Issue 
A&A
Volume 528, April 2011



Article Number  A1  
Number of page(s)  9  
Section  The Sun  
DOI  https://doi.org/10.1051/00046361/201016186  
Published online  16 February 2011 
Nonequilibrium calcium ionisation in the solar atmosphere
^{1}
Institute of Theoretical Astrophysics, University of Oslo,
P.O. Box 1029
Blindern,
0315
Oslo,
Norway
email: sven.wedemeyerbohm@astro.uio.no
^{2}
Center of Mathematics for Applications (CMA), University of Oslo,
Box 1053 Blindern,
0316
Oslo,
Norway
Received: 23 November 2010
Accepted: 10 January 2011
Context. The chromosphere of the Sun is a temporally and spatially very varying medium for which the assumption of ionisation equilibrium is questionable.
Aims. Our aim is to determine the dominant processes and timescales for the ionisation equilibrium of calcium under solar chromospheric conditions.
Methods. The study is based on numerical simulations with the RADYN code, which combines hydrodynamics with a detailed solution of the radiative transfer equation. The calculations include a detailed nonequilibrium treatment of hydrogen, calcium, and helium. Next to an hour long simulation sequence, additional simulations are produced, for which the stratification is slightly perturbed so that a ionisation relaxation timescale can be determined. The simulations are characterised by upwards propagating shock waves, which cause strong temperature fluctuations and variations of the (nonequilibrium) ionisation degree of calcium.
Results. The passage of a hot shock front leads to a strong net ionisation of Ca II, rapidly followed by net recombination. The relaxation timescale of the calcium ionisation state is found to be of the order of a few seconds at the top of the photosphere and 10 to 30 s in the upper chromosphere. At heights around 1 Mm, we find typical values around 60 s and in extreme cases up to ~150 s. Generally, the timescales are significantly reduced in the wakes of ubiquitous hot shock fronts. The timescales can be reliably determined from a simple analysis of the eigenvalues of the transition rate matrix. The timescales are dominated by the radiative recombination from Ca III into the metastable Ca II energy levels of the 4d ^{2}D term. These transitions depend strongly on the density of free electrons and therefore on the (nonequilibrium) ionisation degree of hydrogen, which is the main electron donor.
Conclusions. The ionisation/recombination timescales derived here are too long for the assumption of an instantaneous ionisation equilibrium to be valid and, on the other hand, are not long enough to warrant an assumption of a constant ionisation fraction. Fortunately, the ionisation degree of Ca ii remains small in the height range, where the cores of the H, K, and the infrared triplet lines are formed. We conclude that the difference due to a detailed treatment of Ca ionisation has only negligible impact on the modelling of spectral lines of Ca ii and the plasma properties under the conditions in the quiet solar chromosphere.
Key words: hydrodynamics / shock waves / Sun: chromosphere / waves / radiative transfer
© ESO, 2011
1. Introduction
Modern observations unambiguously show that the chromosphere of the Sun is very dynamic and inhomogeneous (see the reviews by, e.g., Schrijver 2001; Judge 2006; Rutten 2007; WedemeyerBöhm et al. 2009). The interpretation of chromospheric observations, which often involves the construction of numerical models, thus must take into account spatial and temporal variations. Unfortunately, many simplifying equilibrium assumptions that can be made for the low photosphere, are not applicable for the layers above. A realistic chromosphere model must therefore account for deviations from the equilibrium state in the context of an atmosphere that changes on short timescales and small spatial scales. A successful example is the explanation of the formation of “calcium grains” by Carlsson & Stein (1997). Other examples of simulations with a timedependent nonequilibrium treatment include the ionisation of hydrogen (Carlsson & Stein2002, hereafter referred to as Paper I; Leenaarts & WedemeyerBöhm2006; Leenaarts et al.2007) and the concentration of carbon monoxide (Asensio Ramos et al. 2003; WedemeyerBöhm et al. 2005). When an individual process, be it a chemical reaction or atomic transition, changes on finite timescales longer than the dynamic timescales of the atmosphere, then it becomes necessary to solve a system of rate equations instead of the much simpler statistical equilibrium equations. In Paper I, it was shown that the resulting variation of the hydrogen ionisation degree is significantly reduced due to slow recombination rates. The ionisation degree then depends not only on the local gas temperature, density, and the radiation field but also on the history of these properties. Already Rammacher & Cuntz (1991) considered the nonequilibrium ionisation of magnesium (Mg) and calcium (Ca) in their abinitio solar chromosphere models. Their numerical implementation included a nonlocal thermodynamic equilibrium (NLTE) approximation with very simplified twolevel atoms for Mg iiiii and Ca iiiii.
In this paper, we investigate the Ca iiiii ionisation balance in detail. The study is based on RADYN simulations similar to the hydrogen case in Paper I. The numerical simulations are described in Sect. 2. The results of this study are presented in Sect. 3, followed by a discussion and conclusions in Sect. 4.
2. Numerical simulations
We use onedimensional radiation hydrodynamic simulations calculated with RADYN, which are in most aspects very similar to the earlier simulation runs by (Carlsson & Stein 1992, 1994, 1995; Paper I). Here, we summarise only the most important properties. More details can be found in Paper I and references therein.
