Issue 
A&A
Volume 532, August 2011



Article Number  A93  
Number of page(s)  12  
Section  The Sun  
DOI  https://doi.org/10.1051/00046361/201117013  
Published online  01 August 2011 
Toward detailed prominence seismology
I. Computing accurate 2.5D magnetohydrodynamic equilibria
^{1}
FOM Institute for Plasma Physics Rijnhuizen, Association EURATOMFOM, PO Box 1207, 3430 BE Nieuwegein, The Netherlands
email: JW.S.Blokland@Rijnhuizen.nl
^{2}
Centre for Plasma Astrophysics, Mathematics Department, KU Leuven, Celestijnenlaan 200B, 3001 Heverlee, Belgium
Received: 4 April 2011
Accepted: 16 May 2011
Context. Prominence seismology exploits our knowledge of the linear eigenoscillations for representative magnetohydrodynamic models of filaments. To date, highly idealized models for prominences have been used, especially with respect to the overall magnetic configurations.
Aims. We initiate a more systematic survey of filament wave modes, where we consider full multidimensional models with twisted magnetic fields representative of the surrounding magnetic flux rope. This requires the ability to compute accurate 2.5 dimensional magnetohydrodynamic equilibria that balance Lorentz forces, gravity, and pressure gradients, while containing density enhancements (static or in motion).
Methods. The governing extended GradShafranov equation is discussed, along with an analytic prediction for circular flux ropes for the Shafranov shift of the central magnetic axis due to gravity. Numerical equilibria are computed with a finite elementbased code, demonstrating fourth order accuracy on an explicitly known, nontrivial test case.
Results. The code is then used to construct more realistic prominence equilibria, for all three possible choices of a free fluxfunction. We quantify the influence of gravity, and generate cool condensations in hot cavities, as well as multilayered prominences.
Conclusions. The internal flux rope equilibria computed here have the prerequisite numerical accuracy to allow a yet more advanced analysis of the complete spectrum of linear magnetohydrodynamic perturbations, as will be demonstrated in the companion paper.
Key words: Sun: filaments, prominences / instabilities / magnetohydrodynamics (MHD) / plasmas
© ESO, 2011
1. Prominence seismology and equilibrium configurations
One of the most fascinating phenomena embedded in the million degree solar coronal plasma is the presence of socalled filaments, which are plasma concentrations suspended magnetically against the downward pull of the solar gravitational field. They are up to 100 times colder and denser than their immediate surroundings, and in Hα observations of the solar disk appear as dark features extending over huge distances. High resolution observations indicate that the filament is actually composed of many individual threads, down to the resolution limit of modern observations (about 100 km in width, see Lin et al. 2005), while their length can reach several tens of megameters. When viewed at the solar limb, the filaments can be identified as prominences, and the surrounding magnetic geometry introduces a classification supported by early analytical magnetohydrostatic models (see e.g. Priest 1988): normal and inverse polarity prominences differ in the relative orientation of the filamentcarrying flux rope with respect to the underlying (and overarching arcade) magnetic orientation. Comparing their locations to photospheric magnetograms, the filament threads appear primarily suspended above a magnetic neutral line. The study of solar filaments still poses many contemporary challenges to theoretical solar physicists, in terms of their sudden formation, their potential to survive for months on end, and their small as well as largescale dynamics. Reviews of the physics of solar prominences include one by Labrosse et al. (2010), providing an overview of the prominence/filament thermodynamic parameters obtained by modern spectroscopic inversions, and another by Mackay et al. (2010), which compiled insights from essentially magnetohydrodynamic modeling that were compared with observations.
A particularly active research area is known as prominence seismology, whose ultimate goal is the use of observed oscillatory motions in filaments to deduce their internal properties, by matching computed with detected frequencies, damping rates, and possibly spatiotemporal eigenstructure of the vibration modes. As part of this effort, the review by Mackay et al. (2010) collects insights from observations and theory, and points out how recent works account for the multithreaded fine structure (Luna et al. 2010), as well as for nonadiabatic modifications to the wave modes in prominences (Soler et al. 2008). Another review by Arregui & Ballester (2011) concentrates on how the linear MHD modes can help in explaining the observed attenuation. To make analytic progress, virtually all of these efforts make dramatic simplifications about the overall geometry of the magnetic field and thread characteristics: cylindrical flux tubes or segments embedded in uniform, threadaligned magnetic fields form a recurring ingredient. When accounting for internal structure, density variations can explain the observed damping of global eigenoscillations in terms of resonant absorption and/or partial ionization, where global kink modes couple to fluxsurface localized Alfvén modes (Soler et al. 2010). Despite the model restrictions, various indicative relations between threadcorona density contrast on the one hand, and mode damping rate to period ratio on the other hand, have been established by means of combined analytical and numerical techniques (see e.g. Goossens et al. 2011). At the same time, it is as yet unclear whether these relations generalize to the more realistic topologies where magnetic shear, gravity and pressure variations are all incorporated.
A major obstacle on the road to generalizing these findings to more realistic prominence models, is that generating accurate equilibrium models for prominencebearing flux ropes becomes a nonlinear problem of its own. Even when we restrict the problem to a 2.5D magnetohydrostatic configuration by assuming translational invariance along the prominence axis, relatively scarce cases exist where an analytic solution is known. Notable exceptions form the early work by Dungey (1953), where for isothermal conditions the static force balance between the Lorentz force, the (uniform) gravity, and the pressure gradients could be solved analytically. Low & Zhang (2004) developed under polytropic pressuredensity relations, magnetostatic solutions for both normal and inverse polarity quiescent prominences. These latter authors pointed out how their construction avoids the freeboundary problem posed by matching the internal fluxrope solution, to the external (nearly potential) atmospheric field. In practice, this was achieved by prescribing the prominence to be embedded in a horizontal, circular cylinder, whose boundary then coincides with the internalexternal transition. In Petrie et al. (2007), this analytic approach was complemented and generalized with a numerical treatment where again both polarity types were realized, by iteratively solving the governing elliptic PDE which does fully account for the freeboundary problem. It was then demonstrated that a solution can be constructed with the characteristic, observed threepart structure of a cool dense prominence, surrounded by a cavity, within a flux rope in a hot coronal environment.
