Ionization rates in the heliosheath and in astrosheaths
Spatial dependence and dynamical relevance^{⋆}
^{1}
Institut für Theoretische Physik IV, RuhrUniversität Bochum,
44780
Bochum, Germany
email: kls@tp4.rub.de; hf@tp4.rub.de
^{2}
Argelander Institut, Universität Bonn,
53121
Bonn,
Germany
email:
hfahr@astro.unibonn.de
^{3}
Polish Space Science Center, Bartycka 18A, 00716
Warsaw,
Poland
email:
bzowski@cbk.waw.pl
^{4}
Centre for Space Research, NorthWest University,
2520
Potchefstroom, South
Africa
email:
Stefan.Ferreira@nwu.ac.za
Received:
22
January
2013
Accepted:
5
December
2013
Context. In the heliosphere, especially in the inner heliosheath, mass, momentum, and energyloading induced by the ionization of neutral interstellar species plays an important, but for some species, especially helium, an underestimated role.
Aims. We discuss the implementation of charge exchange and electron impact processes for interstellar neutral hydrogen and helium and their implications for the subsequent modeling. We especially emphasize the importance of electron impact and a more sophisticated numerical treatment of the charge exchange reactions. Moreover, we discuss the nonresonant charge exchange effects.
Methods. We discuss rate coefficients and revise the influence of the crosssections in the (magneto)hydrodynamic equations for different reactions and also their representation in the collision integrals.
Results. Electron impact is in some regions of the heliosphere, particularly in the heliotail, more effective than charge exchange, and the ionization of neutral interstellar helium contributes about 40% to the mass and momentumloading in the heliosheath. The charge exchange crosssections need to be modeled with higher accuracy, especially in view of the latest developments made in describing them.
Conclusions. The ionization of helium and the electron impact ionization of hydrogen need to be taken into account in modeling the heliosheath and, in general, astrosheaths. Moreover, the charge exchange crosssections need to be handled in a more sophisticated way, either by developing better analytic approximations or by numerically solving the collision integrals.
Key words: Sun: heliosphere / stars: winds, outflows / hydrodynamics / atomic processes
Appendices are available in electronic form at http://www.aanda.org
© ESO, 2014
1. Introduction
1.1. General aspects
It is wellknown that not only the interstellar plasma, but also the interstellar neutral gas influences the largescale structure of the heliosphere (Baranov & Malama 1993; Scherer & Ferreira 2005; Müller et al. 2008; Zank et al. 2013). This influence is a consequence of the coupling of the neutral gas (consisting mainly of hydrogen and helium) to the solar wind plasma (mainly protons with a small contribution of α particles (He^{2+})) via charge exchange, photoionization, and electron impact processes. Elastic collisions and Coulomb scattering have been discussed in Williams et al. (1997).
In selfconsistent models of heliospheric dynamics, so far only the influence of neutral hydrogen is considered by taking into account its charge exchange with solar wind protons and its ionization by the solar radiation (e.g. Fahr & Ruciński 2001; Pogorelov et al. 2009; AlouaniBibi et al. 2011, and references therein). The dynamical relevance of both the electron impact ionization of hydrogen, although recognized by Malama et al. (2006), and the photoionization of helium, although recognized as being filtrated in the inner heliosheath (Rucinski & Fahr 1989; Cummings et al. 2002), have not yet been explored in detail. Only Malama et al. (2006) included helium selfconsistently in the heliospheric modeling and discussed the additional ram pressure generated by the charged helium ions.
In recent years the discussion has rather concentrated on the correct crosssection for the charge exchange between a proton and a hydrogen atom. While it has been demonstrated by Williams et al. (1997) that the modeling results regarding the largescale structure (location of the termination shock and heliopause) are insensitive to the alternative crosssections given by Fite et al. (1962) and Maher & Tinsley (1977), it was revealed that it is important for the neutral gas (shape of the hydrogen wall and densities inside the termination shock, see, e.g. Baranov et al. 1998; Heerikhuisen et al. 2006). Subsequently, the significance of the revised crosssections by Lindsay & Stebbings (2005) has first been recognized by Fahr et al. (2007) and has been discussed in more detail in the context of global heliospheric modeling by Müller et al. (2008), Bzowski et al. (2008), and Izmodenov et al. (2008).
It has also been recognized that electron impact ionization is not only important for the neutral gas distribution (e.g., Rucinski & Fahr 1989; Möbius et al. 2004; Izmodenov 2007) but to some extent also for the largescale structure of the heliosphere (Fahr et al. 2000; Scherer & Ferreira 2005; Malama et al. 2006). However, these studies contain neither a comparison of the electron impact ionization rates with those of the other two processes, nor a systematic analysis of their dynamical influence.
In addition to addressing the first of these problems here, we show that not only the ionization of neutral hydrogen influences the dynamics in the heliosphere, but that neutral helium must also be expected to play a role. Furthermore, we discuss charge exchange reactions of hydrogen and helium in view of their relevance to astrospheres, particularly to astrosheaths. In astrospheres the relative speed between a stellar wind and the flow of neutrals from the interstellar medium can be up to an order of magnitude higher than in the solar case, see for example the Mdwarf VPeg 374 (Vidotto et al. 2011) or for hot stars (e.g. Arthur 2012).
Before quantitatively addressing these topics, we briefly indicate other heliospheric and astrophysical applications for which the ionization rates studied here also are of interest.
The charge exchange process has recently gained more interest because it is responsible for the outerheliospheric production of energetic neutral atoms (see Fahr et al. 2007,for a comprehensive review) that are presently observed with the IBEX mission (McComas et al. 2009, 2012; Funsten et al. 2009; Dayeh et al. 2012). In this context, Grzedzielski et al. (2010) investigated the distribution of different pickupion (PUI) species, which are products of ionization processes in the inner heliosheath, and Borovikov et al. (2011) discussed their influence on the plasma state of the inner heliosheath. Furthermore, Aleksashov et al. (2004) began to explore the influence of charge exchange of hydrogen atoms with solar wind protons and their impact on the structure of the heliotail. The charge exchange processes of heavier elements were studied in connection with the Xray production in the inner heliosphere (Koutroumpa et al. 2009), while these processes in the local interstellar medium are discussed by Provornikova et al. (2012).
Astrophysical scenarios for which the use of correct ionization rates is crucial (Nekrasov 2012) comprise the Xray emission from galaxies (Wang & Liu 2012), from the interstellar medium (de Avillez & Breitschwerdt 2012), and from hot stars (Pollock 2012), the influence of neutral atoms on astrophysical shocks (Blasi et al. 2012; Ohira 2012), and the jets of active galactic nuclei (Gerbig & Schlickeiser 2007).
We here concentrate on the relative importance of the different ionization processes for the heliosheath and for astrosheaths, that is for the regions between the solar or stellar wind termination shock/s and the helio or astropauses, then to later incorporate into corresponding selfconsistent (magneto)hydrodynamic ((M)HD) modeling with the BoPo (Scherer & Ferreira 2005) and the CRONOS code (see Wiengarten et al. 2013, for an application and references therein). We demonstrate the significance and dynamical relevance of electron impact ionization of hydrogen and of helium in the entire heliosphere by employing the wellestablished heliospheric model by Fahr et al. (2000) and Scherer & Ferreira (2005). The model includes for our computation charge exchange between neutral and ionized hydrogen, electron impact of hydrogen, and photoionization of hydrogen. Considering elastic collisions and Coulomb scattering (Williams et al. 1997) is beyond the scope of this paper.
In Sect. 2 we first give a short introduction to the BoPo code and in Sect. 3 discuss the charge exchange and electron impact crosssections. In Sect. 4 we describe the interaction terms used in the Euler equations (see Appendix A). In Sect. 5 we then concentrate on the electron impact and its contribution to the interaction terms, which is followed by a discussion of the neutral interstellar helium loss in the inner heliosheath in Sect. 6. Section 7 contains a discussion of the nonresonant charge exchange and its relevance to the outer heliosheath. Finally, we assemble our ideas and critically assess our findings in the concluding Sect. 9.
1.2. Astrospheres and the heliosphere
An astrosphere is a generalization of the heliosphere. The physics is similar, except that for huge astrospheres, such as those around hot stars (Arthur 2012), where a cooling function needs to be included in the region beyond the termination shock. Moreover, for hot stars the Strömgren sphere can be larger then the astrosphere, and thus photoionization can be dominant in the entire astrosphere. Nonetheless, HI regions can exist around hot stars (Arnal 2001; Cichowolski et al. 2003) and thus ionization processes become important. Therefore, an HII region with a variable degree of ionization is a better concept than the classical Strömgren sphere. For example, for the Sun the Strömgren radius R_{S} = 2.2 × 10^{10} cm (Fahr 1968) is smaller than the solar radius, while its HII region is considerably larger (Lenchek 1964; Ritzerveld 2005; Fahr 2004).
Some cool stars exist like VPeg 374 (Vidotto et al. 2011) which have stellar wind speeds (≈2000 km s^{1}) much higher than that of the solar wind. Moreover, for nearby stars the relative speeds between the star and the interstellar medium can differ by factors between 0.2 to 2 compared with the interstellar medium that surrounds the solar system (Wood et al. 2007). For these high relative speeds crosssections of other processes and different species may become important.
In most of the stellar wind models (e.g. Lamers & Cassinelli 1999) the wind passes through one or more critical points (surfaces) after which it freely expands. This freely expanding continuous blowing wind is physically similar to the solar wind. In an ideal scenario without neutrals and cooling the solutions can simply be scaled from one scenario to the other.
The models for astrospheres are based on MHD equations (see Appendix A) in the same way as for the heliosphere. Because a fleet of spacecraft has been or is exploring the heliosphere by in situ as well as remote measurements, the knowledge of that special astrosphere is much more detailed than that of astrospheres. In the following we make no difference between astrospheres or the heliosphere. All we discuss applies to the heliosphere as well as to astrospheres immersed in partly ionized clouds of interstellar matter.
One interesting feature of some nearby astrospheres is their hydrogen walls, which are built beyond the astropauses by charge exchange between interstellar hydrogen and protons. This feature can be observed in Lymanα absorption (Wood et al. 2007), which in turn allows one to determine the stellar wind and interstellar parameters of some nearby stars. Because the hydrogen wall is built up in the interstellar medium, where the temperatures are low (<10^{4} K) and because they increase for the heliosphere only by approximately a factor two toward the heliopause, the charge exchange process involved is that between protons and hydrogen as well as some helium reactions, such as He^{+} + He, He^{2+} + He, and He^{+} + He^{+}, which have large crosssections even at low energies. Owing to the low temperatures, electron impact is not effective, because the involved energies are lower than the ionization energy. Up to now, only hydrogen walls were observed, which, nevertheless, allows for some insights into the structure of nearby astrospheres. Helium walls as a result of heliumproton charge exchange were not found (Müller & Zank 2004b). Nevertheless, some heliumhelium reactions with sufficiently large crosssections (see Fig. 2 or Tables C.1 and C.2) may result in a helium wall.
2. Heliosphere model
For this analysis a detailed model of the heliosphere is not necessarily needed. Nevertheless, we used a snapshot of a dynamic heliosphere model computed with the BoPomodel code (Scherer & Ferreira 2005). This model includes three species, protons, neutral hydrogen, and, from the latter, newly created ions, the pickup protons (PUI_{SH+}). The effective temperature distribution, that is the weighted sum of the proton and PUI temperatures of the model, is shown in Fig. 1. The modeled effective temperature nicely reproduces those inferred by IBEX (Livadiotis et al. 2011).
Fig. 1 Proton temperature distribution in the dynamic heliosphere (Scherer & Ferreira 2005). Above the solar pole the features of a highspeed stream can be identified. Because of the influence of the PUI_{SH+} the temperature inside the termination shock is a few 10^{5} K, corresponding to thermal energies of up to a few tens of eV. The temperature in the inner heliosheath is 10^{6} K, which was inferred by IBEX (Livadiotis et al. 2011). 

