Trapped, Two-Armed, Nearly Vertical Oscillations in Disks with Toroidal Magnetic Fields II: Effects of Finite Thickness

# Trapped, Two-Armed, Nearly Vertical Oscillations in Disks with Toroidal Magnetic Fields II: Effects of Finite Thickness

Shoji Kato 2-2-2 Shikanoda-Nishi, Ikoma-shi, Nara, 630-0114
###### Abstract

We examine radial trapping of two-armed () vertical p-mode oscillations in geometrically thin relativistic disks which are vertically isothermal but terminated at a certain height by the presence of hot and low-density corona. The disks are assumed to be subject to toroidal magnetic fields. The oscillations are classified by , a number related to the node number of oscillations in the vertical direction and starting from . In modes with , the frequencies of trapped oscillations depend little on the height of termination, but in modes with the frequencies decrease and the radial extends of trapped region become wide, as the termination height decreases. This study is a preparation to examine whether these oscillations can describe kilo-hertz quasi-periodic oscillations (kHz QPOs), horizontal branch oscillation (HBOs), and their correlations.

S. KatoDisk Oscillations in Vertically Terminated Disks \Received2010/00/00\Accepted2010/00/00

\KeyWords

accretion, accrection disks — quasi-periodic oscillations — neutron stars — two-armed disk oscillations — X-rays; stars

## 1 Introduction

Kilo-hertz quasi-periodic oscillations (kHz QPOs) observed in neutron-star low-mass X-ray binaries (NS LMXBs) are one of promising tools to investigate the innermost structure of relativistic disks and to evaluate the mass and spin of the central neutron stars. Although there is no general consensus on the origin of the kHz QPOs, one of promising origins is disk oscillations trapped in the innermost region of relativistic disks.

There are many disk oscillations which are trapped in the innermost relativistic disks (for review, see Wagoner 1999, Kato 2001, Kato et al. 2008). Recently, Kato (2010) showed that in addition the trapped oscillations reviewed in the above review works, two-armed vertical p-mode oscillations can also be trapped in the innermost region of disks with frequencies relevant to kHz QPOs. The characteristics of these two-armed oscillations were examined by Kato (2011a, paper I) in the case where the disks are subject to toroidal magnetic fields. Subsequently, Kato (2011b) showed that these oscillations can naturally describe the correlated frequency change of the twin kHz QPOs observed in neutron-star LMXBs.

In the above model of twin kHz QPOs, the frequency change of the QPOs are assumed to be due to time changes of acoustic and Alfvén speeds in disks. In addition to them, however, one more possible causes of frequency change will be conceivable. This is time change of vertical disk thickness. The time change of vertical disk thickness will be expected, since geometrically thin disks in LMXBs will be surrounded by hot corona and its transition height will vary with time by a change of evaporation efficiency by change of disk state. In this sense, it will be of interest to examine how the change of transition height affects the frequencies of trapped two-armed vertical p-mode oscillations.

Based on the above considerations, we examine in this paper the characteristics of two-armed () vertical p-mode oscillations in the case where the disks are vertically isothermal but terminated at a certain height by presence of hot low-density corona. Application of the results to observed frequency correlations of QPOs will be made in a subsequent paper (Kato 2012).

## 2 Unperturbed Disks and Equations Describing Disk Oscillations

The unperturbed disks are isothermal in the vertical direction. We assume that the disks are terminated at a certain height by the presence of a hot corona. When we consider oscillations, a revelant boundary condition is imposed at the height of transition between the disk and the corona, as will be discussed later. Except for this, the disks considered in this paper are the same as those considered by paper I. That is, the disks are geometrically thin and relativistic. For mathematical simplicity, however, the effects of general relativity are taken into account only when we consider radial distributions of , , and , which are, in turn, the angular velocity of disk rotation, the epicyclic frequencies in the radial and vertical directions. Except for them, the Newtonial formulations are adopted. Since geometrically thin disks are considered, , is approximated to be the relativistic Keplerian angular velocity, , when its numerical values are necessary. Here, is the radial coordinate of cylindrical ones (,,), where the -axis is perpendicular to the disk plane and its origin is the disk center. Functional forms of , , and are given in many literatures (e.g., Kato et al. 2008).

### 2.1 Unperturbed Disks with Toroidal Magnetic Fields

The equilibrium disks are axisymmetric and vertically isothermal with toroidal magnetic fields. The fields are assumed to be purely toroidal:

 \boldmathB0(r,z)=[0,B0(r,z),0], (1)

and distributed in such a way that the Alfvén speed, , is constant in the vertical direction, i.e., const. in the vertical direction, where is the density in the unperturbed disks.