We here revisit the problem of generating accurate, numerical equilibria that are representative of helical flux ropes, supporting dense prominences, possibly showing axial (shear) flows. The need to demonstrate high accuracy for the obtained numerical equilibria is a prerequisite for any further analysis quantifying the magnetohydrodynamic wave modes. This is common knowledge in fusionrelated plasma configurations, where MHD spectroscopy (Goedbloed et al. 1993) needs to take full account of the detailed magnetic geometry to chart out, and eventually invert from, the complete MHD spectrum of waves and instabilities. Meanwhile, this approach has already been transported to astrophysically relevant accretion tori (Goedbloed et al. 2004; Blokland et al. 2007), where a toroidally caged, axisymmetric plasma torus has both toroidal (Kepleriantype) and possibly also poloidal flows in a delicate force balance with a central external gravitational field. The MHD spectroscopic determination of the eigenoscillations of these accretion tori brought out how fluxsurface localized eigenmodes may become unstable as a result of intricate mode couplings resulting from the poloidal crosssectional variation. We here attempt to demonstrate the same ability to chart out all eigenmodes for realistically structured prominences, starting with the determination of the continuous parts of the MHD eigenspectrum. These MHD continua form the basic organizing structure of the entire collection of MHD eigenmodes (Goedbloed & Poedts 2004; Goedbloed et al. 2010), and because of the multidimensional nature of the prominencecontaining flux rope, will contain avoided crossings and frequency gaps (Poedts & Goossens 1991). To quantify these mode couplings, and to subsequently take the next step towards full diagnosis of all global discrete eigenmodes, we must ensure that our equilibrium solution is amenable to such an analysis.
This paper is therefore organized as follows. We begin in Sect. 2 with reducing the governing equations for a translationally invariant, 2.5D magnetohydrostationary configuration to the extended GradShafranov equation. This section recapitulates how 2D equilibria balancing Lorentz force, gravity, and pressure gradients allow for axial (shear) flow, and are in principle realizable for three categories of solutions, where either density, entropy, or temperature take on a constant value on a single flux surface. We point out the essential role of straight field line coordinates, which must also be constructed from the obtained solution. In Sect. 3, we obtain the analytical equilibria valid for small gravity, where the outer flux surface is assumed to be circular, and the internal, nested flux surfaces are then displaced circles, shifted downwards under the influence of gravity. This is completely analogous to the Shafranov shift (Shafranov 1958) in the axisymmetric tokamak configuration induced by toroidal curvature. This can serve as a clear accuracy test for the numerically generated equilibria. In Sect. 4, we briefly explain the MHD equilibrium code FINESSE (Beliën et al. 2002). This code is used to generate numerical equilibria. Finally, Sect. 5 then uses FINESSE and demonstrates how we obtain fourthorder accurate solutions by recovering the analytical case presented by Dungey (1953). It then continues to show the various types of solutions, how they obey the analytically predicted shift for small gravity, and then surveys those cases that are no longer tractable by analytic means. This includes a case where at sufficiently large gravity, multiplylayered prominence condensations can exist in a helical flux rope. We restrict these computations to cases for given outer crosssectional shape resulting in only the internal solution. This restriction is needed because the followup analysis of diagnosing the wave modes intrinsically depends on the presence of closed, nested magnetic flux surfaces. The wave mode analysis will be presented in an accompanying paper (Blokland & Keppens 2011), where analytic as well as numerical results on the MHD continua for the 2.5D equilibria presented here are analyzed.
2. Solar prominence equilibrium
We begin our analysis by considering a translational symmetric solar prominence. For this kind of symmetry, Cartesian coordinates (x,y,z) are the natural choice. We note that for this symmetry, the equilibrium quantities depend only on the poloidal coordinates x and y. The prominence equilibrium itself is modeled by the ideal MHD equations where ρ, p, v, B, Φ, and γ are the density, pressure, velocity, magnetic field, gravitational potential, and the ratio of the specific heats, respectively. The current density j = ∇ × B and the equation ∇·B = 0 has to be satisfied. We note that the presented ideal MHD equations are in the nondimensional form. The equilibrium will be assumed to be timeindependent. Furthermore, the thermal pressure and the density are related by the ideal gas law p = ρT. From the equations ∇·B = 0 and ∇·j = 0, it follows that the magnetic field and the current density can be written as respectively, where, 2πψ is the poloidal flux and the poloidal stream function I = B_{z}. We restrict ourselves to prominence equilibria with a purely axial flow (7)In this case, Eqs. (2)and (4)are trivially satisfied. The axial velocity v_{z} is related to the electric field (8)From the induction equation presented in Eq. (3), it follows that v_{z} = v_{z}(ψ). Since axial flows are routinely observed in prominence threads, we include the parameter v_{z} in our analysis. Owing to the translational symmetry, it does not play any role in the actual force balance, but we show in an accompanying paper (Blokland & Keppens 2011) how the velocity shear in the equilibrium modifies the eigenspectrum.
The momentum equation Eq. (1)can be projected in three ways. The first one is in the axial direction, which shows that the poloidal stream function is a flux function, i.e. I = I(ψ). The second projection is parallel to the poloidal magnetic field resulting in two equations (9)These two equations have to be satisfied simultaneously. We conclude from these that the pressure p = p(ψ;x,y). The third and last projection is the one perpendicular to the poloidal magnetic field. This leads to the extended GradShafranov equation (10)