The simulation code RADYN solves the equations of mass, momentum, energy, and charge conservation together with the nonLTE radiative transfer and population rate equations, on an adaptive mesh in one spatial dimension. It takes into account nonequilibrium ionisation, excitation, and radiative energy exchange from the atomic species H, He, and Ca with backcoupling on the hydrodynamics. Also, the effect of motion on the emitted radiation from these species is considered. Hydrogen and singly ionised calcium are modelled with sixlevel atoms and helium with a ninelevel atom. Furthermore, doubly ionised helium is included. The transitions between all considered atomic levels are treated in detail. Each line is described with 31 − 101 frequency points, whereas 4 − 23 frequency points are used for each continuum. Other elements than H, He, and Ca are taken into account in the form of background continua in LTE, which are derived with the Uppsala atmospheres program (Gustafsson 1973).
The boundary conditions are the same as for the simulations in Paper I. The lower and upper boundaries are both transmitting. The lower boundary is located at a fixed geometrical depth, which corresponds to 480 km below τ_{500} = 1 in the initial atmosphere. We again use the same piston as in Paper I to excite waves at the bottom, which then propagate through the atmosphere. The piston velocity is based on Dopplershift observations in a Fe I line at λ = 396.68 nm in the wing of the Ca H line (Lites et al. 1993). The upper boundary condition is located at a height of 10 Mm. It represents a corona on top of the simulated layers with a temperature set to 10^{6} K and corresponding incident radiation (Tobiska 1991). The dynamic simulation has an overall duration of 3600 s.
The numerical simulation is characterised by shock waves, which are excited as acoustic disturbances of small amplitude through the piston at the lower boundary. They propagate upwards and steepen into shocks with a sawtooth profile above the photosphere. The simulated chromosphere is therefore subject to strong fluctuations in all hydrodynamic quantities. It takes a few 100 s until the first shock waves transform the initially hydrostatic atmosphere into the characteristic dynamic atmosphere. The first 600 s of the simulation are therefore excluded from the analysis.
A large number of additional short simulation runs are carried out, which are used for a timescale analysis (see Sect. 3.2). Each run starts from a snapshot of the detailed timedependent (TD) simulation in the time window 600 s to 2350 s. The initial atmosphere of the individual runs contains the statistical equilibrium (SE) solution for the thermodynamic state in that snapshot. In the next time step, the atmosphere is perturbed by increasing the gas temperature by 1% and the timeevolution is followed for 50 s. In addition, we calculate the statistical equilibrium state of the perturbed atmosphere. For each snapshot in the dynamic simulation we thus have the following data: (i) the statistical equilibrium solution of that snapshot; (ii) the timeevolution after a perturbation has been applied; and (iii) the final equilibrium state corresponding to the perturbed atmosphere.
Fig. 1
Calcium model atom with the five lowest energy levels of Ca ii, a continuum level (Ca iii), and all included bb and bf transitions. Energies are not to scale. 
2.1. The calcium model atom
The calcium model atom contains 5 bound states of singly ionised calcium (Ca ii) and a continuum level (i = 6), which represents the next ionisation stage (Ca iii). The lowest energy level with i = 1 is the ground state of Ca ii (4s ^{2}S). We also include the two important energy level pairs of 4p ^{2}P (i = 2,3) and 4d ^{2}D (i = 4,5). All five allowed radiative boundbound (bb) transitions are considered: the H and K resonance lines, and the infrared triplet (IRT). Also all five radiative boundfree (bf) transitions with the corresponding photoionisation continua from the five lowest levels to level i = 6 are included. The model atom is illustrated in Fig. 1.
3. Results
3.1. Ionisation fraction
In the solar chromosphere, calcium is mostly present in singly and doubly ionised form, i.e. as Ca ii and Ca iii, respectively. We therefore neglect neutral calcium and define the Ca iiCa iii ionisation fraction as the ratio of the population density of doubly ionised calcium n_{Ca III} and the population density of all included Ca ions (n_{Ca, total} = n_{Ca II} + n_{Ca III}). For our six level atom it reduces to (1)where n_{i} is the population density of level i and n_{Ca III} = n_{6}. In the following, we refer to χ_{Ca} as Ca iiiii ionisation fraction. The variation of χ_{Ca} is shown in Fig. 2 as a function of column mass density in the initial radiative equilibrium atmosphere (thick line). It has a minimum of 2 × 10^{4} in the middle photosphere at lgm_{c} = 0.0, which corresponds to z_{0} ≈ 180 km on the height scale of the initial model. Like the hydrogen ionisation fraction (dashed line) it rises with height but less steeply. At the base of the transition region, χ_{Ca} ≈ 5% is reached. The grey lines in Fig. 2 illustrate the temporal evolution of the Ca iiiii ionisation fraction during the simulation. The thin dotted lines are the 5% and 95% percentiles, which enclose the typical data range of χ_{Ca}. While the temporal variation is small below the middle photosphere, the fluctuations cover usually two orders of magnitude in the layers above. This is caused by the upward propagating shock waves.
