34r-2e21+βϕω∇ω·∇ω-β2ω∇ϕ·∇ϕ+2βω∇2ϕ+32∇ω·∇ϕ-12r-2e2βϕω∇Aφ·∇Aφ+12∇2ω-r-1∇ω·∇r,(8c)Mrr±=1-β∇2ϕ-1-βϕ,rr+β2-2βϕ,r2+ϕ,z2-12r-2e2βϕAφ,r2-Aφ,z2+14r-2e21+βϕω,r2-ω,z2,(8d)Mrz±=12r-2e21+βϕω,rω,z-1-β2+2βϕ,rϕ,z-1-βϕ,rz-r-2e2βϕAφ,rAφ,z,(8e)Mzz±=-14r-2e21+βϕω,r2-ω,z2+ϕ,r2-1-βϕ,zz+1-β∇2ϕ+β2-2βϕ,z2+12r-2e2βϕAφ,r2-Aφ,z2,(8f)Mφφ±=r2∇ϕ·∇ϕ+1-βr2∇2ϕ-1-βr∇ϕ·∇r-12e2βϕ∇Aφ·∇Aφ+e21+βϕ141+3r-2e2βϕω2∇ω·∇ω-β2ω2∇ϕ·∇ϕ+2βω2∇2ϕ+ω∇2ω-2r-1ω∇ω·∇r+3+βω∇ω·∇ϕ-12r-2e2βϕω2∇Aφ·∇Aφ.Moreover, from (6c) the nonzero components of the electric current density on the halo have the form(9a)J±t=e-1-3βϕ∇·ωr-2e1+βϕ∇Aφ,(9b)J±φ=e-1-3βϕ∇·r-2e1+βϕ∇Aφ,where all the quantities depend on r and z.The discontinuity in thez-direction of Qαβ and Jα defines, respectively, the surface energy-momentum tensor (SEMT) Sαβ and the surface electric current density (SECD) Jα of the disk, more precisely(10a)Sαβ≡∫Qαβδzdsn=gzzQαβ,(10b)Jα≡∫Iαδzdsn=gzzIα,where dsn=gzzdz is the “physical measure” of length in the direction normal to the z=0 surface. Accordingly, for metric (7), the nonzero components of Sαβ and Jα are given by(11a)Stt=4βe2+βϕϕ,z,(11b)Stφ=e2+βϕ4βωϕ,z+ω,z,(11c)Srr=21-βe-βϕϕ,z,(11d)Sφφ=e2+βϕ4βω2+21-βr2e-21+βϕϕ,z+2ωω,z,(12a)Jt=r-2e3βϕωAφ,z,(12b)Jφ=-r-2e3βϕAφ,z,respectively. Note that in (11a), (11b), (11c), and (11d) and (12a) and (12b) all the quantities are evaluated on the surface of the disk (z=0).In order to reduce the complexity of the last field equation systems we assume that the halo’s electric current density vanishes (i.e.,J±t=J±φ=0 in (9a) and (9b)), and it turns out that the magnetic potential and the metric functions ϕ and ω become completely determined in terms of an arbitrary harmonic function U(r,z) as follows (see [54, 56] for more details):(13a)Aφ,r=-1krU,z,(13b)Aφ,z=1krU,r,(13c)β+1ϕ=-ln⁡1-U,(13d)ω=kωU, with k and kω arbitrary constants. Since the nonzero components of the EMTD and EMTH and the electric current density directly depend on the metric functions and magnetic potential, we observe that the entire solution is determined by a single harmonic function.