2.1. Further reduction for specific flux functions
The two equations parallel to the poloidal magnetic field given in Eq. (9)can be solved analytically under the extra assumption that either the temperature T, the density ρ, or the entropy S = pρ^{ − γ} is a flux function. The assumption that the temperature is a flux function can be justified because of the high thermal conductivity along the magnetic field lines. The resulting pressure can then be written as (11)where p_{0} is the pressure for a static pure GradShafranov equilibrium without gravity. The extended GradShafranov equation in Eq. (10)reduces to (12)This extended GradShafranov equation is a minor generalization of the one presented in Petrie et al. (2007), by allowing a fully general external gravitational potential. This case where temperature is a flux function is most relevant for the quiescent solar prominences, which are longlived structures and hence will be temperature equilibrated on flux surfaces. The isothermal case forms a subset of this solution class.
Another possibility, on MHD timescales, is to assume that the density is a flux function. In this case, the pressure reads (13)where the quasitemperature T_{ρ} ≡ p_{0}/ρ. Under this assumption, the extended GradShafranov equation in Eq. (10)can be written as (14)This case where density is a flux function will be shown in our companion paper to be susceptible to unstable continuum modes, under quantifiable stability criteria (Blokland & Keppens 2011). Hence, it might be relevant to the shortlived active region prominences, where these instabilities may relate to the sudden disappearance of filaments.
The final option is to assume that the entropy S is a flux function, as also discussed in Petrie et al. (2007). We again generalize it slightly by adopting an arbitrary potential, for which the pressure reads (15)and the extended GradShafranov equation in Eq. (10)reduces to (16)where the quasitemperature . We note that all three cases can also be derived using the expressions for axisymmetric accretion tori with a purely toroidal flow, as presented in the paper by Blokland et al. (2007), by setting R = R_{0} = 1 in their formulae. This case where entropy is a flux function is the natural one to consider when also plasma rotation would be incorporated.
The equation for the density for all three cases can easily be derived by inserting the corresponding pressure equation into the equation for the momentum parallel to the poloidal magnetic field lines given in Eq. (9). The resulting equation is (17)Here, the flux function ρ_{0} corresponds to the density of a related static equilibrium without gravity.
2.2. Straight field line coordinates
As we will adopt them for the actual stability analysis in our accompanying paper, we briefly discuss the “straight field line” coordinates. These coordinates are an essential ingredient of an accurate stability analysis. For the conversion from the Cartesian (x,y,z) to straight field line coordinates (x^{1} ≡ ψ,x^{2} ≡ ϑ,x^{3} ≡ z), one needs the metric tensor and the Jacobian associated with the nonorthogonal coordinates in which the equilibrium field lines appear to be straight. Such a transformation is standard practice in MHD stability studies for laboratory tokamak plasmas. The metric elements g_{ij} and the Jacobian J are (18)respectively. Here, the poloidal angle ϑ is constructed such that the magnetic field lines are straight in the (ϑ,z)plane. The slope of these lines is a flux function (19)where q is the safety factor. Comparing this expression with the one for tokamak plasmas (Wesson 2004), one should realize that for tokamak plasmas the safety factor q is dimensionless, while here the factor q has a length dimension. As for tokamak plasmas (Goedbloed 1975; van der Holst et al. 2000; Blokland et al. 2007), we introduce an expression for the poloidal curvature of the magnetic surfaces (20)where the unit vectors n = ∇ψ/∇ψ and t = B_{ϑ}/B_{ϑ}, and B_{ϑ} is the poloidal magnetic field. The toroidal curvature κ_{t} that is present in actual tokamak equilibria, is of course zero for a translational symmetric equilibrium. It is important to realize that the straight field coordinates can only be constructed when the solution ψ(x,y) has been computed from the extended GradShafranov equation given in Eq. (10).
3. Small gravity expansion
In the previous section, we derived equations for the prominence equilibrium. In this section, we quantify the effect of gravity by means of a small gravity expansion. We will demonstrate in our companion paper that gaps will appear in the continuous MHD spectrum because of mode coupling, which is the result of the presence of gravity. This kind of expansion is similar to the small inverse aspect ratio ϵ = a/R_{0} expansion for tokamak plasmas, where a and R_{0} are the minor radius of the plasma and the geometry axis of the tokamak, respectively (Shafranov 1958). Mathematically, both expansions, small gravity expansion and the small inverse aspect ratio expansion, are Taylor expansions. In the remaining part of this paper, we assume the following gravitational potential in which the prominence is embedded (21)where x_{0} is the location of the center of the last closed flux surface of the prominence and the gravity is represented by the constant g.
The solar prominence equilibrium is expanded assuming that the gravity is small and that the outer flux surface is circular. Using these approximations, the flux surfaces can be represented by slightly displaced circles (Shafranov 1958), which allows for the exploitation of nonorthogonal polar coordinates (r,θ,z), where r and θ are the radius and the polar angle, respectively. Up to first order, we approximate (22)where Δ(r) is the Shafranov shift (Shafranov 1958), which is expected to be in the downwards direction and caused by the gravity. As mentioned before, these polar coordinates are nonorthogonal and the associated metric elements are (23)which means that the Jacobian J ≈ r [1 − Δ′cos(θ)].
Using the polar coordinates and expanding the extended GradShafranov equation given in Eqs. (12), (14), and (16)up to first order leads to one equation for the equilibrium () and one equation for the Shafranov shift () for all three cases. The equilibrium relation is (24)where B_{θ} ≡ ψ′ is the poloidal magnetic field expressed in polar coordinates, where the prime indicates the derivative with respect to the radius r. This is exactly as expected, since this equation merely expresses the force balance in a cylinder. From this equation, one can see that the pressure and the magnetic field components are of the same order . This means that the plasma beta . This is very different from tokamak physics where the pressure is two orders of magnitude lower than the toroidal magnetic field component, which ensures that the plasma beta there is of the order (van der Holst et al. 2000). For such tokamak plasmas, the Shafranov shift is outwards due to the toroidicity, pressure, and toroidal flow (van der Holst et al. 2000).