In Fig. 3, the Ca iiiii ionisation fraction χ_{Ca} is shown as function of time for three different Lagrangian locations, i.e. at fixed column mass densities. The corresponding geometrical heights z vary in time. For orientation, the labels in each panel specify the geometrical height z_{0} in the initial atmosphere. Please note that the fluctuations of the ionisation degree appear much larger at a fixed geometrical height compared to a fixed column mass density because the atmospheric stratification and with it the height of the transition region is influcenced by the propagating shocks.
Fig. 2 Ionisation fractions of calcium (χ_{Ca}, thick solid, see Eq. (1)) and of hydrogen (dashed) as a function of column mass in the initial radiative equilibrium atmosphere. The height scale z_{0} of the initial atmosphere is given as reference. The Ca iiiii ionisation fraction rises from a minimum of 2 × 10^{4} at lgm_{c} = 0.0 (z ≈ 180 km) in the low photosphere to ~ 5% at the base of the transition region. The grey lines represent χ_{Ca} in simulation snapshots at an interval of 10 s during the whole simulation sequence of 3600 s. The thin shortdashed lines are the 5% and 95% percentiles. 
Fig. 3 Logarithmic Ca iiiii ionisation fraction as function of time at different Lagrangian locations. The labels refer to the corresponding geometric height in the initial atmosphere. The lines represent the results from the nonequilibrium simulation (solid) and for statistical equilibrium (dotted) calculated for the same values of the hydrodynamic variables. The horizontal lines are the corresponding timeaverages. 
The ionisation degree in the timedependent nonequilibrium simulation (TD, solid line in Fig. 3) is compared to the statistical equilibrium values (SE, dotted line in Fig. 3). Both are calculated for the same atmospheric states. The differences between both cases are hardly discernible in the lower panel, which refers to the top of the photosphere. It shows that the ionisation fraction does not deviate considerably from the statistical equilibrium values in the lower atmosphere. The deviation is somewhat larger but still moderate in the upper chromosphere at heights around z ~ 1400 km (upper panel in Fig. 3). At times of minimal ionisation, the timedependent and statistical equilibrium results are very similar. At phases of higher ionisation in connection with passing shock fronts, the timedependent simulation gives slightly smaller peak values, which lag behind the SE solution by 5 to 10 s. The timeaverage of the SE case is ~ 27% larger than the TD result (see horizontal lines).
In the middle chromosphere at heights around z ~ 1000 km (see middle panel of Fig. 3), the SE ionisation fraction (dotted line) varies over two orders of magnitude on time scales of a few tens of seconds. In contrast, the detailed timedependent simulation produces a Ca iiiii ionisation fraction that cannot follow the rapid changes (solid line). After a strong increase and a shockinduced peak, which is similar in both cases, the ionisation fraction decays so slowly in the TD simulation that already the next shock front has arrived before the equilibrium value can be attained. As we shall see in Sect 3.3, this behaviour is caused by a relatively slow net recombination process. There is also a general time difference of the order of 5 to 10 s between the occurrence of the ionisation peaks in the timedependent simulation compared to the SE approach. At heights around z ~ 1000 km, the TD ionisation fraction nevertheless varies strongly between values of ~ 10^{3} and ~ 10^{1}. Although the temporal evolution of χ_{Ca} is very different for the TD and SE case at those heights, the timeaverages are relatively similar. The SE average is only ~ 14% smaller than the TD result (see horizontal lines).
3.2. Timescales
In the following, we derive the relaxation timescale of the Ca iiiii ionisation fraction (i) numerically from the temporal evolution of an initially perturbed atmosphere (Sect. 3.2.1) and (ii) from the eigenvalue analysis of the rate matrices (Sect. 3.2.2).
Fig. 4
Relaxation timescale (solid lines) and gas temperature (dotdashed) as function of column mass and time in the dynamic simulation. The thick lines represent the relaxation timescale and the temperature averaged in time over all time steps between t = 600 s and t = 2350 s. Two individual time steps are drawn as thin lines: t = 1600 s (grey) and t = 1620 s (black). The dotted vertical lines mark the temperature peak and the minimum timescale for this time step. For reference, the height scale (z_{0}) of the initial state is given on top. 
3.2.1. Numerical relaxation timescale
The simulation runs are used to determine a numerical timescale as function of time by analyzing each time step in the time range from 600 s to 2350 s individually (see Sect. 2). For each time step, the timescale is derived from the exponential relaxation of the Ca iiiii ionisation fraction towards the equilibrium state of the perturbed atmosphere. The timeaveraged relaxation timescale is then calculated by averaging over the timescales of the individual time steps. This average timescale is shown in Fig. 4 as function of column mass (thick solid line). It is very small in the photosphere (<1 s) and increases strongly with height until a maximum with values of the order of 1 min is reached at heights around z = 900 km. The individual time steps show exactly the same behaviour in the photosphere, whereas the maximum in the chromosphere can reach values of up to 150 s in some cases. In the middle chromosphere above, the timescale is decreasing towards a minimum for all time steps. The average timescale drops to ~ 10 s at z_{0} = 1200 km. The individual time steps also show a minimum but the exact position varies owing to the passage of shock waves. Values down to only a few seconds are found. The timescale starts to rise again at even larger heights but gets very small at the hightemperature transition region.