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Fig. 2 Charge exchange crosssections as a function of energy per nucleon for protons (left panel), He^{+}ions, and αparticles (right panel) of the solar wind with interstellar helium and hydrogen. In the upper part of the two panels we show the crosssections, while the lower parts show the ratio to σ_{cx}(H^{+} + H → H + H^{+}). The black curve in the panels is the reaction H + H^{+} → H^{+} + H. As can be seen in the lower panel the reactions He^{+} + He, He^{2+} + He, and He^{2+} + He^{+} have similar crosssections as that of H + H^{+} and thus are important in modeling the dynamics of the largescale astrospheric structures. Note the different yaxis scales between different panels. 

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Fig. 3 Rate coefficients β(v) = vσ(v) instead of the crosssections as in Fig. 2. We assumed that there is no difference in the relative speeds from the collision integrals and those to be used for the crosssections , i.e., . 

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The PUI_{SH+} are created by a resonant charge exchange process between a neutral hydrogen atom and a proton (1)in which an electron is exchanged between the reaction partners. Because the first reactant is a fast proton, the neutral hydrogen atom resulting from this interaction is an energetic (fast) neutral atom (ENA), which here is assumed to leave the heliosphere without further interaction. The second reactant, a slow interstellar hydrogen atom, becomes ionized and is immediately picked up by the electromotive force of the heliospheric magnetic field that is frozenin in the solar wind. The initial PUI_{H+} velocity distribution is ringlike with a maximum of twice the solar wind speed (Vasyliunas & Siscoe 1976; Isenberg 1995; Gloeckler & Geiss 1998). It very quickly becomes pitchangle isotropized, thus transforming into a nearly spherical shell distribution.
During this charge exchange process the total ion density does not change, but because of the velocity difference between the proton and neutral hydrogen atom, the solar wind momentum is altered (momentumloading) as is the energy of the fluid, that is the temperature of the solar wind increases and momentum decreases because it is lost through the escaping ENA (Fahr & Ruciński 1999). This temperature increase was observed by the Voyager spacecraft (Richardson & Wang 2010), while model runs including only a single proton fluid resulted in temperatures of a few hundred Kelvin at the termination shock (for an example see Fig.1 in Fahr et al. 2000). This contrasts with the abovementioned multifluid and multispecies models with 10^{5} K at the same location (see Fig. 1). The momentumloading leads to a slowing down of the solar wind, which is indeed observed (Richardson & Wang 2010), in agreement with model attempts (Fahr & Fichtner 1995; Fahr & Ruciński 2001; Fahr 2007; Pogorelov et al. 2004; AlouaniBibi et al. 2011). Moreover, including neutrals removes the Machdisks (Baranov et al. 1971; Pauls et al. 1995; Müller et al. 2001) and thus changes the largescale structure of the astro or heliosphere and again demonstrates the importance of including charge exchange processes for an adequate description.
The dynamic BoPo model (Fahr et al. 2000; Scherer & Ferreira 2005) also includes the electron impact (2)in the inner heliosheath, that is the region between the termination shock and the heliopause.
The photoionization inside the termination shock is also included. This leads not only to the abovedescribed momentum and energyloading but, also to a massloading, because new ions are generated.
We briefly mention a few complications that are usually not taken into account. As reported by Lallement et al. (2005, 2010), the direction of the deflected hydrogen and helium inflow can differ by 4°, but see the IBEX results discussed in Möbius et al. (2012). This additional complication was only modeled by Izmodenov & Baranov (2006), while much effort was expended in modeling the hydrogen deflection plane (Pogorelov et al. 2009; Opher et al. 2009; Ratkiewicz & Grygorczuk 2008). The latest IBEX observations (Saul et al. 2013) show that the hydrogen peak moves in longitude during the solar cycle, which according to Saul et al. (2013) is caused by the changing radiation pressure close to the Sun, which affects the effective gravitational force. In the outer heliosphere this effect is assumed to be negligible and, hence, is independent of charge exchange and electron impact processes; it was not taken into account below.
It has been known for decades (Fahr 1979), that close to the Sun helium is focused in the downwind direction, while hydrogen is defocused. This latter effect is again caused by the interaction between the radiation pressure and gravitation that acts on these particles. For a more detailed analysis of the trajectories see Müller (2012).
Because we are mainly interested in the largescale structure far away from the Sun, we can neglect this additional complication, for which the hydrogen and helium fluids have to be treated kinetically (for hydrogen see Osterbart & Fahr 1992).
The ionization processes we discuss are independent of the underlying (M)HD model. If the neutral fluid is treated kinetically (Izmodenov 2007; Heerikhuisen et al. 2008), the distribution functions of the collision integrals cannot be handled by two Maxwellians, but one is determined by the solution of the kinetic equation. Thus the details of the collision terms may vary, but the following principal discussion remains true. Moreover, to avoid the solution of kinetic equations, a multifluid approach with several fluids in different regions is often used (Heerikhuisen et al. 2008; AlouaniBibi et al. 2011; Prested et al. 2012).
Therefore, we used the BoPo code (Scherer & Ferreira 2005) results to visualize and emphasize the aspects discussed (other (M)HD models would be equally suitable), with the intention to draw the attention to these aspects and to point out the need for a selfconsistent model that includes them.
In the next section we discuss some additional charge exchange processes with hydrogen and helium and the electron impact of helium.
3. Charge exchange and electron impact crosssections
A very detailed analysis of the ionization processes at 1 AU that also takes into account temporal variations caused by the solar cycle can be found in Rucinski et al. (1996, 1998, 2003), Bzowski et al. (2013), and Sokół et al. (2013). This is much more complicated for the outer heliosphere, especially in the inner heliosheath, where temporal and spatial variations are mixed and cannot be separated because of the subsonic character of the fluid. To demonstrate the importance of the different effects, it is sufficient for our purpose to use a simplified approach, that is, to assume a stationary model, and discuss the effects along a line of sight between the termination shock and the heliopause in the nose region.
3.1. Charge exchange
In Fig. 2 we show the charge exchange crosssections σ_{cx} as functions of energy per nucleon between protons (left panel) and He^{+}ions and αparticles (right panel) with hydrogen and helium. In the lower part of the panels the different crosssections are normalized to that of the abovementioned standard reaction H^{+} + H → H + H^{+}. All crosssections discussed here are taken from the Redbook^{1} and can be accessed via the ALADDIN webpage^{2}. While for the discussion below the exact values of the crosssections are not important, we still refer to Arnaud & Rothenflug (1985), Badnell (2006), CabreraTrujillo (2010), Kingdon & Ferland (1996), and Lindsay & Stebbings (2005) for more information. Nevertheless, when the crosssections are required for the modeling efforts the more modern results should be taken into account. For convenience the rate coefficients β(v) = vσ(v) we present in Fig. 3.
From the left panel of Fig. 2 one can see that σ_{cx}(H^{+} + H → H + H^{+}) is roughly in the range of 10^{15} cm^{2} below 1 keV, that is the range of interest for heliospheric models. All other crosssections σ_{cx} between protons and neutral H or He are orders of magnitude smaller for slow solar or stellar wind conditions. In the highspeed streams and especially in coronal mass ejections the crosssections like σ_{cx}(H^{+} + He → H + He^{+}), σ_{cx}(H^{+} + H → H^{+} + H^{+} + e) and σ_{cx}(H^{+} + He → H^{+} + He^{+} + e) can become of the same magnitude as σ_{cx}(H^{+} + H → H + H^{+}). For astrospheres with stellar wind speeds in the order of a few thousand km s^{1} the energy range is shifted toward 10 keV up to 100 keV and other interactions, such as other nonresonant chargeexchange processes, need to be taken into account.
While the crosssection σ_{cx} between αparticles and neutral H or He compared to the σ_{cx}(H^{+} + H → H + H^{+}) reaction seem not to be negligible in and above the keVrange (Fig. 2, right panel), the solar abundance of αparticles is only 4% of that of the protons, so that the effect seems to be small. Nevertheless, the mass of He or its ions is roughly four times that of (charged) H, and thus may play a role in mass, momentum, and energyloading.
Most of the crosssections displayed in Fig. 2 are unsuitable for use in a numerical code, because the existing data are fitted in a limited energy range by Chebyshev polynomials as taken from the Aladdin webpage. Using these approximations outside that range leads to unreliable results. For future simulations these crosssections need to be extrapolated to the whole energy range required for the heliosphere and astrospheres, that is from energies about 1 eV to a few 100 keV.
From Tables C.1 and C.2 one sees that the reactions H + He^{+} → p + He and H + He^{2+} → p + He^{+} are a few percent of the H+preaction, but because helium is involved, there may be a change in the total density of the governing equations in the ten percent range. The depletion of helium by charge exchange was discussed by Müller & Zank (2004a), who concluded that it can amount to 2%.
According to Slavin & Frisch (2008), the ionization fraction in the interstellar medium of He^{+} and He is about 0.4, and thus the He^{+} abundances are about 2/3 that of He. Form Fig. 2 and Tables C.1 and C.2 one easily can see that the He^{+} + He reaction has a similar crosssection as that of p + H. The He^{+} fluid should follow a similar pattern than the pfluid in front of the heliopause: the helium ions are slowed down and, via charge exchange with the neutrals, must be expected to build a helium wall. The additional reaction He^{+} + He^{+} → He + He^{2+} with similar crosssections can support the creation of the helium wall. According to Müller (2012), 10% of the neutral helium will become ionized in front of the heliopause. To determine the helium wall a selfconsistent model is needed, which includes the three species He, He^{+}, and He^{2+} and all their reacting channels.
Another consequence of the high He^{+} abundances as modeled by Slavin & Frisch (2008) is that the total ion mass density is remarkably higher than the proton mass density. The latter is usually used to estimate the Alfvén speed, which is proportional to 1/ in the interstellar medium, which is reduced by 10% taking into account the total ion mass, that is the additional He^{+} abundances (Scherer & Fichtner 2014).
For astrospheres with higher stellar wind speeds other reactions such as p + He^{+} → H + He^{+2}, become important as well. A brief discussion is given in Sect. 8.
3.2. Electron impact
The electron impact crosssection σ^{ei} is shown in Fig. 4. We calculated the thermal speed of the electrons assuming thermal equilibrium between protons and electrons (Malama et al. 2006; Möbius et al. 2012), because the electron temperature has, so far, neither been modeled nor observed in the outer heliosphere, while for the inner heliosphere (upstream of the termination shock) it has been modeled (Usmanov & Goldstein 2006) and a limited set of observations in the heliocentric distance range between 0.3 to about 5 AU is available (e.g. Maksimovic et al. 1997). Additionally, care must be taken, because the electron temperature most probably increases during the passage of the plasma across the termination shock (Fahr et al. 2012). Nevertheless, we followed the assumption by Malama et al. (2006), according to which the electrons are in thermal equilibrium with the proton plasma (including PUI_{SH+}). The crosssections were calculated after Lotz (1967) and Lotz (1970), (3)where the index i extends over all relevant subshells up to N. For example, for hydrogenlike atoms N = 1, for helium N = 2, see Lotz (1970). K_{i} is the ionization energy in the i^{th} subshell. The coefficients { a_{i},b_{i},c_{i},q_{i} } are tabulated in Lotz (1970).
Other approaches exist to describe the electron impact crosssections (Mattioli et al. 2007; Mazzotta et al. 1998; Voronov 1997). They are quite similar and differences in details are not of interest for the following discussion.
Fig. 4 Electron impact crosssection σ^{ei} in units of 10^{17} cm^{2} per particle, for the three reactions: H + e → H^{+} + 2e, He + e → He^{+} + 2e, and He + e → He^{2+} + 3e. 