The equation for the Shafranov shift in prominence equilibria is (25)which shows that the magnetic axis is shifted downwards because of the gravity. We note that for zero gravity or a constant density there will be no shift at all, again in accord with the cylindrical configuration then expected.
As mentioned before, to perform the spectral formulation and compute the continuous MHD spectrum, the analysis is done in straight field line coordinates. Exploiting the small gravity expansion, the straight field line metric elements can be approximated by (26)In deriving these expressions, we exploited that the safety factor q from Eq. (19)is a flux function and therefore the Jacobian J( = r/ψ′) has to be a flux function. This allows us to find a relationship between the polar angle θ and the straight field line angle ϑ(27)
4. The equilibrium code FINESSE
4.1. Code basics: discretization
The FINESSE code was originally developed by Beliën et al. (2002) and designed to solve the coupled generalized GradShafranov equation together with the algebraic Bernoulli equation (Hameiri (1983); Zelazny et al. (1993); Goedbloed et al. (2004)). The design of the code is such that we could easily extend it by implementing the extended GradShafranov equations given in Eqs. (12), (14), and (16), as realized in version 1.3 of the FINESSE code. These equations are solved for a given poloidal crosssection using the Picard iteration scheme in combination with a standard matrix solver. The boundary conditions are such that a fixed given boundary shape represents the last closed flux surface. As a discretization scheme, we exploited a finite element method in combination with the standard Galerkin method. As elements, we used isoparametric Hermite elements. These elements ensure that the computed solution has the required accuracy needed for the stability analysis.
4.2. Scaling for prominence equilibria
The exploited scaling in FINESSE is such that all numerical quantities actually computed are quantified in 1) the profile variations of order unity; and 2) the amplitudes that determine the relative strengths. The idea is that solving the governing elliptic PDE numerically should exploit quantities of order unity as much as possible. This means for example that we ensure a scaling such that, e.g. the flux function ψ varies from 0 to 1. In the results section (Sect. 5), we present either dimensionless quantities such as the local plasma β, or quantify the pressure or the gravity parameter g in code units. Since we vary g in what follows, this may seem unusual at first for solar filaments, because one can obviously not alter the solar gravitational field. We therefore here explain the inherent scaling.
For this purpose, some typical values for solar prominence conditions taken from Labrosse et al. (2010) and Mackay et al. (2010) are as follows. Lengths are expressed in units of the prominencecarrying magnetic loop radius. This length unit L can be varied from 100 km (if a single prominence thread is being modeled) to 10 Mm, the latter being an upper width quoted for solar prominence structures. Taking a typical temperature of 8000 K (a factor 100 cooler than the corona) and an electron number density n_{e} ~ 10^{16} m^{3}, the density is then ρ ~ 1.673 × 10^{11} kg m^{3} and a reference pressure value is p ~ 0.00221 N m^{2}. We note that the sound speed can then be estimated to be 15 km s^{1}. If we also use a typical value of magnetic field strength B ~ 10^{3} T, the Alfvén speed is 218 km s^{1}. For these parameters, the plasma beta can be as low as β = 0.0055, but we note that values of up to order 0.1 can be deduced from observations. The gravitational acceleration at a solar radius is of order g ~ 272 N kg^{1}, and a typical hydrostatic scaleheight inferred from these values combined, yields Λ = p/ρg ~ 485 km. When we quantify the parameter g in dimensionless units below, we actually mean the value of the dimensionless combination (with μ_{0} the permeability) (28)We note that this dimensionless quantification of the strength of the gravitational field can meaningfully be altered by orders of magnitude, as it is directly proportional to the size of, and the density in the prominence, and inversely proportional to the square of the field strength. Hence, larger values of the combination represent larger, denser prominences in weaker embedding magnetic fields, while the value given above is a reasonable reference value for a typical flux rope. Code units in essence use a dimensionalization based on L, ρ, and B, so that for instance the pressure is in units of B^{2}/μ_{0} ~ 0.795 N m^{2}. This means that the reference pressure value quoted above is reached at p = 0.0028 in units of B^{2}/μ_{0}.
5. Numerical results
We now demonstrate that FINESSE can accurately compute prominence equilibria by comparing the numerical solution with the analytical solution derived by Dungey (1953). We then discuss two classes of equilibria. The first class represents cool prominences embedded in a hot medium and the second one in combination with proper chosen parameters represents multilayered prominences.
5.1. Accuracy test: the Dungey solution
To demonstrate FINESSE accurately computes the prominence equilibria, we compare the numerical result with the analytical solution derived by Dungey (1953). The derived solution (29)where α ≡ g/T, satisfies the extended GradShafranov equation given in Eq. (12)with the extra assumption that the temperature T is constant. The solution itself is used to specify the last closed surface so FINESSE can compute the interior for various resolutions. The error between the numerical solution and the analytical one as a function of the number of grid points is shown in Fig. 1. The quantities L^{2} and L^{∞} are the average error and the maximum error evaluated over the whole interior. The plot clearly demonstrates that FINESSE shows a fourth order convergence as it was designed to do. Furthermore, it also shows that moderate resolution is enough to obtain a highly accurate equilibrium solution.
Fig. 1 The accuracy test of FINESSE with respect to the analytical solution derived by Dungey (1953). The quantity L^{2} and L^{∞} are the average and maximum error between the Dungey solution and the numerical solution over the whole interior. 