A number of successive individual time steps are represented by thin lines in Fig. 4. They demonstrate the response of the relaxation time scale (solid lines) to the passage of a shock wave (gas temperature as dotdashed lines). At first glance, it seems as if the relaxation timescale and gas temperature are neatly anticorrelated, i.e., the shortest time scales are found at the positions with the highest gas temperatures. This would be expected from high temperatures resulting in large ionisation rates and thus small timescales.
A closer look, however, reveals that the minimum timescale is found at a height slightly below the temperature peak. This can be seen at t = 1620 s (thin black lines in Fig. 4). The height difference is marked by dotted vertical lines. At the beginning of the shock wave passage in the photosphere, when it is still a disturbance with small temperature amplitude, the timescale at the position of the disturbance is mostly set by the thermodynamic state of the background atmosphere and thus the aftermath of previous shock waves. It is only at heights of z > 900 km, where the shock has steepened enough to have a significant effect on the timescale. There, a local timescale minimum develops at the height of the temperature peak. While the shock front continues to propagate upwards in the atmosphere, the peak temperature grows, resulting in shorter and shorter timescales. The timescale minimum starts to appear lower than the peak temperature. This height difference grows during the passage through the chromosphere until values of the order of Δ z ~ 100 km are reached. From the time at which the locations of the temperature peak and the timescale minimum coincide, the relaxation timescale drops from a few 10 s to just a few seconds. This behaviour is commonly found for all shock events.
When looking at the data as function of time at a fixed geometric height, the height offset translates into a small time difference between the occurrence of the temperature peak and the minimum timescale. This time difference decreases in most cases with height from a few 10 s around z ~ 1000 km to only a few seconds around z ~ 1300 km. There are examples where the time difference does not show such a height dependence but rather varies around values of just a few seconds. The time and height offsets are caused by the influence of the hydrogen ionisation on the recombination rates of calcium via the electron density. See the analysis of the transition rates in Sect. 3.3 for more details.
3.2.2. Timescales derived from eigenvalue analysis
As in Paper I, we use the eigenvalues of the transition rate matrix to determine the involved timescales and to indicate the processes governing the timescales. The rates in the dynamic simulation are affected by the previous history of the atmospheric state. The corresponding timescales are therefore not directly comparable to timescales derived from the numerical experiments in Sect. 3.2.1. Therefore, we use the statistical equilibrium state corresponding to the hydrodynamic variables of a given snapshot (see Sect. 2).
The Lagrangian timederivative of the population densities is given by the rate equations: (2)with n being the vector of the level populations and P the rate matrix. The matrix element P_{ij} of the rate matrix is the transition rate per atom from level i to level j with P_{ii} = − ∑ _{j}P_{ij}.
The matrix elements depend on the population densities in general through the nonlinear radiation terms. If these nonlinearities are not dominant we may write the solution to Eq. (2) in terms of eigenvectors and eigenvalues of the rate matrix (Paper I; Judge 2005). For the Ca model atom (Sect. 2.1) with 5 bound states and a continuum level (i = 6, Ca iii), the solution for the relaxation process can then be written as (3)Here, v_{i} is the ith eigenvector of the rate matrix P, λ_{i} is the corresponding eigenvalue, and c_{i} is a coefficient, which depends on the initial conditions. The equilibrium state corresponds to the eigenvector with a zero eigenvalue. All other eigenvalues are negative and represent the evolution of the level populations toward their equilibrium values. The longest timescale, on which the system relaxes towards the equilibrium state, is then given by the inverse of the smallest (in absolute value) nonzero eigenvalue.
Fig. 5 Numerical relaxation timescale as function of column mass determined numerically (solid line) compared to the timescale determined from eigenvalues of the rate matrix in the initial statistical equilibrium states (dotdashed). The thick lines represent the averages over all time steps between t = 600 s and t = 2350 s, whereas the thin lines are for a particular time step at t = 1620 s. Minimum and maximum values for both dynamic and eigenvalue timescales during the considered time window are shown as grey dotted lines. For reference, the height scale at t = 1620 s is given on top. 
In Fig. 5, the timescales from the eigenvalue calculation are compared to the numerically determined relaxation timescales described in Sect. 3.2.1. The timescales averaged over all snapshots between t = 600 s and t = 2350 s match closely throughout the whole atmosphere. The eigenvalue and numerical timescales also match very well for the individual snapshots. This shows that in the case of calcium ionization, the timescales do not depend strongly on the nonlinear parts of the rate matrix and we have a convenient way of calculating the ionization/recombination timescales from an eigenvalue analysis of the rate matrix.
3.2.3. Timescales of individual processes
We now investigate which processes dominate the relaxation timescale by modifying the entries of the rate matrix prior to determining the eigenvalue timescale. The resulting timescales have qualitatively the same run with height but differ in their absolute value. Leaving out the collisional rates does not change the overall timescale in the middle chromosphere because the collisional transitions occur on timescales that are up to 5 orders of magnitude larger compared to the overall timescale. Also setting the radiative bb transition rates to zero has no noticeable effect on the timescale. Setting the rates R_{1 6} and R_{6 1} for the radiative bf transition between the ground level (i = 1) and the continuum (i = 6, Ca III) to zero changes the timescale only slightly.