## 3. Exact Relativistic Model for Magnetized Disk-Haloes

So far, by using the inverse method and the distributional formulation of the Einstein-Maxwell equations, we have obtained the separate energy-momentum tensor of the disk and halo. In addition, we have discussed a method to determine its components in terms of an arbitrary harmonic function. Now, the behavior of the energy-momentum tensors obtained must be investigated to find what conditions must be imposed on the solutions and the parameters that appear in the disk-haloes models in such a way that it can describe reasonably physical sources. We will now study the possible features of the disk by assuming that it is possible to express its energy-momentum tensor in the canonical form:(14)Sαβ=μ+PVαVβ+Pgαβ+QαVβ+QβVα+Παβ, where QαVα=QαVα=0, α=(t,r,φ), and all the quantities are evaluated in z=0+. Similarly, we assume that it is possible to express the energy-momentum tensor of the halo in the canonical form:(15)Mαβ±=μ±+P±VαVβ+P±gαβ+Qα±Vβ+Qβ±Vα+Παβ±, where Qα±Vα=Q±αVα=0, α=(t,r,z,φ), and all the quantities depend on r and z. Consequently, we can say that the disk and halo are constituted by some mass-energy distributions described by the energy-momentum tensors (14) and (15), respectively. Vα is the four-velocity of a certain observer. Correspondingly, μ, P, Qα, and Παβ are then the energy density, the isotropic pressure, the heat flux, and the anisotropic tensor on the surface of the disk. Analogously, μ±, P±, Qα±, and Παβ± are then the energy density, the isotropic pressure, the heat flux, and the anisotropic tensor on the halo, respectively. Thus, it is straightforward to see that for the halo we have(16a)μ±=Mαβ±VαVβ,(16b)P±=13HαβMαβ±,(16c)Qα±=-μ±Vα-Mαβ±Vβ,(16d)Παβ±=HαμHβνMμν±-P±Hμν,where the projection tensor is defined by Hμν≡gμν+VμVν and all the quantities depend on r and z, whereas for the disk we have(17a)μ=SαβVαVβ,(17b)P=13HαβSαβ,(17c)Qα=-μVα-SαβVβ,(17d)Παβ=HαμHβνSμν-PHμν, where all the quantities are evaluated in z=0+. It is easy to note that by choosing the angular velocity to be zero in (A.7) we have then a fluid comoving in our coordinates system. Hence, we may introduce a suitable reference frame in terms of the local observers tetrads (A.3a), (A.3b), (A.3c), and (A.3d) and (A.4a), (A.4b), (A.4c), and (A.4d) in the form(18)Vα,Iα,Kα,Yα≡htα,hrα,hzα,hφα,with the corresponding dual tetrad(19)Vα,Iα,Kα,Yα≡-htα,hrα,hzα,hφα. Since the SECD of the disk Jα can be also written in the canonical form Jα=σVα+jYα, σ can be interpreted as the surface electric charge density and j as the “current of magnetization” of the disk. A direct calculation shows that the surface electric charge density σ=0, whereas the “current of magnetization” of the disk is given by j=-r-1e2βϕAφ,z, where, as above, Aφ,z denotes the jump of the z-derivative of the magnetic potential across the disk and, all quantities are evaluated on the disk.By using the results obtained in the precedent section, we can write the surface energy density of the disk and the energy density of the halo can written as(20)μr=4βU,zβ+11-U2β+1/β+1,(21)μ±r,z=U,r2+U,z2e21+2βϕ1+β2r22β+β2r2-1+β22k2r2e-2ϕ+3kω21+β24,respectively. Moreover, we have a barotropic equation of state on the surface of the disk, which can be given by