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5.2. Cool prominence surrounded by a hot medium
The first equilibrium class of solar prominences is the one where a prominence is embedded in a hot medium. These kinds of equilibria are specified by the following profiles: where A_{2} = 0.1 and A_{3} = 1. The amplitude A is the overall amplitude computed by FINESSE as part of the equilibrium solution. The function T_{0} represents the (quasi) temperature of the three choices of the flux function, the density, the entropy, or the temperature. The gravity g, scaled as explained earlier, has been varied from 0.001 up to 1.000. For most equilibria of this subsection, the temperature is assumed to be a flux function, except when stated differently. Furthermore, we assume a circular boundary. The resolution adopted for the numerical computations are 101 radial points and 129 points in the poloidal direction. The specified profiles for I^{2}(ψ) and p_{0}(ψ) are of the same form used by Low & Hundhausen (1995), Low & Zhang (2004), and Petrie et al. (2007). The form of the T_{0}(ψ) profile is the same as the one used by Petrie et al. (2007), which represents a low temperature in the center while the temperature is high at the edge of the prominence.
Fig. 2 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a cool solar prominence surrounded by a hot medium with a gravity g = 0.001. The solar surface is below the figure. 

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Fig. 3 Top: the safety factor q at the midplane for a gravity g = 0.001. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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Fig. 4 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a cool solar prominence surrounded by a hot medium with a gravity g = 0.100. The solar surface is below the figure. 