We now set all matrix elements to zero except for the entries of individual bf transitions. A rate matrix with nonzero entries only for R_{1 6} and R_{6 1} results in timescales of up to a few thousand seconds in the middle chromosphere. It implies that this transition, which connects the most populated energy level (i = 1) with the ionisation continuum, does not govern the overall timescale. It is the relaxation between level i = 3 and the continuum, which produces the shortest timescales, followed by the transition between level i = 2 and the continuum. Both transitions have timescales of the order of a few 10 s. The ratio of the timescale with just a single transition and the timescale for the full rate matrix is about 2 for the transition 3 − 6 and ~ 3 for 2−6. The ratios for the transitions with lower level 4, 5, 1 are ~ 20, ~ 10, and ~ 70, respectively. We conclude that the transitions between the metastable levels (2 and 3) and the continuum are the most important for setting the timescale for ionization/recombination. Including only these transitions result in a timescale that is only ~ 18% longer than the timescale derived from the full rate matrix.
Fig. 6
Ca iiiii ionisation fraction (left column, solid line, left axis), gas temperature (left column, dotdashed line, right axis), and normalised rates (right column) as a function of column mass for four time steps (rows from top to bottom) in the dynamic simulation. The rates for the radiative transitions from the bound levels 1−5 to the continuum (i = 6, abbreviated “c”) are divided by the total Ca number densities. Positive rates indicate ionisation, negative rates recombination. The sum of all radiative bf transitions is represented by the thick solid line. The gas temperature is repeated in the right column as reference (dotdashed line). The height axis for the individual time step is shown at the top of each panel. Please note the different data ranges for the individual time steps. 
3.3. Transition rate analysis
In contrast to the hydrogen case discussed in Paper I, the shortest timescales do not coincide exactly with the temperature peaks in the shock fronts (see Sect. 3.2). In this section, we show that this behaviour is caused by the dependence of the recombination rates on the density of free electrons, which is influenced by the ionisation/recombination timescale of hydrogen. For the Ca model atom considered here, the recombination process involves a collision between a free electron and a Ca iii ion (see, e.g., Mihalas 1978,p. 130f). Calcium is only a minor electron donor in the solar atmosphere, whereas already small changes in the hydrogen ionisation fraction can lead to significant fluctuations of the electron density. As shown in Paper I, the hydrogen ionisation/recombination timescale is on average on the order of one to several hours in the chromosphere but can be strongly reduced in hot shock fronts. The timescales can then get as short as 10 s to 20 s. The resulting delayed release of electrons has a direct effect on the recombination rates of Ca so that the related timescales reach their minimum only shortly after the occurrence of the temperature peak.
Fig. 7
Temporal evolution at a fixed geometric height of z = 1200 km. Top: total Ca number density n_{Ca,total} and relative level populations n_{i} / n_{total}. Middle: net radiative transition rates P_{r ij} for the bf transitions between the bound levels and the continuum together with the overall sum . Bottom: the involved radiative rates R_{ij} and R_{ji} in comparison to the density of free electrons n_{el}. The Ca iiiii ionisation fraction χ_{Ca} (grey dotted line), the gas temperature (grey dashed line), and the inversed relaxation timescale (grey solid line) are shown in all panels as reference. The rates for the transitions from the bound levels 1 − 5 to the continuum (i = 6) are divided by the total Ca number densities. Positive rates indicate ionisation, negative rates recombination. 
In the following, the role of the individual ionisation and recombination processes is illustrated in detail for a typical shock that propagates through the model chromosphere at t ~ 2200 s in the dynamic simulation. Most other shocks in the simulation show the same behaviour. In Fig. 6, the gas temperature, Ca iiiii ionisation fraction, and transition rates are shown as function of column mass density for the selected shock event. The four different time steps (rows from top to bottom) represent different stages of the upward propagating shock wave, which is most clearly seen as excess in gas temperature (dotdashed line in the left column). The corresponding increase in ionisation fraction (solid line in the left column) is comparatively subtle with a peak (if discernible) slightly below the gas temperature peak.
The normalised net rate P_{r,ij} for a radiative transition between level i and level j is given by (4)with the level population densities n_{i} and n_{j} and the radiative transition rates R_{ij} (upwards, i → j) and R_{ji} (downwards, j → i). The boundfree transition rates P_{r,i6} are shown in the right column of Fig. 6 together with the gas temperature as reference. The net rates P_{r,ij} are thus given per Ca ion with positive values indicating net photoionisation and negative values indicating net recombination. Collisional bf transitions have much smaller rates and can be neglected for this analysis. The sum of the radiative rates (thick solid) is close to zero in the lower parts of the model atmosphere (lgm_{c} > −1.0). There, the rates are in or close to equilibrium with the rates of the individual transitions all being small. The sum of the rates is also close to zero in the upper parts of the model atmosphere below the transition region (lgm_{c} ≈ − 5.6) that have not yet been disturbed by the shock wave (e.g., lgm_{c} < −3.5 in the upper row).