Since both the isothermal acoustic speed, , and the Alfvén speed, , are constant in the vertical direction, the integration of the hydrostatic balance in the vertical direction gives (e.g., Kato et al. 1998)

 ρ0(r,z)=ρ00(r)exp(−z22H2),andB0(r,z)=B00(r)exp(−z24H2), (2)

where the scale height is related to , , and by

 H2(r)=c2s+c2A/2Ω2⊥. (3)

The ratio is a parameter describing the disk structure. It is a function of the radius in general, but in this paper it is taken to be constant throughout the trapped region of oscillations. This is because the trapped region is found to be narrow except for some cases where is large (see figure 7).

The disks described above are assumed to be terminated at a certain height, say , by a high-temperature and low-density corona. The ratio is one of parameters describing the disk, which is also assumed to be constant in the trapped region.

### 2.2 Equations Describing Disk Oscillations

Small amplitude perturbations are superposed on the equilibrium disk described above. The velocity perturbation over rotation is denoted by (, , ), and the perturbed part of magnetic field over the unperturbed one by (, , ).

The azimuthal and time dependences of the perturbed quantities are taken to be proportional to exp, where and are the frequency and the azimuthal wavenumber of perturbations, respectively. In this paper we are interested only in two-armed () oscillations, but is retained here and hereafter without specifying so that we can trace back the terms coming from in the final results. The perturbations are assumed to be local in the sense that their characteristic radial scale, , is shorter than the characteristic radial scale of the disks, . The latter is of the order of , i.e., i.e., . By using this approximation, we neglect such quantities as , , , and , compared with terms of the order of . Then, the -, -, and -components of equation of motion are reduced to (e.g., paper I)

 i(ω−mΩ)ur−2Ωuφ=−∂h1∂r−c2A∂∂r(bφB0), (4)
 i(ω−mΩ)uφ+κ22Ωur=0, (5)
 i(ω−mΩ)uz=−(∂∂z+c2A2c2szH2)h1−c2A(∂∂z−zH2)(bφB0)−imrc2A(bzB0). (6)

In the above equations, defined by has been introduced by assuming adiabatic perturbations, where and are, respectively, pressure and density perturbations over and .

Similarly, the -, -, and -components of induction equation are reduced to

 i(ω−mΩ)brB0=−imrur, (7)
 i(ω−mΩ)bφB0=rdΩdrbrB0−∂ur∂r−(∂∂z−z2H2)uz, (8)
 i(ω−mΩ)bzB0=−imruz. (9)

Finally, the equation of continuity is reduced to

 i(ω−mΩ)h1=−c2s[∂ur∂r+(∂∂z−zH2)uz]. (10)

Now, we further simplify equations (6) and (8). The last term, , of equation (6) can be expressed in terms of by using equation (9). The result shows that the term of is smaller than the left-hand term, , by a factor of . Considering this, we neglect the last term on the right-hand side of equation (6). Next, we consider equation (8). The first term on the right-hand side, , is smaller than the second term, , by a factor of , which can be shown by expressing in terms of by using equation (7). Hence, we neglect the term in the following analyses.

After introducing the above approximations into equations (6) and (8), we multiply to equation (6) in order to express and in equation (6) in terms of and by using equation (10) and (8). Then, after changing independent variables from (, ) to (, ), where is defined by , we have (paper I)

 [∂2∂η2−η∂∂η+(ω−mΩ)2−Ω2⊥c2s+c2AH2]uz+H[∂∂η−c2A/2c2s+c2Aη]∂ur∂r=0. (11)

This is the basic wave equation to be solved in this paper and the same as that in paper I.

## 3 Nearly Vertical Oscillations

Equation (11) is now solved by approximately decomposing it into two equations describing oscillatory behaviors in vertical and radial directions as done in paper I, following Silbergleit et al. (2001) and Ortega-Rodrigues (2008).

### 3.1 Boundary Condition at Disk Surface and Vertical Eigen-functions

As mentioned before, the oscillations which we are interested in here are nearly vertical in the lowest order of oscillations (i.e., vertical p-mode oscillations). The main terms in equation (11) are thus those of the first brackets, and the terms of the second brackets are small perturbed quantities (see paper I). Although the terms of the second brackets are small quantities, they are of importance to determine the wave trapping in the radial direction, as is shown in the next section.