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For the first equilibrium, we set the gravity to be g = 0.001. The resulting pressure and plasma beta β = 2p/B^{2} are shown in Fig. 2. The plot shows clearly a high pressure in the center and a low pressure at the edge of the prominence. A similar observation can be made about the plasma beta, which is around 0.097 in the core and at the edge has the value of 0.014. The variation in the density, not shown, ranges from 0.006 at the edge up to 1.000 in the centre. The central temperature has a value of 0.048, while at the edge it is 0.780, which clearly resembles a cool prominence embedded in a hot medium. For the previously mentioned beta values, the magnetic field as well as the thermal pressure will play an important role in the stability analysis of our accompanying paper. In this stability analysis the safety factor q, shown in Fig. 3, is also an essential ingredient. From fusion research, we know that around the q = 1 and q = 3/2 surface, mode coupling may occur which in its turn can create gaps in the MHD continuous spectrum or even drive the continuous spectrum unstable. The plot of the safety factor shows that both surfaces exist in this cool prominence equilibrium. The same figure also shows the radial derivative of the Shafranov shift. This derivative was calculated in two different ways. The first applied the second of the equations given in Eq. (22)and the ability of FINESSE to perform the transformation to straight field line coordinates. The second method numerically solved the Shafranov shift equation in Eq. (25)using Simpson’s rule (Press et al. 1988). The first method is valid for any value of the gravity parameter as long as the flux surfaces are circles, while the second method can only be used for small gravity in combination with circular flux surfaces. The RHS plot of Fig. 3 shows excellent agreement between the two described methods.
Fig. 5 Top: the safety factor q at the midplane for a gravity g = 0.100. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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Fig. 6 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a cool solar prominence surrounded by a hot medium with a gravity g = 1.000. The solar surface is below the figure. 

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We then increase the gravity parameter by a factor of 100, i.e. g = 0.100. The pressure and plasma beta are shown in Fig. 4. Since the fact that the parameter g is 100 times stronger, the pressure maximum is shifted downwards as expected. The plasma beta has values similar to those in the previous case, its maximum and minimum values being 0.105 and 0.014, respectively. The twodimensional density profile, not shown here, has a similar behavior to that of the pressure profile. Its maximum is also shifted downwards as expected. Figure 5 shows the safety factor q and the radial derivative of the Shafranov shift Δ(r). Comparing the safety factor with the one of the previous equilibrium, one notices that there is hardly any difference. The two methods for computing the Shafranov shift now show a small difference. The second method, which using the Shafranov shift equation in Eq. (25), underestimates the radial derivative for all radii.
The last cool solar prominence we discuss is the one for which the dimensionless gravity parameter is g = 1.000. The gravity is 1000 times stronger than in the first discussed equilibrium and 10 times stronger than the last one. The downward shift of the pressure is even stronger as shown in Fig. 6. For this strong g case, the plasma beta varies from 0.013 at the edge up to 1.107 at the core of the plasma. The latter value is larger than one would expect from observations. However, it is straightforward to compute an even more realistic equilibrium by adjusting the coefficient A_{2} of the pressure equation in Eq. (31). For this equilibrium, the safety factor and the Shafranov shift are shown in Fig. 7. Owing to the strong gravity the safety factor is very different from its value for the two previous equilibria, particularly in terms of the multiple q = 1 surfaces. In addition, the plot of the Shafranov shift shows a large discrepancy between the two methods, because of the strong gravity. The first method of determining the Shafranov shift is superior in terms of accuracy and numerical cost.
Fig. 7 Top: the safety factor q at the midplane for a gravity g = 0.500. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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Fig. 8 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a cool solar prominence surrounded by a hot medium with a gravity g = 1.000 for the case that the density (top) or the entropy (bottom) is a flux function. The solar surface is below the figure. 

