Solitary plasma rings and magnetic field generation involving gravity and differential rotation
Consorzio Interuniversitario per la Fisica dello Spazio,
10133
Torino,
Italy
email: coppi@mit.edu
Received:
14
October
2011
Accepted:
4
October
2012
A new theoretical framework for describing how magnetic fields are generated and amplified is provided by finding magnetogravitational modes that involve gravity, density gradients, and differential rotation in an essential way. Other factors, such as the presence of a high temperature particle population or of a temperature gradient, can contribute to their excitation. These modes identified by a linearized analysis are shown to be important for the evolution of plasma disks surrounding black holes toward different configurations. Since the nonlinear development of these modes can lead to radially localized regions with a relatively small differential rotation, new stationary structures have been identified, in the (fully) nonlinear limit, which are localized radially over regions with negligible gradients of the rotation frequency. These structures, characterized by solitary plasma rings, do not involve a preexisting “seed” magnetic field, unlike other configurations found previously. The relevant magnetic energy density is comparable to the gravitationally confined plasma pressure. The “source” of these configurations is the combination of the gravitational force and of the plasma density gradient orthogonal to it that is an important factor in the theory of magnetogravitational modes, another important factor being an anisotropy of the plasma pressure.
Key words: plasmas / magnetohydrodynamics (MHD) / instabilities / black hole physics
© ESO, 2012
1. Introduction
The investigations undertaken with the purpose of identifying the plasma and field configurations around black holes have led to envisioning a clear sequence of processes and a theoretical framework for generating and amplifying significant magnetic fields in the Universe. The relevant physical factors for these processes are both the plasma differential rotation and the (vector) product of the gravitational force and of the orthognal density gradient. In particular, starting from a “conventional” disk surrounding a compact object in which a “seed” magnetic field is present, magnetogravitational modes, which can be excited and produce a rapid amplification of the field, are found. These modes, which are described by a linearized theory, can be axisymmetric or of the trailing spiral type with low toroidal mode numbers.
In particular, by adopting a fully nonlinear approach at first, stationary axisymmetric configurations are identified that can be regarded as the result of the nonlinear evolution of magnetogravitational modes. In particular, considering a region in which the rotation frequency gradient is small when compared to the Keplerian rotation frequency, solitary ring configurations are found that do not depend on the presence of a seed magnetic field. In fact, the local “flattening” of the rotation frequency can be envisioned to result from the excitation of a magnetogravitational mode as the “driving factor” of the identified nonlinear configurations is the (vector) product of the gravitational force and of the density gradient orthogonal to it. This analysis is followed by the complete linearized theory of the magnetogravitational modes emerging from a conventional disk configuration for which an important additional driving factor is the differential rotation of Keplerian orbits.
In this connection we mention that a large category of black holes can be referred to as “shining” in view of the highenergy radiation emission that can be associated with them. This emission is attributed to accretion of highenergy plasmas that surround these objects. However, this generic interpretation leads to opening a number of questions concerning both (i) the specific processes that can allow accretion to occur, or can prevent it as in the case of “dark” black holes, and (ii) the nature of the plasmas that can be involved. In fact, a fairly complete theoretical description of these plasmas would require consideration of the full phase space. A relevant observation is that Xray astronomy has shown that these plasmas can access characteristic “states”, on the basis of their radiation emission, which are nonthermal and correspond to nonMaxwellian distributions of the particle populations that are responsible for the emission. For the sake of simplicity, the analysis that is presented here adopts a single fluid description with an isotropic pressure tensor. In fact, the theory of nonlinear stationary configurations (e.g. solitary ring structures) and of the related magnetogravitational modes has been developed (Coppi 2012) for plasmas with two components, one of which has a higher longitudinal (to the magnetic field) pressure than that of the population with isotropic pressure. This theory will be the subject of a subsequent paper.