P(r)=ημ, with η=(1-β)/3β, in such a way that we can use the energy conditions and the causality requirement for the speed of sound on the disk to obtain the physical range of possible values of the parameter β. Analogously, the pressure of the halo is as follow: P±(r,z)=Θμ±(r,z), where(22)Θ≔4-2β-β2r2-1+β2/2k2r2e-2ϕ+kω21+β2/41+3kω2r-2U2e2βϕ1-e2ϕ32β+β2r2-1+β2/2k2r2e-2ϕ+3kω21+β2/4, in such a way that the pressure of the halo depends not only on the energy density but also on the gravitational and magnetic fields through the function Θ. The heat function of the disk is given by(23)Qαr=-kωU,z1-Uδαφ.Similarly, by inserting (15) into (16a), (16b), (16c), and (16d) we obtain for the heat flux of the halo(24)Qα±=kωe1+2βϕ21+βr21+βU,r-3+βrU,r2+U,z2e1+βϕδαφ.The nonzero components of the anisotropic tensor of the disk read Πφφ(r)=r2Πrr(r), where(25)Πrrr=21-βU,z31+β1-U1/1+β. Moreover, it is easy to see that the anisotropic tensor of the halo reads(26)Παβ±=Pr±IαIβ+Pz±KαKβ+Pφ±YαYβ+2PT±IαKβ, where, 2IαKβ=IαKβ+IβKα, as in the usual manner and(27)Pr±=e2βϕΠrr±,Pz±=e2βϕΠzz±,Pφ±=e2βϕr2Πφφ±,PT±=e2βϕΠrz±,(28a)Πrr±=e21+βϕ31+β2r2kω21+β22+21+β2k2r2e-2ϕ-41+β-β2r2-3kω41+β24r-2U2e2βϕ1-e2ϕUr2+-kω21+β2-1+β2k2r2e-2ϕ+21+β-β2r2-3kω41+β24r-2U2e2βϕ1-e2ϕUz2-31-β2r2e-1+βϕU,rr,(28b)Πzz±=e21+βϕ31+β2r2-kω21+β2-1+β2k2r2e-2ϕ+21+β-β2r2-3kω41+β24r-2U2e2βϕ1-e2ϕUr2+kω21+β22+21+β2k2r2e-2ϕ-41+β-β2r2-3kω41+β24r-2U2e2βϕ1-e2ϕUz2-31-β2r2e-1+βϕU,zz,(28c)Πφφ±=U,r2+U,z2e21+βϕ31+β221+β-β2r2-1+β2k2r2e-2ϕ+kω21+β221+3kω2r-2U2e2βϕ1-e2ϕ-1-β1+βre1+βϕU,r,(28d)Πrz±=e21+βϕ1+β2-21+β-β2+1+β2k2e-2ϕ+kω21+β22r2U,rU,z-1-β2e-1+βϕU,rz.Notice that P±≡Pr±+Pz±+Pφ±=0 and, consequently, the trace Π±αα=0. We have obtained expressions for the energy, pressure, and the other quantities characterizing the dynamic of the halo. All the dynamic quantities have been expressed in terms of an arbitrary U(r,z) harmonic function. Finally, as we know, the electric current density of the halo is zero whereas it is easy to note that the magnetization current density on surface of the disk is(29)jr=-U,rk1-U3β/1+β.It is important to remark thatkω is a defining constant in (23) and (24). Indeed, when kω=0 the heat flux functions Qα and Qα± vanish, a feature of the static systems. Because we used the inverse method, no “a priori” restriction is imposed on the physical properties of the material constituting the disk and halo. The nonzero components of the energy-momentum tensors of the disk and halo result from “the nature” of the chosen metric and the corresponding solutions. So, in our case, the nonzero components Srr and Stφ are conditioned by the parameter β and the metric function ω in such a way that when β=1 the component Srr vanishes, whereas Stφ=0 when ω vanishes. The decomposition of the energy-momentum tensor of the disk-halo system into (14) and (15) was chosen with the aim of describing the SEMT and EMTH by the more general fluid model. Hence, the heat flux appears here in a “natural” way as a function determined by the metric function ω and, consequently, by the “rotation.” Unfortunately, as we can see from (17c) and (16c), this function is oriented along the closed circular orbits and thus its physical interpretation is unclear. It is an issue that remains unanswered in this paper but should be addressed in the future.