First, we should notice that the quantity with in the first brackets depends weakly on radius . Hence, in order to consider this weak -dependence of the quantity as a small perturbed one, the third term in the first brackets of equation (11) is now expressed as

 (ω−mΩ)2−Ω2⊥c2s+c2AH2=[(ω−mΩ)2−Ω2⊥c2s+c2AH2]c+ϵ(r), (12)

where the subscript c represents the value at capture radius, , which is the outer boundary of the radial propagation region of oscillations and will be determined later. By definition, vanishes at , i.e., . The magnitude of is found from equation (12) when and are determined later by solving an eigen-value problem in the radial direction (see subsequent sections, especially see the final paragraph of section 5 and figure 9).

The fact that is really the capture radius of oscillations can be found from the following considerations. The final results show that is a small positive quantity which monotonically decreases outwards in the region of and vanishes at (see figure 9), i.e., for . This implies that is positive throughout the region of , when is positive. This further implies that is also positive in the region since is always smaller than . The facts of and in the region of means that the region is a propagation region of oscillations and the oscillations are trapped there [see equation (36)].

If the term of is transported to terms of small perturbations, equation (11) in the lowest order of approximations is written in the form:

 ∂2∂η2u(0)z−η∂∂ηu(0)z+[(ω−mΩ)2−Ω2⊥c2s+c2AH2]cu(0)z=0, (13)

where the superscript (0) is attached to in order to emphasize that it is the quantity of the lowest order of approximations. To solve equation (13), we must impose boundary conditions. In the case of isothermal disks which extend infinitely in the vertical direction, we impose that does not grow exponentially at (see Okazaki et al. 1987). In the present case of finite thickness of disks, however, a natural boundary condition to be imposed at (half-thickness of the disks) will be vanishing of the Lagrangian perturbation of the total pressure, i.e., , where . This is because outside the surface acoustic perturbations (more accuratly, fast mode of MHD perturbations) will be propagated away quickly by the presence of high-temperature and low-density corona.

The condition of can be written for nearly vertical oscillations as

 p1+B204πbφB0+ξz∂∂z(p0+B208π)=0, (14)

where is the vertical component of displacement vector, , associated with the perturbations. Since , , and the vertical hydrostatic balance gives , equation (14) can be written as

 h1+c2A(bφB0)−ξzΩ2⊥z=0. (15)

Since we are considering nearly vertical oscillations, in the lowest order of approximation, we have from equation (10) and from equation (8). Hence, substituting these relations into equation (15), we have, with the help of equation (3),

 ∂u(0)z∂η=0atη=±ηs(≡±zsH). (16)

Let us introduce a symbol defined by

 [(ω−mΩ)2−Ω2⊥c2s+c2AH2]c=Kn,s. (17)

Then, by solving equation (13) with the boundary condition (16), we have a discrete set of as eigen-values. The value depends on the node number of oscillations in the vertical direction (characterized by subscript n) and the height of disk surface (characterized by subscript s). In the lowest mode of oscillation with respect to node number in the vertical direction, we have const. and , independent of s. In this paper as in paper I, this mode is labelled by not by , i.e., , and has no node in the vertical direction.111 The reason why this fundamental mode is labelled by in spite of having no node in the vertical direction is that mode classification is made in many cases by the node number of , and has one more node(s) in the vertical direction, compared with . Figure 1 shows the eigen-value, , of three modes of , 2, and 3 as function of . In figure 2 the functional forms of of , 2, and 3 are shown for some values of . It is noted that in the limit of , and tend, respectively, to

 Kn,s=n−1,ρ0u(0)z,(n,s)∝exp(−η2/2)Hn−1(η), (18)

which are the same as the eigen-value and eigen-function of non-terminated isothermal disks (Okazaki et al. 1987), where is the Hermite polynomial of the order of with argument .

### 3.2 Orthogonality of Eigen-functions

The orthogonality of eigen-functions, , of different ’s is noted here, since we need it to derive wave equation in the radial direction, as is shown in the subsequent section. Now, is separated into - and -dependent terms as . At the present stage, the functional form of is arbitrary, which is determined later. The eigen-function then satisfies the following wave equation:

 ∂∂η[exp(−η2/2)∂g(0)n,s∂η]+exp(−η2/2)Kn,sg(0)n,s=0 (19)

[see equations (13) and (17)]. Hence, if the above equation is multiplied by and integrated from to , we have, after integrating by part with the help of boundary condition (16),

 (Kn,s−Kn′,s)∫ηs−ηsexp(−η2/2)g(0)n,sg(0)n′,sdη=0. (20)

This equation gives the orthogonality relation:

 ⟨g(0)n,s(η), g(0)n′,s(η)⟩=0,forn′≠n. (21)

Here and hereafter, means the integration of the product of and over to with weighting function .