The present paper is organized as follows. In Sect. 2, the basic assumptions that are made in order to find nonlinear, stationary, and axisymmetric configurations of plasmas and magnetic fields are described. In Sect. 3 the master equation is derived from the total momentum conservation equation by assuming a scalar plasma pressure and relates the plasma density distribution to a consistent magnetic field configuration. In Sect. 4 two classes of radially localized configurations are introduced and the master equation for the locally differential rotator configurations is given. In Sect. 5 the main features of locally rigid rotor configurations are illustrated, the relevant form of the master equation is discussed, and the important fact is pointed out that a seed magnetic field does not appear in the theory for these configurations. In Sect. 6 the vertical momentum density balance equation is introduced. This relates the plasma pressure to the magnetic field configuration and is to be analyzed in combination with the master equation. In Sect. 7 a class of special solutions for the nonlinear equations introduced in earlier sections that are separable functions of the vertical and radial coordinates is identified. In Sect. 8 a solitary ring solution is found in the context of the locally differential rotor class of configurations. In Sect. 9 the periodic sequence of rings for the same class of configurations, and published earlier, is recovered. In Sect. 10 the master equation of the locally rigid rotor class of configurations is analyzed. In Sects. 11 and 12 a periodic ring sequence, as well as a solitary ring solution, are found for the same class of configurations. In Sect. 13 the basic equation describing the magnetogravitational modes in the linearized approximation is introduced. In Sect. 14 the spatial profiles and the growth rates of two different kinds of magnetogravitational modes are analyzed. Section 15 describes the tridimensional spiral configurations, which are of the ring type and were found earlier in the linearized approximation. Then nonlinear ring configurations with a corresponding spiral structure are identified. In Sect. 16 a theoretical framework is proposed in order to explain the generation of significant magnetic fields in the Universe by the combined effects of gravity, density gradient, differential rotation, and other factors. The excitation of magnetogravitational modes and the formation of locally rigid rotation configurations have the key role in this. In Sect. 17 final consideration is given to both the limitations of the presented theory and its envisioned developments.
2. Basic assumptions
Given the intent to identify the simplest stationary plasma and field configurations that can (theoretically) exist around compact collapsed objects such as black holes, we limit our analysis at first to axisymmetric geometries with the following characteristics:

a)
Perfectly conducting plasma conditions are considered and, consequently,(2.1)where V is the plasma flow velocity, is the magnetic surface function, and cylindrical coordinates are used.

b)
No appreciable poloidal flow velocity is included.

c)
The relevant particle distributions in velocity space are close to Maxwellian and refer to a scalar pressure (P = pI) is appropriate.

d)
The relevant Lorentz force does not have a toroidal component and, consequently, the corresponding magnetic field configurations are represented by (2.2)as, in this case, the Lorenz force F_{L} is given simply by (2.3)where (2.4)

e)
A Newtonian gravitational potential Φ_{G} is included for simplicity. In particular, for the relative thin plasma structures that we analyze, (2.5)where (2.6)and is the Keplerian frequency. We observe that when considering scale distances that are relatively close to black holes, we have found it convenient to make use of effective gravitational potentials in order to include relevant General Relativity effects in the theory (Coppi 2011).
3. Relevant form of the master equation
Referring to the total momentum conservation (3.1)we observe that (3.2)and (3.3)Therefore, we obtain the “master equation” (Coppi 2011) that relates ψ to ρ(3.4)We consider local plasma and field structures in an interval R − R_{0} < R_{0} around R − R_{0}, and we indicate the characteristic scale distance, over which R − R_{0} and z vary, by Δ_{R} and Δ_{z}, respectively. Here , for In particular, we consider ρ to be an even function of both R_{∗} and that is positive for all values of R_{∗} and .
4. Classes of local configurations
Now we consider two classes of local configurations
a) locally differential rotator configurations;
b) locally rigid rotator configurations.