In the shock front, the sum of the rates is increased, leading to net ionisation (positive values in the figure). The largest contribution is due to photoionisation from the metastable level i = 3, followed by photoionisation from level i = 2. As the lower levels of these transitions belong to the same term and are energetically close together (see Fig. 1), the transition rates show a very similar behaviour. The photoionisation from the ground level (i = 1) is seen at all heights below the transition region with a local maximum in the shock front, where it has a small but positive contribution to the net ionisation. The normalised rate reaches much larger relative values above the shock front close to the transition region, compensating the recombination in most of the other bf transitions. These large values are a result of the previous shock wave and long relaxation timescales for this transition (see Sect. 3.2.3). The transitions from level i = 4 and i = 5 have much smaller rates with recombination prevailing throughout the model atmosphere. They both behave very similarly because the lower levels are energetically close together.
As the shock propagates through the chromosphere, the normalised photoionisation rates increase significantly. While the sum of the rates (thick solid line) is of the order of 10^{4} s^{1} at the shock front at z ≈ 900 km (top row of Fig. 6), values of ≈ 2.5 × 10^{3} s^{1} are found at z = 1150 km only 50 s later (bottom row). The second row from the bottom (t = 2250 s) shows the instant shortly before the shock wave reaches the transition region (seen as sharp jump in gas temperature around lgm_{c} = −5.6). Once the shock reaches the transition region (20 s later, bottom row), the rates decrease rapidly. Except for a very small and smooth photoionisation from the ground level (i = 1), all other transitions and with it the sum of the rates show recombination in almost the entire model atmosphere from just behind the shock front down to the low photosphere. It demonstrates that the timescales on which the ionisation equilibrium is restored are relatively short – except for a comparatively sluggish photoionisation from the ground level.
In Fig. 7, the time evolution of the shock event is analysed at a fixed geometric height of z = 1200 km. The vertical dotted lines divide the time span into a preshock phase, a phase I (when the shock occurs) and a phase II (during the passage of the shock wake). As the processes are complex and the timescales are small, the Ca iiiii ionisation fraction, the gas temperature, and the inverse relaxation timescale are shown in all panels for reference purposes (all scaled to their full data range). The gas temperature (grey dashed line) shows a clear shock signature with a rapid increase, a peak of T_{gas} = 8543 K at t = 2248 s and a slower decay in the shock wake afterwards. The Ca iiiii ionisation fraction (grey dotted line) seems to react on the shock with some delay and also much smoother. It peaks only at t = 2258 s with a value of 3.2%, i.e. 10 s after the occurrence of the temperature peak. The relaxation timescale τ reaches a minimum of τ_{min} = 7.6 s even later at t = 2262 s. The inverse timescale τ^{1} is shown as solid grey line in the figure. While the change in phase I occurs rapidly (with a slope of τ^{1} being between those of the gas temperature and the ionisation fraction), the postshock evolution in phase II is much slower. Then (e.g. at t = 2300 s) the timescale τ is still reduced while the gas temperature and the ionisation fraction are already relatively close to their preshock state again.
The uppermost panel of Fig. 7 displays the total Ca number density n_{Ca,total}, i.e. the sum of levels 1 to 6 (thick solid line, right axis). As the element abundance of Ca is constant in the simulation, it behaves exactly like the gas density. It decreases before the arrival of the shock front and rises rapidly again in the shock front and more gradually in the shock wake afterwards.
The level population densities n_{i}, i.e. the number densities of Ca atoms with their valence electron in a specific energy level i, are divided by the total Ca number density n_{Ca,total} in the uppermost panel. It removes the fluctuations due to the change in gas density and reveals the relative distribution of the Ca atoms over the 6 included levels. At midchromospheric heights, usually 95% or more of all Ca ii ions are in the ground level (i = 1) before and after the shock passage (i.e., in the cool phases). During the passage of a shock wave, the ground level is depopulated but usually maintains at least 70% of n_{Ca,total} and thus remains the most populated level at all times. The population densities n_{i} of all other levels with i > 1 increase during the shock passage as Ca ii atoms are excited from the ground level into a higher level. The increase of the population densities of levels 2 and 3 correlates with the change in gas temperature, while levels 4 and 5 react with a delay of 5 s, shortly followed by the continuum level (i = 6). The density of the latter, n_{6}, increases at most to a few percent of n_{Ca,total}. Most Ca atoms therefore remain singly ionised, even during the shock passages. The Ca iii ions are actually by a factor of more than 3 less abundant than the Ca ii ions with an electron in level 3 alone. Ionisation is thus only a “minor process” compared to the boundbound transitions within the Ca atom. The level populations of levels 4 and 5 on the other hand are much smaller than the Ca iii number density. Even if all ions in these levels would ionise, the resulting rise of the Ca iii population would be negligible. Levels 4 and 5 are nevertheless important as upper levels of radiative bb transitions.