## 4. Rotating Kuzmin-Like Disk with Magnetized Haloes

As an example of application of the formalism described in the precedent sections, we now consider the magnetized haloes surrounding the rotating disks generated by a generalization of the Kuzmin-disk potential in the form [57, 61](30)U=-∑n=0NbnPnz/RRn+1,PnzR=-1nRn+1n!∂n∂zn1R, where Pn=Pn(z/R) is the Legendre polynomial in cylindrical coordinates that was derived in the present form by a direct comparison of the Legendre polynomial expansion of the generating function with a Taylor series expansion of 1/R [62], being R2≡r2+z2 and bn arbitrary constant coefficients. The corresponding magnetic potential, obtained from (13a) and (13b), is(31)Aφ=-1k∑n=0Nbn-1nn!∂n∂znzR, where we have imposed Aφ(0,z)=0 in order to preserve the regularity of the axis of symmetry. Next, to introduce the corresponding discontinuity in the first-order derivatives of the metric potential and the magnetic potential required to define the disk we perform the transformation z→|z|+a. It is worth noting that, for the two first members of the family of solutions (N=0 and N=1) we have(32a)U0=-b~0r~2+z~+12,(32b)A~φ0=-b~0z~+1kr~2+z~+12,(33a)A~φ1=-b~0z~+1kr~2+z~+121-b~1r~2b~0z~+1z~+12+r~2,(33b)U1=-b~0r~2+z~+121+b~1z~+1b~0z~+12+r~2,respectively, where b~0=b0/a and b~1=b1/a2 whereas r~=r/a and z~=z/a; moreover A~φ=Aφ/a. For the two first members of the family of solutions the surface energy density of the disks can be written as(34)μ~0=4βb~01+βr~2+1β+2/2β+2b~0+r~2+12β+1/β+1,(35)μ~1=4βb~0-b~1r~2+b~0+2b~11+βr~2+12-β/2β+2r~2+13/2+b~0r~2+1+b~12β+1/β+1,respectively. Similarly, for the two first members of the family we have the heat flux of the disks(36a)Qα0=b~0kωδαφr~2+1+b~0,(36b)Qα1=kωδαφb~0r~2+1+b~1r~2+13/2+b~0r~2+1+b~1,and the corresponding anisotropic tensor(37a)Π~rr0=21-βb~031+βr~2+1+b~01/1+βr~2+13β+2/2+2β,(37b)Π~rr1=21-βb~0-b~1r~2+b~0+2b~131+βr~2+13/2+b~0r~2+1+b~11/1+βr~2+15β+2/2+2β.As we know, other quantities are P=(1-β)μ/(3β) and Πφφ=r2Πrr. In the last expressions we have used the dimensionless expressions μ~=aμ, Π~φφ=aΠrr. Finally, for the two first members of the family we have the current of magnetization as(38a)j0~=-2b~0r~kr~2+13+β/2+2βb~0+r~2+12β/β+1,(38b)j1~=-2r~b~0r~2+1+3b~1kr~2+15-β/2+2βr~2+13/2+b~0r~2+1+b~12β/1+β,where j~=aj and we first have assumed that the z-derivative of the magnetic potential presents a finite discontinuity through the disk. In fact, as we have said above, the derivatives of U and Aφ are continuous functions across the surface of the disk. We artificially introduce the discontinuity through the transformation z→|z|+a.It is worth noticing that the mass surface density as well as the isotropic pressure of the disk decays very rapidly (as1/r3 and 1/r5 for N=0 and N=1, resp.) indicating that the above solution can be associated with a disk with a finite energy-momentum distribution. In every case, the characteristic size can be adjusted through the parameters b0 and b1 of the solutions. Moreover, a simple calculation of the curvature invariants reveals that the solution is asymptotically flat and singularity-free.To illustrate the results corresponding to the principal quantities describing the halo in Figure1, we show the behavior of energy densities μ± on the halo as a function of r and z. In each case, we plot μ0±(r,z) (Figure 1(a)) and μ1±(r,z) (Figure 1(b)) for the indicated values of the parameters. It can be seen that the energy density is everywhere positive and vanishes sufficiently fast as r increases.Figure 1
Surface plots of the energy densities (a)μ0± and (b) μ1± on the halo as functions depending on r and z with parameters a=b0=b1=k=kω=1 and β=0.75.
(a)
(b)In Figure2, we show the behavior of pressure P± on the halo as a function of r and z. In each case, we plot P0±(r,z) (Figure 2(a)) and P1±(r,z) (Figure 2(b)) for the indicated values of the parameters. We can see that pressure is always positive and behaves as the energy density of the halo. Thus, we can see that the behavior of these quantities is in agreement with the results published in [53]. Moreover, we also computed these functions for other values of the parameters within the allowed range and in all cases we have found a similar behavior.Figure 2
Surface plots of the pressures (a)P0± and (b) P1± on the halo as functions depending on r and z with parameters a=b0=b1=k=kω=1 and β=0.75.
(a)
(b)