## 4 Wave Equation in Radial Direction

Our next object is to proceed to the next order of approximations of equation (11), where is taken into account. Then, is no longer separated into a product of - and -dependent terms. That is, we expand as

 uz(r,η) =u(0)z,(n,s)+u(1)z,(n,s)+... (22) ≡f(r)[g(0)n,s(η)+g(1)n,s(r,η)+....].

In the lowest order of approximations, is separated as , but in the next order quantities, is a product of and a weakly -dependent term . Then, from equation (11), as equation describing , we have

 f(r)(∂2∂η2−η∂∂η+Kn,s)g(1)n,s(r,η)=−ϵ(r)f(r)g(0)n,s(η)−H[∂∂η−c2A/2c2s+c2Aη]∂u(0)r∂r, (23)

where the superscript (0) has been attached to in order to emphasize that in its lowest order quantity is enough in this equation.

The next subject is to express in terms of in order to solve equation (23). By the same procedures as in paper I, we have (see paper I), after some manipulations,

 (24)

where and are operators defined by

 Ls(f)=c2s/H−(ω−mΩ)2+κ2[ddr−dln(ω−mΩ)dr]f(r) (25)

and

 LA(f)=c2A/H−(ω−mΩ)2+κ2[ddr−dln(ω−mΩ)dr]f(r). (26)

Equation (23) is an inhomogeneous differential equation of with respect to . Hence, the solvability condition of inhomogeneous differential equation (23) with respect to is that when the right-hand side of equation (23) is expanded by the orthogonal set of functions, , it does not contain any term proportional to . That is, the condition is

 ϵf⟨g(0)n,s,g(0)n,s⟩+AHddrLs(f)+BHddrLA(f)=0, (27)

where

 A=⟨g(0)n,s(η),(ddη−12c2Ac2s+c2Aη)(ddη−η)g(0)n,s(η)⟩ (28)

and

 B=⟨g(0)n,s(η), (ddη−12c2Ac2s+c2Aη)(ddη−12η)g(0)n,s(η)⟩. (29)

This solvability condition (27) is an ordinary differential equation of with respect to , since disappears here by integrations over .

If expressions for and given by equations (25) and (26) are substituted into equation (27) under approximations of neglecting weak radial dependences of , , and , we see that equation (27) is a wave equation describing behavoir of in the radial direction and is expressed as

 −Ac2s+Bc2A⟨g(0)n,s,g(0)n,s⟩ddr[ω−mΩ(ω−mΩ)2−κ2ddr(fω−mΩ)]+ϵf=0. (30)

To obtain detailed expressions for and from equations (28) and (29), we need some manipulations, which are given in appendix. The results show that

 A=[−(Kn,s+1)+14c2Ac2s+c2A]In,s,0+14c2Ac2s+c2AIn,s,2−12c2Ac2s+c2AS (31)

and

 B=[−(Kn,s+34)+14c2Ac2s+c2A]In,s,0+14In,s,2+12c2sc2s+c2AS (32)

where

 In,s,0=⟨g(0)n,s(η), g(0)n,s(η)⟩andIn,s,2=⟨ηg(0)n,s(η), ηg(0)n,s(η)⟩, (33)

and is a surface value defined by

 S=ηsexp(−η2s/2)[g(0)n,s(ηs)]2. (34)

Then, becomes

 Ac2s+Bc2A=−[(c2s+c2A)Kn,s+(c2s+12c2A)]In,s,0+12c2Ac2s+c2A/2c2s+c2AIn,s,2. (35)

By using expressions for given above, we can finally write down the wave equation (30) in the form

 An,s(c2s+12c2A)ddr[ω−mΩ(ω−mΩ)2−κ2ddr(fω−mΩ)]+ϵf=0, (36)

where is defined by

 An,s=c2s+c2Ac2s+c2A/2Kn,s+1−c2A/2c2s+c2AIn,s,2In,s,0, (37)

where the ratio can be obtained by using vertical eigenfunctions shown in figure 2. It is noted that in the limit of , goes to . Then, given by equation (37) tends to in paper I, and equation (30) becomes equal to equation (36) in paper I.