The net rates P_{r,ij} for the radiative boundfree transitions are shown as function of time in the middle panel of Fig. 7. They are again given per Ca ion with positive values indicating net photoionisation and negative values indicating net recombination (see Eq. (4)). The sum of the net radiative rates (thick solid line) gives the change of the Ca iii number density and thus the Ca iiiii ionisation fraction. Contributions from collisional bf transitions are again small here. The sum exhibits a net (photo)ionisation in phase I, which peaks shortly (here 1 s) before the gas temperature, and rapidly turns into net recombination for phase II. While the shock wake is passing through the analysed height point, the recombination becomes weaker and the rates approach zero again. The bf transitions from levels 3 and 2 contribute most (in that order) and show the same temporal behaviour as the sum. The net radiative boundfree rate for the ground level, P_{r,16}, exhibits net photoionisation throughout the whole shock passage. The rate increases with time and reaches a first hardly discernible maximum together with or shortly before the gas temperature. It roughly stays at the same level and smoothly declines in phase II. At that time, it is the only transition with a positive net contribution. The boundfree transitions for levels 4 and 5 behave very much oppositely, producing a net recombination the whole time. The absolute values, however, stay small and even below the maximum recombination rates of P_{r,26} and P_{r,36} that are reached during phase II.
The peculiar behaviour of the net rates P_{r,26} and P_{r,36} is caused by a temporal delay between the photoionisation (n_{j}R_{ji}) and the recombination part (n_{i}R_{ij}, cf. Eq. (4)). The photoionisation terms increase first and produce the strong net photoionisation in phase I, while the recombination part reaches a maximum only about 20 s later. At that time both parts are equal, resulting in a zero net rate. Afterwards the recombination part, which lags behind, stays larger than the ionisation part, causing the net recombination in phase II. The differences in the rates R_{ij} are balanced by the number densities of the lower levels so that the recombination part is only slightly smaller than the photoionisation part. In contrast, the recombination into level i = 1 is much smaller than the corresponding photoionisation, which produces the smooth behaviour in time.
Finally, the radiative boundfree transition rates R_{i 6} for i = 1,2,3 are shown in Fig. 7. The photoionisation rates R_{2 6} and R_{3 6}, which are almost identical due to the similarity of their lower levels, exhibit no sharp response to the passage of the shock wave. In contrast, the recombination rates R_{6 3} and R_{6 2} increase strongly during the shock phase I. The rate R_{6 3} is larger than R_{6 2} but both only differ by a constant factor. The strong increase of these rates correlates very well with the inverse relaxation time scale (grey solid line) and the electron density (solid black line). It demonstrates that the relaxation timescale is set by the recombination into the bound levels 3 and 2, which is directly depending on the density of free electrons. With hydrogen being the main electron donor in the chromosphere, the temporal behaviour of the recombination rates R_{6 3} and R_{6 2} is therefore similar to the H ii number density. This leads to the conclusion that the Ca iiiii ionisation in the quiet solar chromosphere is governed by the finite timescales on which hydrogen reacts on strong temperature changes.
Fig. 8 Emergent intensity in the Ca ii K line: temporal evolution of the line core intensity (top row) and timeaveraged spectrum (bottom row) at the solar limb (μ = 0.05, left column) and at diskcentre (μ = 1.0, right column). Each panel contains the results from the nonequilibrium simulation (I_{K,TD}, solid) and from the statistical equilibrium solution (I_{K,SE}, red thick dashed) together with the corresponding difference (I_{K,TD} − I_{K,SE}) / I_{K,SE}) between both (solid grey line at the top of each panel). The grey areas in the bottom panels represent the full data ranges of all intensity profiles during the simulation sequence between t = 600 s and t = 2350 s. 
4. Discussion and conclusions
The ionisation/recombination timescales, which are here derived from 1D RADYN simulations, are too long for the assumption of an instantaneous ionisation equilibrium to be valid. On the other hand, the timescales are not long enough to warrant an assumption of a constant ionisation fraction. We find noticeable deviations from the ionisation equilibrium in the middle model chromosphere but in general the Ca iiiii ionisation fraction remains small. The error due to the often made simplifying assumption of statistical equilibrium is therefore negligible for most applications. The effect is barely visible in the synthesized intensity for the diagnostically important spectral lines of Ca ii, i.e., the H and K lines and the infrared triplet. This finding is illustrated for the Ca ii K line in Fig. 8. The differences in the emergent intensity between the statistical equilibrium approach (I_{K,SE}) and the timedependent nonequilibrium simulation (I_{K,TD}) are very small and hardly discernible in the temporal evolution of the intensity at a fixed wavelength position in the line core (top row) and even smaller (order of 0.1%) in the average spectrum (bottom row). The relative difference (I_{K,TD} − I_{K,SE}) / I_{K,SE} reveals peaks with values of up to a few percent for wavelengths close to the line core. This is true both at diskcentre (right column) and close to the limb (left column). The differences are even smaller away from the line core and the emission peaks. Noticeable deviations occur only in connection with shock fronts and thus sharp intensity increases. There, the effect is caused by a small temporal offset in the evolution of the level populations in the TD case with respect to the SE case, like it is seen for the ionisation fraction in Fig. 3. It is safe to conclude that the timedependent nonequilibrium treatment of the Ca iiiii ionisation appears to be of minor importance for the lower atmosphere in quiet Sun regions.