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From the above assumption it is evident that the thermal speed of the electrons is higher by the “mass” factor than that of the protons. The same argument holds true for heavier ions, and thus the thermal speed of αparticles is half of that of the protons. The electron impact crosssections σ^{ei}(H,He) are smaller by roughly a factor 100 than σ_{cx}(H^{+} + H → H + H^{+}). Nevertheless, because the thermal speed of the electrons is, due to the mass factor, 43 times higher than that of the protons, the rate coefficients β_{s} = σ_{s}(v_{rel})v_{rel} between these reactions become similar. The electron impact ionization can dominate in the heliosheath with its high temperatures because there the maximum of its crosssections is about 3 × 10^{17} cm^{2} (He) or 6 × 10^{17} cm^{2} (H), where v_{rel} is assumed to be (4)The index s represents one of the hydrogen or helium ionizing reactions. See Appendix B for a more thorough discussion including the factor f_{e}. Note: if the relative kinetic energy is lower than the ionization energy K_{s} for the species s no ionization of the neutral atom s will occur.
In the outer heliosphere the temperature plays an increasingly essential role, because the relative bulk speed between the ionized and neutral species u_{2} − u_{1} becomes small, and the corresponding thermal speeds increase. This can easily be seen in Fig. 6, where the ratio of the bulk speed to the thermal speed is plotted. Moreover, only electrons with energies higher than the ionization potential can ionize neutral atoms.
4. Interaction terms
The complex dynamics of the largescale system in a multifluid multispecies (M)HD set of equations are only described by Euler equations that include the total density (the sum of all species densities) and the total pressure (the sum of all partial pressures). Moreover, the equations for all ionized and all neutral species need to be treated differently. This set of equations including the total densities and pressures is called the governing equations. The governing equations include the ram pressure and other force densities or stresses (see Appendix A).
Each single species, ionized or neutral, needs to be followed as a tracer fluid, for instance their densities and thermal energy contributions to the governing equations need to be known. This set of equations is called the balance equations.
In most of the hydrodynamic (e.g. Fahr et al. 2000; Scherer & Ferreira 2005) or magnetohydrodynamic models (e.g. Malama et al. 2006; Pogorelov et al. 2009; AlouaniBibi et al. 2011) of the heliosphere the interactions between neutral hydrogen and protons can be written as balance equations and governing equations for the dynamics (Izmodenov et al. 2005). In the balance equations only the interaction terms are needed, which are summed over all interactions terms and is zero, and the two governing equations are the sum of all dynamically relevant ionized and neutral species, respectively. The ENAs are taken into account, so that the sum over all species is zero. The interaction of a PUI_{H+} with a neutral hydrogen atom produces a PUI_{H+} and an ENA. Therefore, the gains and losses in the PUI_{H+} balance equation are zero and thus are omitted. In the governing equations the energetic neutral atoms (ENAs) are neglected, because it is assumed that they do not contribute to the dynamics.
Nevertheless, when we assume to have two distinct populations of ions and neutrals, we must be careful about the heliospheric regions in which the interactions occur:

1.
Inside the termination shock, a charge exchange between H andp produces an ENA_{0} and a PUI_{0}. This new PUI_{0} population is hotter and can also interact with the neutrals, thus producing a new population of ENA_{1} and PUI_{1}. The populations can then interact again with each other, which creates a hierarchy of populations. These secondorder effects may be neglected inside the termination shock (see e.g. Zank et al. 1996; Pogorelov et al. 2006).

2.
In the heliosheath, we have a cooler population of shocked solar wind protons p′ and a hotter shocked PUI′ population. Both can now interact with the neutrals and create additional ENA′ populations that now contribute to the original hydrogen distribution and increases the temperature of the latter. The ENAs can also interact with the ions in the heliosheath and then produce ions that are much faster than the bulk speed. If picked up, they will lose energy to the plasma and heat it. Another plausible scenario is that this hot new PUI′ population, which has energies of keV, may become the seed population for anomalous cosmic rays. A detailed analysis of these heating processes will be conducted in a future study.