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To illustrate the difference between the chosen flux function, we also computed the cases where the density or the entropy is a flux function for gravity g = 1.000. For these choices, the pressure and plasma beta are plotted in Fig. 8. When density is a flux function, the plasma beta varies from 0.011 up to 0.254, and for the entropy case the range is 0.012 up to 0.395. Both plots are clearly distinct from the case where the temperature is chosen to be a flux function. From the equilibrium viewpoint, all three are realizable, but high resolution observations will be required to help us to select the proper flux function for a particular filament.
5.3. Multilayered prominences
The second class of equilibria, based on the description presented by Petrie et al. (2007), allows for multilayered prominences. This class is specified by the following expressions \arraycolsep1.75ptwhere A_{2} = 0.1 and A_{3} = 1. In addition, the overall amplitude A is computed by FINESSE. The gravity g is varied from 0.001 up to 5.000. As for the previous class of cool prominences, we assume that the boundary is circular and that the temperature is a flux function. The function T_{0} has the same meaning as in the previous subsection, and represents the (quasi) temperature of the chosen flux function. As for the previous class, the numerical computations are done for 101 and 129 points in the radial and poloidal direction, respectively.
Fig. 9 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a doublelayered solar prominence with a gravity g = 0.001. The solar surface is below the figure. 

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Fig. 10 Top: the safety factor q at the midplane for a gravity g = 0.001. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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Fig. 11 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a doublelayered solar prominence with a gravity g = 1.000. The solar surface is below the figure. 

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Starting with small gravity g = 0.001, Fig. 9 shows the twodimensional pressure and the plasma beta β = 2p/B^{2}. The latter quantity varies from 0.001 at the edge to 0.097 at the center of the prominence. Once more, we emphasize that for these plasma beta values the magnetic field as well as the pressure play an important role in the stability analysis of our accompanying paper. The pressure shows a ring structure. By increasing the parameter g, we show below that one can create a doublelayered prominence. The safety factor q and the radial derivative of the Shafranov shift are plotted in Fig. 10. For small g, the safety factor q has two flat regions that correspond to the ringlike cavity of low pressure. Furthermore, note that the q = 1 and q = 3/2 surfaces both exist for this equilibrium. As for cool prominences, this will mean that gaps or instabilities may occur in the MHD continuous spectrum. The figure also shows that the two methods for computing the Shafranov shift, as discussed in the previous subsection, show excellent agreement. For the next equilibrium, we have set the gravity parameter g = 1.000, which is 1000 times stronger than in the case above. This example shows the onset of the doublelayered pressure profile as can be seen in Fig. 11. If one closely looks at the plot, one still sees the ring structure but because of the stronger gravity compared to the small gravity g = 0.001 case this structure has almost disappeared. The plasma beta ranges from 0.00069 in the low pressure regions up to 0.117 in the high pressure regions. For this equilibrium, we also computed the safety factor q and the Shafranov shift. Both quantities are presented in Fig. 12. A comparison between the safety factor for this equilibrium and that for the small gravity g = 0.001 case finds hardly any differences. The only real difference is the maximum of the q profile, which is shifted slightly downwards because of the stronger gravity. The plot of the Shafranov shift shows that a small difference between both means of determining the shift is clearly evident. The second way of applying the Shafranov equation given in Eq. (25)again underestimates the radial derivative.
The increase in the gravity parameter to g = 5.000 creates a clear doublelayered pressure structure as can be seen in Fig. 13. A similar structure is found for the density. The plasma beta varies from 0.000031 up to 1.994. The latter value is higher than we expect based on observations. As mentioned before, it is straightforward to compute a more realistic value by changing the coefficient A_{2} of the profile pressure equation in Eq. (35). The safety factor of this doublelayered prominence, shown in Fig. 14, varies widely. It no longer contains a q = 3/2 surface as in the previous two cases of this equilibrium class. Furthermore, we note that near the magnetic axis (around x = −0.5) it almost creates new q = 1 surfaces. The magnetic axis is the location where the poloidal magnetic field is zero. The Shafranov shift is also shown in Fig. 14. As expected, the two methods for determining the shift no longer agree. As in the previously discussed case, the Shafranov shift equation in Eq. (25)underestimates the radial derivative. Figure 15 presents this prominence configuration in 3D, illustrating the varying twist of the magnetic field lines. In our accompanying paper, we will analyze the way in which this more realistic field configuration modifies the MHD eigenspectrum of the fluxsurface localized continuum modes.
Fig. 12 Top: the safety factor q at the midplane for a gravity g = 1.000. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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Fig. 13 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a doublelayered solar prominence with a gravity g = 5.000. The solar surface is below the figure. 

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Fig. 14 Top: the safety factor q at the midplane for a gravity g = 5.000. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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Fig. 15 A threedimensional impression of the doublelayered solar prominence for gravity parameter g = 5.000. Shown are an isosurface of density, at a value showing the layering of the condensation, with the crosssectional view shown midway this 3D impression. The magnetic field structure is visualized by drawing selected fieldlines, demonstrating the varying twist of the helical configuration. The field lines are colored by the magnetic field strength. The solar surface is below the figure. 