In paper I we have introduced a new unknown function defined by . By using this function, we can reduce equation (30) to

 1ω−mΩddr[ω−mΩ(ω−mΩ)2−κ2d~fdr]+ϵAn,sΩ2⊥H2~f=0. (38)

Next, we solve equation (38) as an eigen-value problem to study where the oscillations are trapped and how much the eigen-frequency of the trapped oscillations are. We introduce now a new independent variable defined by

 τ(r)=∫rri~ω2(r′)−κ2(r′)−~ω(r′)dr′,τc≡τ(rc), (39)

where is defined by , and is the inner edge of disks where a boundary condition is imposed. Then, equation (38) is written in the form:

 d2~fdτ2+Q~f=0, (40)

where

 Q(τ)=~ω2~ω2−κ2ϵAn,sΩ2⊥H2. (41)

Equations (40) and (41) show that the propagation region of oscillations is the region where , which is the region of .

We solved equation (40) by a standard WKB method with relevant boundary conditions (for details, see Silbergleit et al. 2001 and Ortega-Rodrigues et al. 2008). The WKB approximation shows that the solution of equation (40) can be represented as

 ~f∝Q−1/4(τ)cos [Φ(τ)−Φc] (42)

in the whole capture region , except small vicinities of its boundaries of (i.e., ) and (i.e., ). Here, is defined by

 Φ(τ)=∫τ0Q1/2(τ′)dτ′=∫rriQ1/2(r′)~ω2(r′)−κ2(r′)−~ω(r′)dr′, (43)

and is a constant to be determined by boundary conditions. To determine the outer boundary condition, we take into account the fact that the capture radius, , is a turning point of equation (40) since the sign of changes there. The inner boundary condition we adopted is at . As the inner boundary radius we take the marginary stable radius. Then, WKB analyses show that the trapping condition is222see Silbergleit et al. (2001) or paper I for the case where boundary condition is adopted at .

 ∫τc0Q1/2dτ=π(nr+3/4), (44)

where is zero or a positive integer specifying the node number of in the radial direction. The constant is determined as

 Φc=π/2. (45)

For a given set of parameters, including spin parameter and mass of neutron stars, , any solution of equation (44) specifies , which gives of the trapped oscillation through equation (17). In other words, and are related by equation (17), i.e., or , and the trapping condition determines or (see also the next section and figure 3).

## 5 Numerical Results

We consider the same disks as in paper I, except that the present disks are terminated at a certain height, . The height is taken as a parameter, independent of . The temperature distribution adopted in the radial direction is that of the standard disks where the gas pressure dominates over the radiation pressure and the opacity mainly comes from the free-free processes, i.e., the acoustic speed on the equator, , is taken as (e.g., Kato et al. 2008)

 c2s0=1.83×1016(αMM⊙)−1/5(˙M˙Mcrit)2/5(rrg)−9/10 cm2 s−2, (46)

where is the conventional viscosity parameter, is the Schwarzschild radius defined by , and is the critical mass-flow rate defined by the Eddington luminosity. Throughout this paper, we fix , , and , as in paper I, since our purpose here is to examine how disk termination at a certain height affects on frequencies of trapped oscillations.

Before examinig parameter dependences of frequency, , of trapped oscillations, it is helpful to study how is related to the capture radius . The relation is specified by and given by equation (17), i.e.,

 ω=[mΩ−(c2s+c2Ac2s+c2A/2Kn,s+1)Ω⊥]c. (47)

The relation depends on , and in addition to the node number in the vertical direction. As mentioned before, we consider only the case of throughout this paper. Figure 3 shows relation (47) to oscillation modes of and , in cases of disks with and 2.0. The strength of magnetic fields is taken as . For comparison, the case of is also shown. It is noted that in the case of , the relation is free from . This comes from the fact that when . In the case of , however, the relation is affected by and moves downward on the frequency-radius diagram as the height of termination decreases. The downward shifts of the curve on the frequency – radius diagram means that the frequency of trapped oscillations decreases and the trapped region extends in the radial direction, although detailed values of the frequencies are obtained after the wave equation (38) is solved.

The frequencies of trapped oscillations obtained by solving equation (38) by the WKB method of the last section are shown in figures 4 – 6. In figure 4, the frequencies of trapped oscillations with or are shown as functions of for three cases of , 2.5, and 2.0. Figure 5 is the same as figure 4, except that the oscillations are considered. Comparison of figures 4 and 5 shows that in the case of oscillations of , frequency of trapped oscillations are much affected by termination of disks, i.e., their frequencies decrease with decrease of disk thickness (decrease of ). Figure 6 shows effects of spin of the central source on frequency of trapped oscillations in the case of for oscillations of and 2 with and 1. The value of adopted is 10.0. As in the case of non-terminated disks, the spin acts so as to increase the frequencies of trapped oscillations.