3.
Furthermore, new populations of neutrals will be generated in the outer heliosheath and beyond the bow shock (if it exists, Gruntman 1982; BenJaffel et al. 2013; McComas et al. 2012; BenJaffel & Ratkiewicz 2012; Zank et al. 2013; BenJaffel et al. 2013; Scherer & Fichtner 2014). These new populations legitimate the multifluid approach for most of the MHD models (e.g. Pogorelov et al. 2009; AlouaniBibi et al. 2011; Izmodenov et al. 2005).
These new populations of PUIs and ENAs need to be integrated into the governing equations (see Appendix A), while the new balance equations are needed to describe the individual states of the species in mind.
To avoid a clumsy notation in the following we do not distinguish between the different regions of the helio or astrosphere, because the equations are the same. Nevertheless, one should keep in mind that the different populations, with their distinct thermodynamical states, lead to various dynamic effects and need to be taken into account, either by the abovementioned multifluid approach or similar approaches (Fahr et al. 2000).
Because we assumed that all involved species have the same bulk speed as that of the corresponding governing equations, the balance momentum equation can be neglected. In the energy equation one only needs to treat the thermal energy of the species in mind.
This assumption implies a caveat: because of the different behavior of the neutral hydrogen and helium fluid inside the heliopause, for example, the defocusing of hydrogen and focusing of helium close to the Sun, these species may not be handled as one fluid in the entire heliosphere. At least close to the Sun a kinetic treatment is necessary (e.g. Osterbart & Fahr 1992; Izmodenov et al. 2003). Nevertheless, for the present study it is a reasonable approximation, because a difference of a few km s^{1} in the bulk speeds is negligible in the relative speeds, which are determined mainly by the thermal speed in the heliosheath.
We discuss the individual balance terms from the general (M)HD set of equations (see Appendix A) with the following convention: σ^{s} is the cross section for s ∈ {cx, ei, pi}, where cx stands for the charge exchange, ei for the electron impact, and pi for the photoionization. denotes the rate coefficient, where r denotes the different relative speeds r = c,m,e for the continuity equation c, the momentum equation m, and the energy equation, and ij denote the corresponding interaction. The superscripts {σ, I_{coll}} denote the different relative speeds defined by McNutt et al. (1998). For details see Appendix B. Most useful are also the charge exchange rates , where n_{X} is the number density in the corresponding balance equation: for example, the balance term for protons. The balance term for the momentum equation is a vector . The quantities ρ_{X},v_{Y},E_{X} denote the density, bulk velocity, and total energy density of species. The indices X include that of the governing equations with the indices Y ∈ {i, n} for the ions i and neutrals n and for each species X ∈ {Y, p, H, H^{+}, H^{0},...}, where p are the protons, H the neutral hydrogen atoms, H^{+} the newly generated ions (pickup hydrogen), and H^{0} the newly created energetic neutral H atoms. We denote with the thermal speed for temperature T_{X} with the Boltzmann constant κ and mass m_{X}.
In the following the balance equations are expressed in a form discussed by McNutt et al. (1998) and the governing equations as sum of the balance equations, where the ENA contribution to the neutral component is neglected. The equations given below are only valid for particles with the same mass. Interaction terms between heavy and light species need a correction term (see Eq. (20) in McNutt et al. 1998). This is discussed in more detail in Appendix B.
The balance and governing equations for the interaction between protons, PUI_{H+}, the neutrals, and the hydrogenENAs are explicitly stated below. Because the indices {PUI, ENA} are not unique and can also be used for other ions or neutrals, we here used to denote the PUI and ENAs for hydrogen.
The balance terms in the continuity equations are where the dynamics is governed by the sum of protons and PUI_{SH+} for the ions (index i) as well as for the neutral component (index n) The ENA_{SH0} are taken into account, so that the sum over all species is zero. Because the ENAs produced in the solar wind have velocities of about 400 km s^{1}, they will leave the system without further interaction. In that case the hydrogen population is diminished, as indicated by the last two terms in Eq. (10). In the heliosheath where the speeds of the ENAs and the solar wind plasma are similar, the total number of neutrals remains constant and the last two terms of Eq. (10) vanish. As explained above, the secondorder interactions with a PUI_{H+} and a neutral hydrogen atom produces a PUI_{H+}′ and an ENA_{H0}′, which is sorted into the PUI_{H+} and ENA_{H0} balance equations. Therefore, gains and losses in PUI_{H+} and ENA_{H0} balance equation are zero, for instance, and .
The balance terms in the momentum equations read
Here the exchange between the PUI_{SH+} and hydrogen atoms must be taken into account, because the momentum loss of the PUI_{H+} is not balanced by the momentum gain from the hydrogen.
As discussed above, we assumed that the bulk velocities of all charged and neutral species are v_{i} = v_{p} = v_{H0} and v_{n} = v_{H} = v_{H+}. This assumption does not hold everywhere, for example, inside the termination shock of the heliosphere the velocities of the newly created ENAs are high and they escape the system without further interaction. In the heliosheath, where the bulk velocities of the charged and neutral particles are similar, the ENA contribution to the hydrogen population is not to be neglected. For a discussion to include secondorder effects see Zank et al. (1996), Pogorelov et al. (2006), Izmodenov (2007), and AlouaniBibi et al. (2011).
The balance terms in the governing equations are: For better reading, we omitted the subscripts for electron impact and photoionisation in the rates ν^{ei} and ν^{pi} because they are unique.
The energy equations are slightly more complicated. We first defined the total energy E_{k} of a species k as , where P_{i} is the (partial) thermal pressure of species i, and the ram pressure of either the sum of ions (j = i) or the sum of the neutrals j = n. The thermal energy after the exchange is according to McNutt et al. (1998)(17)
where we have indicated with the superscript {m, e} that the relative speeds from the collision integrals for the momentum and energy equation have to be taken (see Appendix B). Moreover, with the above assumption v_{p} = v_{H0} and v_{H} = v_{H+} some terms in the energy balance equation vanish.
For the governing energy equations we have to include the change in the total energy, which adds the following terms because of v_{p} = v_{H0} and v_{H} = v_{H+} all other contributions vanish.
The balance terms in the governing energy equations are To save space we waived the explicit sums.
The photoionization rate is given by with r_{0} = 1 AU. For the electron impact rates, was assumed and for the electron number density n_{e} = (n_{p} + n_{PUIH+}) (quasi neutrality). For the relative speed a similar approach was used as in Appendix B. Because of the high thermal speeds of the electrons (assuming thermal equilibrium between ions and electrons), the relative speed is roughly equal to the thermal electron speed. As discussed in Chalov & Fahr (2013), the electron temperature may increase farther downstream the termination shock.
Usually all interaction terms with the newly created PUIs and ENAs are neglected, that is all terms in the above equations that contain terms with H + H^{+}, p + H^{0} and H^{+} + H^{0} are set to zero. These assumptions may not hold beyond the termination shock where the speeds of charged and neutral particles can be in the same order depending on the location.
Other forms of the interaction terms are discussed by Williams et al. (1997). A detailed description of the relative speeds is given in Appendix B.