In the first case we assume that a seed magnetic field B_{0}e_{z} is present corresponding to a magnetic surface function ψ_{0} ≃ B_{0}R_{0}R and referring to a surface function ψ ≃ ψ_{0} + ψ_{1} with ψ_{1} < ψ_{0}, but . Then we take α_{v} = 0 and (4.1)and define In this case considering the asymptotic limit where the master equation reduces to (4.2)where (4.3)Clearly the symmetries of this equation indicate that δΩ and therefore ψ_{1} have to be odd functions of R_{∗}. We observe that is the driving factor for the field configuration represented by ψ_{1}. Then we note that the scale distance Δ_{z} does not affect Eq. (4.2) in the limit where can be neglected, and in this case, it was analyzed earlier (Coppi & Rousseau 2006): (4.4)
5. Locally rigid rotor configurations
The locally rigid rotor configurations we consider are characterized by (5.1)then (5.2)We observe that an important property of this class of configurations is that the presence of a seed magnetic field is not required.
Clearly, the simplest case to analyze is that where B_{φ} = 0 and Ω(ψ) = Ω_{0}. Then the master Eq. (3.4) reduces to (5.3)As we can see from Eq. (5.3), (5.4)which corresponds to (5.5)If we consider that Δ_{z} could be comparable to Δ_{G} ~ v_{thi}/Ω_{K}, the height of a conventional thermal disk (see Sect. 6), then the magnetic energy density can be of the same order of magnitude as the plasma thermal energy density. The plasma pressures corresponding to the solution for ρ and ψ given by Eqs. (4.2) and (5.3) are obtained by the vertical momentum density conservation analyzed in Sect. 6.
We note that in this limit ψ can be either an odd or an even function of R_{∗} and an even or odd function of z. Clearly the driving factor of the relevant magnetic field configurations is the term (∇ρ × ∇Φ_{G})·e_{ϕ}, which is a combination of the gravitational force and the density gradient orthogonal to it.
6. Vertical momentum density conservation equation
The vertical equilibrium equation connects the total plasma pressure to the particle density and the magnetic field configuration. In particular, this equation can be written as (6.1)and we find it convenient to separate p into p_{G} + p_{M} where (6.2)Thus we may define the temperature (6.3)where m_{i} is the mass of the nuclei of which the plasma is composed and consider sufficiently high values of T_{G} such that p = p_{G} + p_{M} is always positive. A brief discussion of the profiles that can be present in a “conventional” disk is given in the appendix.
Clearly, (6.4)If we consider axisymmetric configurations for which I = I(ψ), this reduces to (6.5)Moreover if we assume that p_{M} = p_{M}(ψ),∂p_{M}/∂_{z} = (dp_{M}/dψ)∂ψ/∂zand we obtain the socalled “GS equation” for magnetically confined laboratory plasmas. In fact, the socalled “pulsar equation” describing the magnetic configuration of an axisymmetric plasma surrounding a rotating neutron star was derived first and solved along similar lines by Cohen et al. (1973).
In the present case we do not consider p_{M} = p_{M}(ψ), and have, for configurations localized around R = R_{0}, (6.6)In particular, if we introduce the dimensionless variables R_{∗} and , Eq. (6.6) becomes (6.7)
7. Factorized solutions
Now we limit our analysis to functions ψ, which can be factorized as (7.1)and Eq. (6.7) becomes (7.2)Therefore (7.3)Then we refer to Eq. (6.2), assume for simplicity that T_{G} = T_{G0} = constant, write (7.4)and define (7.5)Consequently, (7.6)The relationship between and will depend on the classes of solutions of the master equation that we consider. In particular, for the locally differentially rotator configurations we find (7.7)and for the locally rigid rotor configurations (7.8)We also observe that (7.9)and in the case where ψ ≃ ψ_{0} + ψ_{1}, we have (7.10)Therefore in the present case this component of p_{M} has the same zprofile as p_{G}.