### 4.1. The Constants of Motion

To proceed further, we evaluate the constants of motion. Therefore, from (13c) we have(39)ϕ=11+βln⁡11-U.Then, for solution (32a) we may write(40)ϕ0=11+βln⁡R~2+2z~+1R~2+2z~+1+b~0,where R~2≡r~2+z~2. This follows that the metric potentials gtt and gtφ for R→∞ in the disk (z=0) become(41a)gtt≃-1+2b~01+βR~-b~023+β1+β2R~2+O1R~3,(41b)gtφ≃kωb~0R~-2kωb~021+βR~2+O1R~3.This implies, as is well known (see [41]), that the total mass-energy of spacetime associated with the disk is(42)M0=b01+β. On the other hand, in (x,y,z) coordinates we find that(43a)g01≃-kωb~0yR~3+O1R~4,(43b)g02≃kωb~0xR~3+O1R~4,(43c)g03≃O1R~4.As an application, we use the same procedure as in [63] and see that the angular momentum LM0 is in the z-direction and is given by(44)LM0=12kωb0. According to (32b) the magnetic field is(45)B0=-b~0r~kR~2+2z~+13/2r~er+z~+z~z~ez, where eα are unit basis vectors in cylindrical coordinates. Accordingly, by expressing the components of the magnetic field in Cartesian coordinates and taking the limit as R→∞ of B0(x,y,z) and by using formula (44.4) of Landau and Lifshits [64] we may conclude that the magnetic momentum may be written as(46)LB0=b0k. We thus see that constants k and kω define the gyromagnetic ratio LM0/LB0=(kkω)/2.


## 4.1. The Constants of Motion

To proceed further, we evaluate the constants of motion. Therefore, from (13c) we have(39)ϕ=11+βln⁡11-U.Then, for solution (32a) we may write(40)ϕ0=11+βln⁡R~2+2z~+1R~2+2z~+1+b~0,where R~2≡r~2+z~2. This follows that the metric potentials gtt and gtφ for R→∞ in the disk (z=0) become(41a)gtt≃-1+2b~01+βR~-b~023+β1+β2R~2+O1R~3,(41b)gtφ≃kωb~0R~-2kωb~021+βR~2+O1R~3.This implies, as is well known (see [41]), that the total mass-energy of spacetime associated with the disk is(42)M0=b01+β. On the other hand, in (x,y,z) coordinates we find that(43a)g01≃-kωb~0yR~3+O1R~4,(43b)g02≃kωb~0xR~3+O1R~4,(43c)g03≃O1R~4.As an application, we use the same procedure as in [63] and see that the angular momentum LM0 is in the z-direction and is given by(44)LM0=12kωb0. According to (32b) the magnetic field is(45)B0=-b~0r~kR~2+2z~+13/2r~er+z~+z~z~ez, where eα are unit basis vectors in cylindrical coordinates. Accordingly, by expressing the components of the magnetic field in Cartesian coordinates and taking the limit as R→∞ of B0(x,y,z) and by using formula (44.4) of Landau and Lifshits [64] we may conclude that the magnetic momentum may be written as(46)LB0=b0k. We thus see that constants k and kω define the gyromagnetic ratio LM0/LB0=(kkω)/2.


## 5. Motion of a Charged Test Particle in the Halo

The motion of a test particle of chargee and mass m moving in the halo is described by the following Lagrangian density:(47)L=12gαβvαvβ+emAαxα,where gαβ and Aα are, respectively, the components of the metric and electromagnetic potential, given here by (13a), (13b), (13c), and (13d).The equations of motion of the test particle can be derived from (47) by using the Euler-Lagrange equation. Then,(48)dvαds+Γβγαvβvγ=emgαμFμλvλ. The velocity of the particle as measured by the local observers is given by vα=vt(tα+Ωφα), where(49)vt=1-U1/1+β1+kωUΩ1-v2. Here, the 3-velocity v and the angular velocity Ω of the particle as measured by the local observers are given by(50)v=rΩ1-U1+kωUΩ,(51)Ω=kωU,r2+U,z21+β+2U/1-U±U,r2+U,z2D21+βr1-U2U,r-2U,r2+U,z2A,D=41+βr1-UU,r+U,r2+U,z2kω21+β2-4βr2,A=βr21-U+kω2U1+β+U1-U, respectively. All the quantities depend on r and z. In Figures 3(a) and 4(a) we show the behavior of the velocities v02 and v12 of a charged particle following “magnetogeodesic” motion on the halo for the values of indicated parameters, respectively. Additionally, in Figures 3(b) and 4(b), we plot the z-slices of the surface plot of the velocity and v02 and v12 for the indicated values of the parameters, respectively. These curves are obtained via vertical slices of the surface v2=v2(r,z) (a vertical slice is a curve formed by the intersection of the surface v2=v2(r,z) with the vertical planes). For each curve, we can see that the velocity is always less than 1, its maximum occurs around r=0, and it vanishes sufficiently fast as r increases. It can also be observed that the maximum of the velocity decreases as the values of z increase. We also computed these functions for other values of the parameters within the allowed range and in all cases we found a similar behavior. Naturally, the description of the motion of charged particles on disk here deduced is in agreement with the results of analysis of the magnetogeodesic motion of the particle in the magnetized disks discussed in [59].Figure 3
Surface plot of the velocity (a)v02 and z-slices of the surface plot of the velocity (b) on the halo as functions depending on r and z with parameters a=b0=b1=k=kω=1 and β=0.75.
(a)
(b)Figure 4
Surface plot of the velocity (a)v12 and z-slices of the surface plot of the velocity (b) on the halo as functions depending on r and z with parameters a=b0=b1=k=kω=1 and β=0.75.
(a)
(b)