To include a new species into the model, the above equations have to be extended: for each species a separate set of Euler equations is required. Differences in the ion velocities are assumed to be equalized on a kinetic scale by waveparticle interactions. Thus, for the much larger MHD scales we assumed that all ion velocities are equal to the bulk velocity of the main fluid.
Therefore, the dynamics is governed by the above equations with the indices {i, n}, where now the additional species need to be added. Including helium, the set of the balance equations consists of those for H, He, H^{+}, He^{+}, and He^{2+}, and the governing equations for ions and neutrals. In the latter the total density ρ_{i} is the sum of all ionized species, that is ρ_{i} = ρ_{H+} + ρ_{He+} + ρ_{He2 +} and ρ_{n} = ρ_{H} + ρ_{He} for the neutral species. The governing momentum equation for {i, n} describes the bulk velocity of the system, where the pressure term is the sum of the partial pressures of all relevant species. The energy equations have to be treated analogously. The momentum equations for the individual species can be neglected for regions far away from obstacles, because we assumed, that due to waveparticle interactions all bulk velocity differences vanish. Close to obstacles, such as the Sun or stars or a shock front, the individual bulk velocities of the species may differ by the Alfvén speed, as observed in the solar wind for αparticles (Marsch et al. 1982; Gershman et al. 2012), and L. Berger (priv. comm.). Because the Alfvénic disturbances travel along the magnetic field, which is assumed to be in the shape of a Parkerspiral, the radial speed in the outer heliosphere is the bulk speed for all species. Nevertheless, these particles can induce a perpendicular pressure as well as the diamagnetic effects described for PUI_{SH+} (see Fahr & Scherer 2004b,a). A thorough discussion of the effects of αparticles in the heliosheath is far beyond the scope of this paper and will be studied in future work.
For all practical purposes, one needs to solve the governing equations, including the continuity and energy balance equations of all other species, because they can influence the dynamics in the inner heliosheath and, in general, that of astrosheaths.
The above set of equations concerning the interaction terms now have to be extended to include the charge exchange between ionized and neutral hydrogen and/or helium atoms, as well as the electron impact reactions for the two neutral species. A complete set of equations can be found in Appendix C in Tables C.1 and C.2.
Because, the solar abundance of αparticles is 4% (LieSvendsen et al. 2003) of that of the protons, and because the singly charged helium is even less abundant, we neglect in the following the interaction with ionized solar wind helium and neutral interstellar hydrogen or helium atoms. For other astrospheres these abundances can change and the stellar wind speed can also be much higher, in that case the charge exchange and electron impact crosssections discussed below can have completely different relevance.
All the reactions discussed in Appendix C can play an important role depending on the astro or heliosphere model.
For example, astrospheres can have bulk velocities in the range of a few thousand km s^{1} and hence their relative energies per nucleon can be in the ten keV range, where reactions, like He^{2+} + H → H^{+} + He^{+} become important, see Fig. 2 or Tables C.1 and C.2. These can be neglected in the heliosphere. In the following section we concentrate on the electron impact ionization of H and He and show that they play a nonnegligible role in the inner heliosheath and inside the termination shock.
Note that including species other than hydrogen in charge exchange processes can change the number density of electrons, for example, He^{+} + He^{+}→ He^{+} + He^{2+} + e. This must be taken care of in equations that contain the electron number density (not discussed here).
5. Electron impact ionization of H and He
The crosssection for the electron impact reactions were shown in Fig. 2. To demonstrate their importance we estimate their contribution to the governing continuity equations. They can be written in the following form (see Eq. (9)): where we neglected all charge exchange reactions between H and He, either neutral or ionized, because the rate coefficients β_{i} are lower than a factor 10^{3} of those for electron impact or photoionization. The only comparable ratecoefficient is that between protons and neutral hydrogen atoms. For the corresponding balance equation see Appendix A. The notation or indicates the ionization of neutral helium into singly and doubly ionized helium. Moreover, we neglected all the higherorder interaction between PUIs and ENAs.
Care must also be taken when the interstellar ionized helium is taken into account. The abundances of singly charged helium can be on the same order as those of the neutral component (Wolff et al. 1999). The incidence of He^{++} in the interstellar medium has been modeled (Slavin & Frisch 2008) and is negligible according to the model.
First we assumed that the interstellar abundances of helium are 10% of those of hydrogen (Asplund et al. 2009), but see also Möbius et al. (2004) and Witte (2004) for the determination of the helium content based on observations inside 5 AU. Furthermore, we approximated the helium mass m_{He} to be four times that of the hydrogen mass m_{H}. Then we can write for the region inside the heliopause (27)The consequences for the governing equations are discussed in Appendix A.
Furthermore, the photoionization rate at 1 AU for hydrogen and helium at solar minimum is roughly 8 × 10^{8} s^{1} (Bzowski et al. 2012, 2013). With these assumptions, we can rewrite Eqs. (25) and (26) To determine these rates, we need to estimate the relative velocities. Because, to our knowledge, the electron and helium temperatures in the heliosheath have been neither observed nor modeled, we assumed that the electron temperature T_{e} and helium temperature are the same as the proton temperature T_{p}, that is T_{p} = T_{e} = T_{He+} = T_{He2 +} = 10^{6} K. The temperatures in the interstellar medium for the neutral hydrogen T_{H} and helium T_{He} are on the order of 8000 K, but the exact values do not play a role, because only the sum of the ion and neutral temperature determines the relative speeds for protons v_{rel,p} and electrons v_{rel,e}. For our estimation we assumed that the relative speeds . Furthermore, we assumed that in the heliosheath the relative bulk speeds are km s^{1}, and neglecting the temperature of the neutrals (see above), we obtain The relative speed of the electrons corresponds to an energy eV, and we can then read from Fig. 4 that the electron impact crosssection to produce singly or doubly ionized helium differs roughly by a factor 4, and that of singly ionized helium is approximately the same as for hydrogen. Thus cm^{2}. From Fig. 2 we determine the charge exchange crosssection σ^{cx}(H^{+} + H) ≈ 10^{15} cm^{2}. The electron density in the inner heliosheath is assumed to be ρ_{p + H+} = ρ_{e} = 3 × 10^{3} cm^{3}. With these estimates we derive for the different rates in that region see www.cbk.waw.pl/~jsokol/solarEUV.html for the photoionization rates of H, He, Ne, O, and He^{+}. From this it is evident that all the rates are on the same order. Now Eqs. (28) and (29) can be written as From Eq. (30) we learn that the massloading in the inner heliosheath for the combined He and H electron impact interaction terms is an important effect, and not only that of hydrogen needs to be taken into account, but helium contributes about 20% to the massloading. From Eq. (31) it is evident that within our estimation the mass loss of neutrals through electron impact is 20% that of the charge exchange between solar wind protons and neutral interstellar hydrogen.
Fig. 5 Ratios as defined in Eq. (36). The left panel shows the ratio for hydrogen while the right panel presents the ratio for singly ionized helium. Positive values indicate that the charge exchange process (H + H^{+} → H^{+} + H) dominates, while for negative values the electron impact is more relevant. Note the different scales in the color bars. 