8. Locally differential rotator configurations: solitary rings
A radially localized solution of the master Eq. (4.2) that involves a Gaussian function is (8.1)The expression for that we obtain in this case is (8.2)Requiring that . We observe that the profile (9.2) corresponds to a single ring when (8.3)Clearly, B_{R} ~ B_{z} when Δ_{R} ~ Δ_{z}. We note that, if we take ψ_{N} ~ ψ_{0} and , we have and if Δ_{R} ~ Δ_{z}, for v_{φ} = Ω_{k}R_{0} and .
Thus we may argue that the pair of rings collapses into one ring as (Δ_{R}/Δ_{z})^{2} is increased. The poloidal magnetic field components now are (8.4)and (8.5)thus the relevant magnetic surfaces exhibit two Opoints, at R_{∗} = ± 1 and . The current density J_{φ} becomes (8.6)and corresponds to opposite current channels for R_{∗} > 0 and R_{∗} < 0.
Now, if we refer to Eq. (7.3) where we take I = 0, we have (8.7)which is always negative for R^{2}_{∗} > 3. On the other hand, in this case (8.8)Therefore, (8.9)Clearly, for adequate values of p_{NG} the total plasma pressure can remain positive with a finite total temperature T for all values of and R_{∗}. We observe that the “complex” toroidal current density pattern represented by Eq. (8.6) is reminiscent of the one found for the modes identified in Coppi (2009).
We note that the complete magnetic surface function ψ is, in this case, (8.10)and we consider ψ_{N}/Δ_{R} > ψ_{0}/R_{0}. Therefore, the relevant magnetic surfaces are represented by (8.11)with ε_{z} < 1. A graphic representation of these surfaces is given in Fig. 1.
Fig. 1
Graphic representation of the magnetic surfaces for the configuration corresponding to Eq. (8.10). The curve with dotted heavy lines indicates the single ring density profiles represented by Eq. (8.2) for . 

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9. Periodic ring structures for locally differentially rotating configurations
These structures can be found in the limit where the ratio can be considered as negligibly small. Thus they may be viewed as having a “microscopic” radial modulation, while the kind of structure identified in Sect. 8 can have a “macroscopic” radial thickness on the order of Δ_{z}. In the present case case the Master Equation reduces to that derived already in (Coppi & Rousseau 2006), (9.1)and the considered solution is (9.2)leading to the following radial density profile (9.3)where the dimensionless parameter ε_{∗} ≤ 1/4. We observe that is the solution corresponding to ε_{∗} = 0 and to a vanishing modulated density ρ_{∗}.
Then the question that remains to be investigated is whether this periodic solution will survive when appreciable values for are considered and the assumption of separability cannot be maintained. Moreover, we observe that (9.4)and given the expression (7.6) for ρ if we take I^{2} ≲ (ψ/Δ_{R})^{2}, we have no evident problems with the expression for .
10. Master equation for locally rigid rotor configurations
Now we refer to the locally rigid rotor case and to the master Eq. (5.3). Considering the dependence of ψ on z indicated by Eq. (7.1), we note that in this case a more peaked expression for ρ is appropriate, that is (10.1)and that Eq. (5.3) becomes (10.2)Then we obtain, for , (10.3)Consequently, the relationship between ρ and ψ can be expressed as (10.4)Clearly, in the considered limit , (10.5)Therefore, (10.6)and if we require that (10.7)The relevant toroidal current density is about (10.8)
11. Rigidly rotating periodic magnetic field configurations
A particularly interesting set of field and plasma configurations that has not been looked for until now is the one for which the rotation frequencies are about constant in the region over which these configurations are radially localized. Thus we argued earlier that the development of these configurations may be considered as a candidate process for generating magnetic fields associated with the combined product of the gravitational force vertical component and of the local plasma density gradient.