## 6. Conclusions

We used the formalism presented in [54] to model an exact relativistic rotating disk surrounded by a magnetized halo. The model was obtained by solving the Einstein-Maxwell distributional field equations. In doing so, we introduced an auxiliary harmonic function that determines the functional dependence of the metric components and the electromagnetic potential. Accordingly, we separated the total energy-momentum tensor of the system disk-halo. Additionally, we expressed the energy-momentum tensor of the halo as a sum of two distributional contributions, one due to the electromagnetic part and the other due to a material part. As we can see, because the spacetime here considered is nonstatic (conformastationary), the distributional approach of the Einstein-Maxwell equations allows us to work with a strongly nonlineal partial equations system. We considered, for simplicity, the astrophysical consistent case in that there is no electric charge on the halo. We obtained that the charge density on the disk is zero.In order to analyze the physical content of the energy-momentum tensor of the halo and disk, we projected each tensor, in the canonical form, in the comoving frame defined by the local observers tetrad. This analysis allowed us to give a complete dynamical description of the system in terms of two parameters (i.e.,β and kω) which determine the matter content of the sources. Indeed, the parameter β in the metric vanishes when it is equal to the isotropic pressure and the anisotropic tensor on the material constituting the disk. Similarly, when the parameter kω is equal to zero the heat flux on the disk and halo vanishes, a feature of the static systems. So, in this paper we presented, for first time, the complete analysis of the most general energy-momentum tensor of a disk-haloes system obtained from exact conformastationary axially symmetric solutions of the Einstein-Maxwell equations.The expressions obtained here are the generalization of the expressions obtained for the conformastatic disk-haloes without isotropic pressure, stress tensor, or heat flow presented in [54]. Moreover, when we take simultaneously kω=0 and β=1, we obtain the corresponding electrized disk-haloes version. Furthermore, our results are compatible with the description of the relativistic models of perfect fluid disks in a magnetic field presented in [59] and the halo presented in [53]. Furthermore, we have shown that the description of the motion of charged particles on the disk is in agreement with the results of analysis of particles motion in the magnetized disks discussed in [59]. In accordance with the results presented in [53, 65], it is also worth noticing that one can fix the values of the parameters β, kω, and bn as well as the number of members of the particular solutions presented here in order to have velocity increasing linearly with radius of the disk.We have considered specific solutions in which the gravitational and magnetic potential are completely determined by a “generalization” of the Kuzmin-disk potential. Accordingly, we have generated relativistic exact solutions for magnetized haloes surrounding rotating disks from a Newtonian gravitational potential of a static axisymmetric distribution of matter. The solution obtained is asymptotically Minkowskian in general and turns out to be free of singularities.In short, we concluded that we have presented a well-behaved exact general relativistic rotating disk surrounded by a well-behaved magnetized “material” halo. In our description we do not impose restriction on the kind of “material” constituting the system disk-halo. Consequently, we can speculate that the halo could be made of magnetized dark matter. This work provides a solid footing to refine future studies of relativistic disk-haloes systems and applications, for example, relativistic generalization of alpha-effect which will be discussed somewhere.



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*Source: 916026-2015-12-10.xml*