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For the momentum equations we derive after a similar consideration where we assumed that the interstellar bulk velocity of helium is the same as that of hydrogen.
The energy balance terms become In Fig. 5 we present the ratios of the rates for electron impact ionization of hydrogen and helium (singly charged). To enhance the visibility, we normalized to the charge exchange rate σ(H^{+} + H) in the following form (36)where X ∈ {H, He}. The ratio r was estimated from an existing dynamic model with highspeed streams over the poles. The crosssections were calculated from the modeled plasma parameters, hence they are not selfconsistently taken into account. Nevertheless, this demonstrates the relative importance of electron impact ionization in the heliosphere, which finally has to be modeled selfconsistently. Figure 5 shows a contribution of about 20%, as discussed above, especially in the tail region. The significance can be seen when estimating the Alfvén speed, which is inversely proportional to the square root of the total density of charged particles. An enhancement of 20% in the charged density (according to the model by Slavin & Frisch 2008) will lead to approximately 10% reduction in the Alfvén speed (Scherer & Fichtner 2014). This is important for the recent discussion about the bow shock (McComas et al. 2012). It can even be seen in Fig. 5 that the electron impact ionization is not negligible inside the termination shock.
As can be inferred from Fig. 5, the electron impact is significant almost everywhere inside the heliopause and dominates close to the heliopause and in the tail region, at least for the ionization of hydrogen. The structures in the heliotail visible in Fig. 5 are caused by the previous solar cycle activities, which are still propagating down the heliotail (see Scherer & Fahr 2003b,a; Zank & Müller 2003). For our calculations, we estimated the crosssection from the relative velocity and temperature taken from the model, with the assumption of thermal equilibrium. It also shows that our rough approximations above are quite good.
The discussion shows that electron impact effects for hydrogen and helium needs to be taken into account to improve heliospheric models, which otherwise can lead to results that differ in extreme cases by 20% (see Eqs. (30) to (36)).
6. Helium loss in the inner heliosheath
To interpret the IBEX observation for helium and other species (Bzowski et al. 2012) it is important to know how much helium is lost in the inner heliosheath. To estimate the order of these losses, we used the balance continuity equation for helium (37)where we took only the photoionization to singly charged helium from Table C.1 in Appendix C, and the electron impact to both ionization states as losses. Other losses are small, even the photoionization to the doubly charged state (Rucinski et al. 1996). The plasma is subsonic in the heliosheath, and the divergence term may be neglected with the usual assumption of incompressibility for subsonic flows. Nevertheless, because due to the ionization some particles are lost, this assumption holds no longer true, strickly speaking. If we assume for the moment that we can neglect the divergence, Eq. (37) has the solution (38)with . For the following estimation, we furthermore assumed a lower limit for the photoionization rate at 1 AU ν^{pi}(1 AU) = 8 × 10^{8} s^{1} (Rucinski et al. 2003) and that it decreases like r^{2}, that the heliosheath has a width of 40 AU, and that the photoionization rate inside the heliosheath has a constant value ν^{pi}(100 AU) = 8 × 10^{12} s^{1}. Since the total temperature in the heliosheath is 10^{6} K, see Livadiotis et al. (2011), but also Richardson et al. (2008) for a lower proton temperature, with the values for the electron impact as discussed above, we derive τ ≈ 300 years. Particles with speeds of 20, 25, or 30 km s^{1} need ≈9.45, 7.56, and 6.29 years to travel through the inner heliosheath. Inserting these numbers into Eq. (38) leads to a decrease of 2–3% integrated over that distance. Increasing the distance between the heliopause and termination shock, that is for higher latitudes or different solar activity, these numbers will increase approximately linearly.
This loss is on the same order as that determined by Cummings et al. (2002), who discussed, in view of anomalous cosmic ray composition, a loss of helium in the heliosheath in the order of 5% in the inner heliosheath. Obviously these losses may be even more pronounced for more extended astrosheaths.
7. Charge exchange with particles of different masses
For the interaction of particles with different mass, the approach by McNutt et al. (1998) can be applied. The calculation of the collision integrals between two species requires knowing the functional form of the chargeexchange crosssection, that is, one has to solve integrals of the form
where  g = V_{2} − V_{1}  is the modulus of the velocities V_{1},V_{2} of the individual particles of species 1 or 2, and the indices { c,m,e } indicate the integrals for the continuity, momentum and energy equation (see Eq. (A.1)), k ∈ {1, 3} for {c, e}, respectively. The collision integrals are equivalent to the balance terms S^{c,e} and S^{m}, which are their solution under simplifying assumptions, for an example see below.
In most derivations it is assumed that σ^{cx}(g) is nearly constant (Heerikhuisen et al. 2008; McNutt et al. 1998; AlouaniBibi et al. 2011). This is in general not the case; even for σ^{cx}(H + p) this holds only below energies of 5 keV. Unfortunately, the integrals can only be solved analytically for a polynomial functional dependence of σ^{cx}. The solution to this dilemma was sketched by McNutt et al. (1998) by developing σ^{cx} into a Taylor series and assuming that after a given order all higherorder terms vanish. McNutt et al. (1998) required that only the zeroth order is relevant, and determined the characteristic speed () at which the crosssections should be taken. The authors calculated the characteristic speed by inserting the first order of the Taylor expansion of σ^{cx} into the integrals and requiring that the sum of these integrals vanishes. This allows one to determine a characteristic speed, which follows mathematically from the mean value theorem for integrals. Nevertheless, this procedure holds only as long as the crosssections are weakly varying. In general, this is not true and as correction the higherorder terms shall be used (see Appendix B).
Moreover, the relative velocities calculated for the collision integrals are mutually distinct and also not identical with the characteristic speeds discussed above, see also Appendix B. With a notation introduced in Appendix B, which is slightly different from that of McNutt et al. (1998), the dimensionless parameter α reads (41)with the individual particle velocities v_{1},v_{2} and thermal speeds w_{1},w_{2} for the particles of species 1 or 2, respectively. Then one finds that the abovementioned different speeds normalized to the thermal speeds are functions of α alone that is , where j ∈ {c, m, e, P} for the continuity, momentum, and energy equations and j = P for the thermal pressure, respectively. The indices i ∈ {cx, rel} are the speeds needed for the characteristic speeds in the charge exchange crosssection and the corresponding relative speeds, respectively. All speeds are called collision speeds in the following. The explicit formulas are stated in Appendix B.
Fig. 6 α parameter throughout the heliosphere. α is the ratio of the modulus of the relative bulk velocity to the thermal speed of the two species, see Eq. (41). 

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In Fig. 6 the parameter α is presented throughout the heliosphere. It can be seen that it ranges from values near zero close to the heliopause, in the tail region, and in the outer heliosheath, where the relative velocities are low, but the thermal ones high, to values in the range of 30 inside the termination shock, where the relative velocity is high and the thermal speed low. In the left panel of Fig. 7 the dependence of the from α is shown and in the right panel of Fig. 7 the relative “error” is presented.
The collision speeds for the continuity equations nicely follow the approximation for α > 1, while the speeds and for the momentum and energy equation, respectively, differ strongly for all values of α, as well as those for the continuity equations for small α, as can be nicely seen in the right panel of Fig. 7.
Fig. 7 Characteristic collision speeds normalized to the thermal speed as a function of the parameter α (left panel) and the relative “error” , r ∈ { c,m,e }. 