In particular, we observe that the function sink_{∗}R_{∗} and cosk_{∗}R_{∗} are solutions of Eq. (10.3) for , as in this case, (11.1)Therefore, we may consider a periodic solution of the form (11.2)which, given Eq. (10.4), can lead to (11.3)
12. Rigidly rotating solitary rings
A solitary ring solution of the master Eq. (10.2) can be found that is compatible with a realistic profile of the plasma pressure represented by . In particular we rewrite Eq. (10.2) as (12.1)where we have taken (12.2)In addition, if we consider a configuration represented by (12.3)implying that and (12.4)we have (12.5)Then we rewrite Eq. (12.1) as (12.6)and define (12.7)which gives (12.8)To solve this equation we take (12.9)and obtain (12.10)Thus (12.11)and (12.12)In conclusion we may choose to consider the “ring” density profile, (12.13)To identify the radial temperature profile that corresponds to the solution represented by Eqs. (12.3) and (12.13), we refer to Eq. (7.3) and analyze the function (12.14)We note that (12.15)Consequently, (12.16)and (12.17)Therefore we can verify that the total temperature T_{G} + T_{M} can remain positive for all values of R_{∗}.
13. Magnetogravitational modes equation
We may now argue that the class of configurations treated in the previous sections should emerge as the fully nonlinear saturated stage of the magnetogravitational modes that we analyze in this section and in Sect. 14. These can be excited from a “conventional” disk configuration (Pringle 1981), and for their excitation they involve the product of the vertical gravitational force and the radial density gradient in addition to the differential rotation. One of these modes was identified in Coppi (2009) for a fairly extreme asymptotic limit. We note that, as in the case of the original magneto rotational instability (Velikhov 1959), the presence of seed (vertical) field, even if small, is essential for the onset of these modes.
The linearized equation that we use to describe magnetogravitational modes, for which both the differential rotation term and the gravitational term were of key importance, was derived in Coppi (2009). On the other hand, only a special class of solutions of this equation was considered. Therefore, without repeating the derivation we consider normal mode perturbations from the initial state, that is, a “conventional” currentless axisymmetric plasma disk, in which the gravity associated with the central object prevails, and the Keplerian velocity is the only one present. The relevant axisymmetric modes are represented by the perturbed toroidal velocity where R_{0} is a radial distance at which the modes are considered to be localized and . Moreover, are the other perturbed velocity components where, in particular, .
We indicate Fourier transform of by , and the relevant dispersion equation is (13.1)Here, modes that are vertically localized around z = 0 over distances smaller than H_{0}, for equilibrium density profiles represented by are considered, and the local equilibrium temperature gradient is included in the definition of (13.2)where η_{T} = (dlnT/dz^{2})/(dlnρ/dz^{2}). The temperature T is defined by p = 2nT and n = ρ/m_{i} where m_{i} is the ion mass. Clearly, the rhs of Eq. (13.1) vanishes if the local density and temperature gradients vanish. Moreover, where B_{z} is the seed vertical field, , in the sense that , and we assume . This corresponds to assuming that .
14. Magnetogravitational modes profiles and growth rates
Since it is convenient to deal with dimensionless variables we, define (14.1)Then we take and and the dispersion equation to be analyzed becomes (14.2)for .
Therefore if we consider rather flat or inverted temperature profiles, such that D_{N} > 0 and finite, we can find localized solutions around , where for . Around these points . Then we take , and. In this case around , Eq. (14.2) becomes (14.3)and has the solution where Σ^{2} ≡ (2ℰ_{0}/D_{N}) and . Consequently, we consider 2ℰ_{0} > D_{N}.
In general, such as, in the case where ℰ_{0} ~ 1, the asymptotic solution of Eq. (14.2) takes the form (14.4)for and for . Thus it will have a minimum at and two symmetric maxima before decaying for . To evaluate as a function of ℰ_{0}, we can make use of the quadratic form (14.5)where (14.6)considered as a variational principle for ℰ_{0} for given values of . In particular, the instability threshold can be evaluated from Eq. (14.5) by taking Γ_{0} ≡ 0.
If instead we refer to peaked temperature profiles such that we look for solutions to the equation (14.7)where ϵ_{N} ≪ 1, which are localized near . These take the form when Σ^{2} ≫ 1, requiring that D_{T}Σ^{2} = ℰ_{0} and . Thus , and we see that depends both on the temperature vertical gradient through D_{T} and the differential rotation through ℰ_{0}. Clearly this asymptotic form of the solution of Eq. (14.7) is valid for ℰ_{0}/D_{T} ≫ 1.