Next, parameter dependences of the radial width, , of the trapped region (i.e., capture zone) are examined for some modes of oscillations. Figure 7 shows the -dependence of the width for four oscillation modes ( and with , and and with ) in the case where and . For comparison, the cases of and are shown by thin curves for the above four oscillation modes. In general, the width of trapped region increases with decrease of disk thickness. This trend is prominent in oscillations of , although it is not so in the oscillations of . In the case of highly rotating sources, however, the trapped region decreases with increase of as shown in figure 8, where is again fixed to .

Finally, validity of the perturbation method adopted in this paper is checked. We have separated the - and - dependences of eigen-functions by assuming that the dimensionless quantity introduced by equation (12) is a small positive quantity in the radial propagation region of oscillations, i.e., in . This assumption can be checked after the radial eigen-value problem has been solved. The results show that the approximation is allowed in the first order of approximation. As an example, the radial distribution of obtained in some cases of and 2.5 are shown in figure 9.

## 6 Discussion

In this paper we have examined trapping of two-armed vertical p-mode oscillations in isothermal disks which are terminated at a certain height and subject to toroidal magnetic fields. The two-armed vertical p-mode oscillations are of interest since they are trapped in the innermost region of disks with moderate frequencies because of the very fact of (Kato 2010). For the vertical p-mode oscillations to be a good candidate of observed QPOs, their frequencies should not be robust but vary with time with a change of disk structure. Furthermore, the time variations of their different modes must correlate in such a way as they can describe the correlated variations of observed QPOs.

In the present model of QPOs, the major causes of time variation of frequencies of trapped oscillations are time changes of i) toroidal magnetic fields, ii) disk temperature, and iii) vertical thickness of disks. Time change of toroidal magnetic fields is generally expected, since magnetic fields are wound by differential rotation and loosened by magnetic reconnection. Time change of disk temperature will occur if, for example, mass accretion rate varies. Time change of vertical thickness of cool disks will also occur in real disks, since cool disks with strong toroidal magnetic fields and corona are expected as disks which bridge between ADAFs and optically thick disks (Machida et al. 2004, Oda et al. 2007, 2009, 2010). Evaporation of disk gas to hot corona will also depend on stages of disk activity.

The results of this paper show that a change of vertical disk thickness on frequencies of trapped oscillations is little in the case of oscillations. This is related to the fact that the eigen-value of purely vertical p-mode oscillations, , is independent of , and is zero when , i.e., . In the case of oscillatios of , however, vertical termination of disk thickness has non-negligible effects on their frequencies. That is, as the height decreases, the frequencies of trapped oscillations of decrease and the radial extend of trapping region becomes wide. The trapped region is, however, not wide compared with that of c-mode oscillations (Silbergleit et al 2001) in the case of small . Different from c-mode oscillations which are incompressible motions in the limit of , the two-armed vertical p-mode oscillations are the fast mode of the three MHD modes, and thus strong density and temperature variations are associated with the oscillations. Hence, in the case of disks which are vertically terminated by hot coronae, hard X-ray time variations by inverse Compton processes will be expected as the results of geometrically thin disk oscillations.

In the case of oscillations, the trapped region is wide compared with the case of oscillations, as mentioned above. Thus, our basic approximation introduced in this paper that the radial variations of and are negligible should be improved in more realistic studies. Furthermore, more careful considerations on inner boundary condition will be necessary to do more quantitative studies. Concerning the radius where an inner boundary condition is imposed, however, the ISCO will be relevant as the first approximation, unless strong poloidal magnetic fields anchored to the central sources are present.

One of basic assumptions involved in our analyses is that the disks are vertically isothermal and is also constant in the vertical direction. We think that the assumption of vertical isothermality will be better than that of polytropic disks where temperature decreases from equator toward disk surface,333 Trapping of two-armed p-mode oscillations in polytropic disks has been examined (Kato 2010). The results show that an increase of polytropic index decreases the frequency of the trapped oscillations. especially in disks surrounded by hot corona. Examinations how our present results are modified if is not constant in the vertical direction are of importance to evaluate whether the present disk oscillation model is relevant to describe the observed QPOs. We suppose that the frequency of trapped oscillations decreases in the case where increases toward surface, compared with the case where