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With these speeds, the charge exchange terms read
In these formulas i ∈ {1, 2} stands for the respective particle species, and the ± sign has to be chosen in such a way that a loss in one species (for example, ions) is a gain in another one (for example, fast neutrals).
Even when the neutrals are treated kinetically (Izmodenov et al. 2005; Heerikhuisen et al. 2008), the moments of the collision integrals must be calculated, because the ions are handled with an MHD approach, in which implicitly the solution of those for Maxwelliandistributed particles are modeled. Thus, these calculations have to be repeated with a different velocity distribution, for instance, a κdistribution (Heerikhuisen et al. 2008), to obtain the required collision speeds.
Moreover, as discussed briefly in Appendix B, this discussion is only valid when the crosssections are mainly independent of the collision speeds . This is in general not true; even for the reaction H + p this holds only for energies (speeds) below 5 keV (≈1000 km s^{1}), and thus the assumption of a nearly constant crosssection may not be valid for highspeed streams of the solar wind, nor even for astrospheres of hot stars, where the speed is on the order on a few 1000 km s^{1}. Thus higherorder approximations of the Taylor expansions are required. Because this leads to clumsy expressions, which also need a lot of computational effort, it may be better for practical purposes to solve the collision integrals numerically as in Fichtner et al. (1996).
8. Astrospheres revisited
Most of the aspects discussed above hold in general for astrospheres. Nevertheless, because the stellar winds and the interstellar medium can be very different from that of the heliosphere, care must be taken which of the collision channels displayed in Tables C.1 and C.2 needs to be taken into account. For example, a stellar wind of 2000 km s^{1} has kinetic energies of about 20 keV and most of the interactions become important. Such wind speeds were derived by Vidotto et al. (2011) and are common in winds around hot stars (Arthur 2012; Decin et al. 2012). For such astrospheres, there may be strong bow shocks, because the interstellar wind is comparatively strong. We may then encounter the situation where the low first ionization potential (FIP) elements cannot reach the inner astrosheath, but the highFIP elements do. This is an interesting aspect when discussing the acceleration of energetic particles. Such a filtering of lowFIP elements occurs in the heliosphere concerning carbon, which becomes easily ionized already in the interstellar medium and thus cannot penetrate into the heliosphere (Cummings et al. 2002).
In astrospheres additional effects can play a role, such as elastic collisions into an excited atomic state and subsequent photon emission, thus energy loss. Recombination can take place, as well as Bremsstrahlung or synchrotron radiation, when a strong enough magnetic field is present, which can lead to additional cooling of the stellar wind plasma.
Astrospheres show a variety of shapes, and all can be described by the set of (hybrid) (M)HD equations discussed in Appendix A. If the surrounding interstellar medium is partially ionized, it must be carefully determined which of the charge exchange reactions play a role. Especially, the charge exchange between particles with different masses needs to be carefully implemented, because in the collision integrals m_{i}/(m_{i} + m_{j}) (where m_{i},m_{j} denote the corresponding mass of species i,j) appears as a factor.
9. Conclusions
We have demonstrated that electron impact ionizations are important processes inside the heliopause and particularly in the heliosheath, while other charge exchange processes, except for that of H^{+} + H → H^{+} + H, have been neglected because of their small crosssections for solar wind speeds. They become important when modeling astrospheres, where the stellar wind speeds can be higher by a factor 5 or more (up to 3000 km s^{1}, see Arthur 2012). In that case it is evident from Fig. 2 that a thorough discussion of the charge exchange between hydrogen and helium atoms, both neutral and ionized, is needed. The newly generated PUIs heat the stellar wind even inside the termination shock, so that the threshold for electron impact ionization is exceeded, and here electron impact plays a role, which then can additionally diminish the neutral helium density by 3%.
Care must also be taken because the crosssections are taken from a fit curve that may deviate by up to 10% from the data, see also the discussion by Bzowski et al. (2013). Moreover, for the continuity, momentum, and energy equations the different collision speeds need to be taken into account in the modeling efforts. Additionally, depending on the representation of the crosssections, the assumption that they are nearly constant, as in McNutt et al. (1998), and Heerikhuisen et al. (2008) over a wide range, does not hold anymore. Therefore, either higherorder corrections in the Taylor expansion of the crosssections need to be taken into account, or a numerical estimation of the collision integrals is needed in modeling the heliosphere or astrospheres.
Especially for astrospheres, which can have relative speeds of a few thousand kilometers per second, the nonresonant charge exchange processes for helium become increasingly important. For the huge astrospheres of Ostars of tens of parsecs (Arthur 2012) the ionization of other species should be carefully considered, because they can play a role in heating the supersonic stellar wind.
Moreover, during highspeed solar wind streams or coronal mass ejections traveling into the outer regions of the heliosphere the dynamics of the solar wind and propagating shock fronts of CMEs will be influenced by charge exchange processes, including electron impact, and by different helium ionizing processes.
For (M)HD simulations, one can use the governing equations, that is, one set of Euler equations for the combined ions and one for the sum of neutrals. The densities of all included species can be handled with a test particle approach, that is, only solving the corresponding continuity equation to derive the correct density distribution in the heliosphere. A better strategy is to solve in addition the energy equation for each species to compute their contribution to the total pressure selfconsistently. In the governing energy equation a sophisticated heat transport can also be included. In a forthcoming work we will include these processes in our model, specifically add a new species, helium, as well as the heat flow caused by the electrons, and study the relevance of all these effects.
Finally, there are clear indications that the electrons downstream of the termination shock can easily attain much higher temperatures compared than those of the protons (Chalov & Fahr 2013).
We also point out that the He^{+} abundance modeled by Slavin & Frisch (2008) reduces the Alfvén speed by about 10%, which again shows the importance of including helium in models.
We have shown here that all charge exchange processes need to be reanalyzed carefully to minimize the errors in largescale models and to improve the fits to the newly available IBEX and Voyager data.
Acknowledgments
K.S. and H.F. are grateful to the Deutsche Forschungsgemeinschaft, DFG for funding the projects FI706/151 and SCHE334/101. M.B. was supported by the Polish Ministry for Science and Higher Education grant NN203513038, managed by the National Science Centre. S.E.S.F. thanks the South African National Research Foundation for financial support.
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Online material
Appendix A: Set of MHD equations
A general set of the Eulerian continuity, momentum, and energy equations is the following (see e.g. Boyd & Sanderson 2003): (A.1)