In general the relevant solution of Eq. (14.7) has a single maximum at and is only marginally stable for D_{T} = 0. In this case, the solution reported earlier in Coppi (2009) again takes of the form but with Σ^{2} = 1/ϵ_{N}, Σ = ℰ_{0}/(3ϵ_{N}) and . Moreover, if we consider both D_{T} and to be small, and in particular ,andwe have, and. More precisely, in this case takes the same form as in the case where D_{T} = 0, with Σ^{2} = 1/ϵ_{N}and but . Then, in the limit where ℰ_{0} ~ D_{T}/ϵ_{N} we find and Σ^{2} ~ ℰ_{0}D_{T} as expected.
15. Tridimensional ring configurations
Ring configurations have been found previously (Coppi 2009) on the basis of a linearized theory of tridimensional modes emerging from a “conventional” disk. In fact, these modes can be viewed as extensions of the linear modes discussed in the previous sections and can be represented by (15.1)We can see that the dependence of on is very similar to that of represented by Eq. (12.3). On the other hand Δ_{R} ≃ [(γ_{0}/Ω_{0})R_{0}/(k_{0}m_{φ})] ^{1/2}, where m_{φ} is the toroidal mode number, and clearly the finiteness of Δ_{R} depends on m_{φ} not being zero. In particular, the condition k_{R}m_{φ}dΩ_{k}/dR < 0 under which Eq. (15.1) is valid indicates that the relevant modes are trailing spirals.
When considering the configurations that can be identified by a nonlinear analysis, we may refer to the rings obtained in the rigid rotor limit (Sect. 12). Then we may take (15.2)where m_{φ} is a relatively low number, (15.3)and (15.4)Therefore ΔB_{p}/( Δψ/R) ≪ 1 and, to lowest order in this ratio, the analysis given in Sect. 12 should remain valid. We note, however, that J × B)_{φ} = J_{p} × ΔB_{p})_{φ} ≠ 0 in this case, where J_{p} is the poloidal current. Thus as expected, a configuration represented by Eq. (15.2) involves a torque that will have to be compensated for in order to have a steadystate configuration to order ΔB_{p}/B_{p}.
16. Theoretical outline for the generation of magnetic fields in the universe
On the basis of the linearized theory of the modes that are excited in a disk configuration and of the nonlinear structures, in particular rings, that can evolve from disks as a result of the development of these modes, we may give the following outline for the production of significant magnetic field through the dynamics of plasmas surrounding compact astrophysical objects such as black holes.

a)
Starting from a situation where no magnetic field ispresent, we may assume that nonthermal particle distributions, such as those with anisotropic pressures(p_{∥} ≠ p_{ ⊥ }), are produced. These distributions can give rise to instabilities that can produce “seed” magnetic fields of limited amplitudes and relatively short wavelengths.

b)
Assuming that these fields can interact to produce locally small fields with macroscopic wavelengths in the radial direction, magnetogravitational modes can then be excited under the combined effects of gravity the vertical plasma pressure gradient, the differential plasma rotation, and other factors.

c)
During the nonlinear evolution, the amplified magnetic field can become larger than the original seed field.

d)
The saturated state of the instability can be represented by one of the stationary nonlinear configurations of the type that is described in particular in Sect. 12, and for which the magnetic energy density becomes comparable with the plasma thermal energy density (pressure).
Therefore we can propose a new theoretical line of analysis that can lead to an explanation of the generation of significant magnetic fields in the Universe. Clearly, the main steps of this line should be compared with the dynamo theories that preceded it.