One restriction of the simulations is the use of only one spatial dimension, which could cause the shock wave profiles to be too extreme with potentially too high peak temperatures. In 3D, the shock fronts are expected to be weaker owing to the larger number of degrees of freedom. The consequences of the deviations from the Ca iiiii ionisation equilibrium would be even less important in that case. Furthermore, we neglect the effect of incident radiation from the corona on the photoionisation of Ca. Most important in that respect would be the Lyman alpha line at λ = 121.5 nm. However, the Lyman α photons have too little energy to ionise Ca ii from the ground state (11.88 eV or λ = 104.4 nm). The photoionisation edges for levels 2 and 3, on the other hand, both lie close to the Lyman alpha line. The incident radiation certainly matters most at large heights close to the transition region. There, however, photoionisation from the ground level dominates, which is obviously not influenced by Lyman alpha photons. We conclude that the RADYN simulations employed here are sufficiently realistic for an evaluation of the importance of nonequilibrium effects for the ionisation of calcium in the context of a strongly varying chromosphere in quiet Sun regions.
Acknowledgments
This work was supported by a Marie Curie IntraEuropean Fellowship of the European Commission (6th Framework Programme, FP62005Mobility5, Proposal No. 042049) and a grant from the Research Council of Norway (No. 191814/V30).
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All Figures
Fig. 1
Calcium model atom with the five lowest energy levels of Ca ii, a continuum level (Ca iii), and all included bb and bf transitions. Energies are not to scale. 

In the text 
Fig. 2 Ionisation fractions of calcium (χ_{Ca}, thick solid, see Eq. (1)) and of hydrogen (dashed) as a function of column mass in the initial radiative equilibrium atmosphere. The height scale z_{0} of the initial atmosphere is given as reference. The Ca iiiii ionisation fraction rises from a minimum of 2 × 10^{4} at lgm_{c} = 0.0 (z ≈ 180 km) in the low photosphere to ~ 5% at the base of the transition region. The grey lines represent χ_{Ca} in simulation snapshots at an interval of 10 s during the whole simulation sequence of 3600 s. The thin shortdashed lines are the 5% and 95% percentiles. 

In the text 
Fig. 3 Logarithmic Ca iiiii ionisation fraction as function of time at different Lagrangian locations. The labels refer to the corresponding geometric height in the initial atmosphere. The lines represent the results from the nonequilibrium simulation (solid) and for statistical equilibrium (dotted) calculated for the same values of the hydrodynamic variables. The horizontal lines are the corresponding timeaverages. 

In the text 
Fig. 4
Relaxation timescale (solid lines) and gas temperature (dotdashed) as function of column mass and time in the dynamic simulation. The thick lines represent the relaxation timescale and the temperature averaged in time over all time steps between t = 600 s and t = 2350 s. Two individual time steps are drawn as thin lines: t = 1600 s (grey) and t = 1620 s (black). The dotted vertical lines mark the temperature peak and the minimum timescale for this time step. For reference, the height scale (z_{0}) of the initial state is given on top. 

In the text 
Fig. 5 Numerical relaxation timescale as function of column mass determined numerically (solid line) compared to the timescale determined from eigenvalues of the rate matrix in the initial statistical equilibrium states (dotdashed). The thick lines represent the averages over all time steps between t = 600 s and t = 2350 s, whereas the thin lines are for a particular time step at t = 1620 s. Minimum and maximum values for both dynamic and eigenvalue timescales during the considered time window are shown as grey dotted lines. For reference, the height scale at t = 1620 s is given on top. 

In the text 
Fig. 6
Ca iiiii ionisation fraction (left column, solid line, left axis), gas temperature (left column, dotdashed line, right axis), and normalised rates (right column) as a function of column mass for four time steps (rows from top to bottom) in the dynamic simulation. The rates for the radiative transitions from the bound levels 1−5 to the continuum (i = 6, abbreviated “c”) are divided by the total Ca number densities. Positive rates indicate ionisation, negative rates recombination. The sum of all radiative bf transitions is represented by the thick solid line. The gas temperature is repeated in the right column as reference (dotdashed line). The height axis for the individual time step is shown at the top of each panel. Please note the different data ranges for the individual time steps. 

In the text 
Fig. 7
Temporal evolution at a fixed geometric height of z = 1200 km. Top: total Ca number density n_{Ca,total} and relative level populations n_{i} / n_{total}. Middle: net radiative transition rates P_{r ij} for the bf transitions between the bound levels and the continuum together with the overall sum . Bottom: the involved radiative rates R_{ij} and R_{ji} in comparison to the density of free electrons n_{el}. The Ca iiiii ionisation fraction χ_{Ca} (grey dotted line), the gas temperature (grey dashed line), and the inversed relaxation timescale (grey solid line) are shown in all panels as reference. The rates for the transitions from the bound levels 1 − 5 to the continuum (i = 6) are divided by the total Ca number densities. Positive rates indicate ionisation, negative rates recombination. 

In the text 
Fig. 8 Emergent intensity in the Ca ii K line: temporal evolution of the line core intensity (top row) and timeaveraged spectrum (bottom row) at the solar limb (μ = 0.05, left column) and at diskcentre (μ = 1.0, right column). Each panel contains the results from the nonequilibrium simulation (I_{K,TD}, solid) and from the statistical equilibrium solution (I_{K,SE}, red thick dashed) together with the corresponding difference (I_{K,TD} − I_{K,SE}) / I_{K,SE}) between both (solid grey line at the top of each panel). The grey areas in the bottom panels represent the full data ranges of all intensity profiles during the simulation sequence between t = 600 s and t = 2350 s. 

In the text 
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