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6. Conclusions
We have presented the equations describing translational symmetric solar prominence equilibria. These equations have been specialized for three choices of the freedom in flux function in which the temperature, density, or entropy can be fluxdependent. For small gravity and circular crosssection, we have expanded these equations to derive the equation for the equilibrium of a cylindrical plasma and the equation for the Shafranov shift.
The MHD equilibrium code FINESSE has been used to compute accurate prominence equilibria. A comparison between the numerically generated equilibrium and the Dungey solution shows fourth order convergence, and moderate resolution is needed to obtain an accurate solution.
We have considered two equilibrium classes, cool prominences surrounded by a hot medium and doublelayered prominences, for different values of the dimensionless gravity parameter (in a range corresponding to solar filament cases) with plasma beta of the order 0.1. For both classes, a comparison between the numerical solution and the derived equation for the Shafranov shift has been made. This comparison shows excellent agreement for small gravity, while for strong gravity only method 1 is able to quantify the shift.
For cool prominences, the results show that by increasing the gravity, the location of the maximum pressure shifts in the downwards direction. This downward shift is largest when the temperature is a flux function. Furthermore, in a strong gravitational potential the three choices of the chosen flux function show large deviations from each other in, for example, the pressure and density. This means that observations could indicate what the most suitable choice of the flux function should be.
The results of the doublelayered prominences have revealed that a doublelayered structure in pressure and density can be created in actual filament configurations. The relative strength of the gravitational potential must be sufficient: if the potential is weak, a ring structure appears, where a cavity surrounds the prominence. As for cool prominences, the location of the maximum pressure and density is shifted increasingly downwards if the gravity importance is increased.
In our accompanying paper (Blokland & Keppens 2011), the stability properties of these equilibria will be analyzed, with special attention to the continuous MHD spectrum. Owing the presence of gravity, gaps or even instabilities may appear in this continuous spectrum. Furthermore, inside these gaps new global modes may occur, which provide us with important information about the internal structure of the prominence. Before investigating the possible appearance of global modes, a detailed analysis of the continuous spectrum will be required.
Acknowledgments
This work was carried out within the framework of the European Fusion Programme, supported by the European Communities under contract of the Association EURATOM/FOM. Views and opinions expressed herein do not necessarily reflect those of the European Commission. R.K. acknowledges financial support by project GOA/2009/009 (K.U.Leuven). The research leading to these results has received funding from the European Commission’s Seventh Framework Programme (FP7/20072013) under the grant agreement SWIFF (project No. 263340, http://www.swiff.eu).
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All Figures
Fig. 1 The accuracy test of FINESSE with respect to the analytical solution derived by Dungey (1953). The quantity L^{2} and L^{∞} are the average and maximum error between the Dungey solution and the numerical solution over the whole interior. 

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In the text 
Fig. 2 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a cool solar prominence surrounded by a hot medium with a gravity g = 0.001. The solar surface is below the figure. 

Open with DEXTER  
In the text 
Fig. 3 Top: the safety factor q at the midplane for a gravity g = 0.001. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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In the text 
Fig. 4 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a cool solar prominence surrounded by a hot medium with a gravity g = 0.100. The solar surface is below the figure. 

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In the text 
Fig. 5 Top: the safety factor q at the midplane for a gravity g = 0.100. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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In the text 
Fig. 6 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a cool solar prominence surrounded by a hot medium with a gravity g = 1.000. The solar surface is below the figure. 

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In the text 
Fig. 7 Top: the safety factor q at the midplane for a gravity g = 0.500. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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In the text 
Fig. 8 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a cool solar prominence surrounded by a hot medium with a gravity g = 1.000 for the case that the density (top) or the entropy (bottom) is a flux function. The solar surface is below the figure. 

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In the text 
Fig. 9 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a doublelayered solar prominence with a gravity g = 0.001. The solar surface is below the figure. 

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In the text 
Fig. 10 Top: the safety factor q at the midplane for a gravity g = 0.001. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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In the text 
Fig. 11 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a doublelayered solar prominence with a gravity g = 1.000. The solar surface is below the figure. 

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In the text 
Fig. 12 Top: the safety factor q at the midplane for a gravity g = 1.000. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

Open with DEXTER  
In the text 
Fig. 13 The twodimensional pressure (redscale) and plasma beta β = 2p/B^{2} (contours) profile for a doublelayered solar prominence with a gravity g = 5.000. The solar surface is below the figure. 

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In the text 
Fig. 14 Top: the safety factor q at the midplane for a gravity g = 5.000. Bottom: the radial derivative of the Shafranov shift Δ(r) as a function of the radius r. 

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In the text 
Fig. 15 A threedimensional impression of the doublelayered solar prominence for gravity parameter g = 5.000. Shown are an isosurface of density, at a value showing the layering of the condensation, with the crosssectional view shown midway this 3D impression. The magnetic field structure is visualized by drawing selected fieldlines, demonstrating the varying twist of the helical configuration. The field lines are colored by the magnetic field strength. The solar surface is below the figure. 

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In the text 
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