17. Concluding observations
A theoretical framework to explain the generation of magnetic fields in the Universe has been given on the basis of two clear findings. One is that of magnetogravitational modes that are driven by the combined effects of the product of the gravitational force, the plasma density gradients orthogonal to it, differential rotation, and other factors, when considering plasmas surrounding compact astrophysical objects such as black holes. The other is that of ring configurations by the relevant nonlinear analysis where the “driving factor” for the magnetic fields is the (vector) product of the gravitational force and the density gradient orthogonal to it. In the latter case, which can be envisioned as the result of the evolution of magnetogravitational modes with a ring structure into the nonlinear regime, no trace of a “seed” magnetic field is left in the relevant nonlinear theory and the magnetic field pressure comparable to the gravitationally confined plasma pressure. As pointed out in the main body of the paper, there are gaps to be filled, the most important being the nonlinear evolution of the appropriate magnetogravitational modes. The problem of identifying the simplest quasi stationary plasma configurations that can surround collapsed objects has led to limiting our attention to plasma regimes where the isorotation condition can be enforced, taking inspiration from the theory of equilibrium configurations developed for magnetically confined laboratory plasmas and extended to pulsar magnetospheres (Cohen et al. 1983).
In particular, the experimental observation of the socalled quasi periodic oscillations of Xray emission, in one of the radiation emission regimes associated with galactic black holes (Remillard & McClintock 2006), indicates that non axisymmetric configurations (Coppi & Rebusco 2008) have to be included in the evolution of relevant plasma structures. We note that “solitary rings” have been found earlier in the linearized approximation when considering spiral structures that can emerge from simple disk configurations (Coppi 2009). Now we have shown that structures of the same kind are found in the nonlinear limit as well.
Referring to axisymmetric configurations, the conditions under which separable solutions in the variable R − R_{0} and z can be found (Sect. 7) deserve to be scrutinized. Therefore, an adequate (Regev & Umurhan 2008) computational effort including the investigation of nonseparable solutions will have to be undertaken. Other issues to be dealt with are the connection between the fine scale structure of the plasma configurations around black holes and the grand distribution of currents and electromagnetic fields on the larger scale around them (Blandford 1976; Lovelace 1976), the accretion flows, the appearance of jets in certain regimes, and relevant global transport processes such as angular momentum (Shakura & Sunyaev 1973).
Moreover, we note that both the linear and nonlinear analyses that we reported here relied on the assumption that the particle distributions in momentum space are Maxwellian, so a scalar pressure can be defined. This is a serious limitation in view of the fact that there are important radiation regimes that have been observed experimentally (Remillard & McClintock 2003), and are associated with compact objects, such as galactic black holes. They are definitely nonthermal. The case where a population with a strongly anisotropic pressure has therefore been analyzed recently. This was in addition to a thermal population, one with an isotropic pressure, which is smaller than that of the high energy population in the direction of the magnetic field. The main results, which will be reported in a later paper, are that the pressure anisotropy (p_{∥} > p_{ ⊥ }) makes a significant new contribution to the growth rate of magnetogravitational modes and can produce a new kind of ring structures (Coppi 2012).
Acknowledgments
It is a pleasure to thank E. P. Velikhov for a series of stimulating conversations on magnetic field generation processes, A. Nekrasov for his timely and useful suggestions, T. Rabga for proposing Eq. (8.1) as a possible solution, P. Rebusco for her insightful questions, and T. Zhou for his work on the manuscript. The present work was sponsored in part by the US Department of Energy.
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Appendix A: Temperature and density vertical profiles for a “conventional” disk
Given the importance that the parameter η_{T} = (dlnT/dz)/(dlnρ/dz) has in the linearized theory of
magnetogravitational modes, we consider the vertical equilibrium equation that for B = B_{z} reduces to where ,,,,, and Consequently, and In particular, if we take we have ,η_{T} ≃ α_{T}/(1 − α_{T}) and.
All Figures
Fig. 1
Graphic representation of the magnetic surfaces for the configuration corresponding to Eq. (8.10). The curve with dotted heavy lines indicates the single ring density profiles represented by Eq. (8.2) for . 

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In the text 