v_{j}= fluid velocity

ρ_{j}= fluid density

E_{j}= internal energy of fluid

P_{j}= pressure of fluid

Î= unit tensor

= viscosity/stress tensor

F= external force per unit mass and volume

Q= heat flow

= sources and sinks

A_{j}= ambipolar diffusion between ions and neutrals
where the index j ∈ { H,H^{+},He,He^{+},He^{+ +},i,n }. As discussed above for the index j of the ionized fluid, the density is the sum of all densities of ionized species, the total pressure P_{j} = ∑ kP_{k}, the total energy E_{j} = ∑ kE_{k}, with k ∈ {H^{+}, He^{+}, He^{+ +} }.
The force densities, stress tensor and the heat transport on the righthand side of Eq. (A.1) are usually neglected in modeling the largescale structure of the heliosphere, that is, . While external forces, such as solar gravitation, can be neglected, the stress tensor will play an important role in studying the details of the termination shock or heliopause structure, but to our knowledge this was not discussed so far. Especially the heat transport by electrons can be expected to be significant, because of the high thermal speed of these particles, and will be analyzed in future work. If the righthand side of Eq. (A.1) vanishes, the set of equations is called ideal MHD.
From Eq. (27) it is evident that the interstellar helium contributes about 40% to the total mass density, thus the total mass density ρ_{n} in the above neutral continuity equation is ρ_{n} = ρ_{H} + ρ_{He} ≈ 1.4ρ_{H}. This results in an increased ram pressure and momentum flow ρ_{n}v_{n}. Together with the total pressure P_{n} = P_{H} + P_{He} = κ(n_{H}T_{H} + n_{He}T_{He}) and the previously made assumption T_{H} = T_{He} and n_{He} = 0.1n_{H} yields P_{n} = 1.1P_{H}. These estimates show, that helium contributions are not negligible. A similar consideration holds for the governing equations of the charged particles.
If the helium inflow velocity differs in direction from that of hydrogen (Lallement et al. 2005), helium has to be treated as a separate fluid and an additional complete set of the Eulerequations must be solved. If one can assume that the flow velocities of the neutrals and charged fluids are the same for all neutral and ionized species, it is sufficient to solve the two governing equations and treat the other species as tracer particles to calculate their densities and thermal pressures.
Handling the neutrals with a kinetic set of equations (Izmodenov 2007; Heerikhuisen et al. 2008) requires a similar approach for the collision integrals (see Eqs. (39) and (40)) to obtain the balance terms for the (M)HD equations of charged particles, when including heavier ions.
Appendix B: “Collision” speeds
For the interaction of particles with different masses (nonresonant charge exchange processes), the approach by McNutt et al. (1998) can be applied. Nevertheless, the relative velocities for the momentum exchange differ from those for the energy exchange, in contrast to what was discussed in McNutt et al. (1998)
As described in Eqs. (57) to (60) in McNutt et al. (1998), the relative speeds for the crosssections for charge exchange differ for all three Euler equations, as well as the speeds needed for the charge exchange crosssection. The speeds are denoted as above , where j ∈ {c, m, e, P} for the continuity, momentum, and energy equations and j = P for the thermal pressure, respectively. The governing energy equation contains the ram pressure and the thermal pressure, which are both influenced. The balance equations only contain the thermal pressure, because changes in the ram pressure or bulk speed are calculated in the governing equations with the assumption that all species flow with the same speed. The indices i ∈ {cx, rel} are the speeds needed for the charge exchange crosssection and corresponding relative speeds. With the definitions from McNutt et al. (1998) we have to solve the following type of integrals: (B.1)The following recursion holds: (B.2)Thus we need only to know the four integrals (Gradstein & Ryshik 1981), Nr. 3.562.33562.6: These integrals need to be multiplied by the factors given in McNutt et al. (1998).
With these integrals it is easy to calculate the required speeds (for details see McNutt et al. 1998):
The approximations in Eqs. (B.3) to (B.8) fit nicely, except for small errors (see Fig. B.1). Note that the fit in Eq. (B.6) differs by a factor 0.5 from that of McNutt et al. (1998).
Fig. B.1 Relative errors of the fitted characteristic collision speeds, where are the approximations given in Eqs. (B.3)−(B.8). 

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With the help of the integrals it is easy to calculate the higherorder correction terms. However, this is not necessary for the p + H reaction, because the secondorder derivatives of the crosssections, as shown in Fig. B.1, are orders of magnitudes lower than the crosssection. Shown in Fig. B.2 are the functional dependencies given by Fite et al. (1962) and by Lindsay & Stebbings (2005), that is
(B.9)where v_{rel} is given in cm/s and the σ in cm^{2}.
With the help of the computer algebra system wxMaxima^{3} it is easy to calculate the second derivatives of these commonly used crosssections for the p + H reaction and the integrals for the secondorder terms of the Taylorexpansion for σ^{cx}. For the terms needed in the continuity equation, we have to compare with the secondorder terms , where we neglected common factors for simplicity. In our notation . With some algebra, we find that and thus finally (B.10)The function h(v) defined above is small for all v, so that we can assume that the higherorder terms in the Taylor expansion of σ^{cx} vanish. In Fig. B.2 the function is shown for the two crosssections.
Fig. B.2 Ratio h(v) (Eq. (B.10)) of the secondorder integrated Taylorexpansion to the zeroth order for the two Hp charge exchange crosssections discussed by Fite et al. (1962) and Lindsay & Stebbings (2005). The bump between the two downward spikes in the LindsayStebbings curve is negative, but to represent it in a logarithmic scale, its absolute value was taken. See text for restrictions of the fit functions. 

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It can be seen in Fig. B.2 that for the Fite et al. (1962) crosssection the secondorder terms are nearly a factor 10 lower than the zerothorder term for all speeds. For the Lindsay & Stebbings (2005) crosssections this holds only for speeds lower than 4 × 10^{7} cm/s = 400 km s^{1}. Around these speeds, that is, a commonly used solar wind speed, the secondorder corrections are on the same order than the zerothorder term.
Gains and losses from the original populations.
In the latter case, that is, if the higherorder terms cannot be neglected, in the analytic representation this will lead to clumsy formulas, which also need some computational time. Thus, it might be better to solve the collision integrals numerically.
Note, that for the hydrogenproton reactions the fit function discussed in Fite et al. (1962) has an upper boundary of 10 keV, which corresponds to a relative speed of ≈1400 km s^{1}. The range in which the data were fitted by Lindsay & Stebbings (2005) has an upper boundary of 300 keV, which corresponds to a speed lower than ≈7500 km s^{1}. The data presented in Fig. 2 were taken from the Redbooks^{4} and reach to 63 keV, corresponding to ≈3400 km s^{1}. Some of the helium reactions have their maximum crosssection at higher energies, as can be seen in Table C.1, and their upper limits in energy/amu are higher than shown in Fig. 2.
All the fits given for the data from the Redbooks or the Aladdin database are mainly based upon a fit with Chebyshev polynomials. These polynomial fits are only good in the range given by the corresponding upper and lower (energy) boundaries and cannot be extended beyond these. Because usually it cannot be guaranteed in a largescale model that the relative speeds are always in that range, a better fit function is needed, which can be extended beyond the boundaries, keeping in mind not to violate quantum mechanical requirements.
We here only discussed the simplest case, that is, the collision terms for the continuity equation. Of course this analysis must be performed not only for the remaining set of MHD equations, but has, especially, to be verified for all interactions.
Appendix C: Interaction terms
Gains from the new populations.
In the following we provide an overview of possible ionization reactions. In Table C.1, the first column gives the interaction term in the continuity equation, indicating the particle species: X^{n} with X∈ {H,He}, while n ∈ { 0,1,2 } gives the ionization state (usually the index 0 is omitted). Newly created ions are named as PUI_{Xn} and energetic atoms by ENA_{X}. The reaction rates have the indices {cx, ei, pi} for charge exchange, electron impact, and photoionization, respectively. The rates are also denoted by ν(i,j), where i describes different reactants, while j stands for different products of the same reaction i. The tuple (i,j) is given in the fourth column, where a minus sign stands for losses and a plus sign for gains. To derive the total gains and losses one has to sum over all { i,j }. In the fifth and sixth column the maximal crosssection and its corresponding relative speed is given, respectively. In the third column the first reactant is a particle from the solar wind, while the second reactant is from the interstellar medium. This distinction is necessary to ensure correct sorting.
Note that in the charge exchange rate ν^{cx} = ρ_{X}σ^{cx}v_{rel} the density of the first reactant is included and is indicated in the table by ν_{cx,X}.
Table C.1 contains the losses, Table C.2 the gains. In Table C.1 the approximate highest values for the crosssection are listed. They may vary by a factor of three and only indicate the correct order of magnitude. If a range is given for the corresponding relative velocity, the crosssection is a flat curve in that range.
All reactions that have a charged particle as the second reactant cannot flow in from the interstellar medium. Because the heliopause is a contact discontinuity that separates the solar wind and interstellar medium plasma, there is no flow of charged particles across the heliopause. Thus in Tables C.1 and C.2 the reactions labeled (3,1), (4,1), (5,1), (6,1), (8,1), (10,1), and (12,1) can be neglected.
The reactions labeled with an asterisk are sorted in pickup channels, even though they do not create new PUIs. For example, the reaction He^{++}+H→He^{+}+H^{+} produces a new pickup hydrogen, but the change from doubly to singly charged helium does not change its character, that is He^{+} has the same bulk speed as He^{2+}. Only the charge is changed, thus the new He^{+} does not
affect the dynamics (the H^{+} does). Nevertheless, these processes can have an effect on magnetic field turbulence (e.g. Shalchi et al. 2012). This aspect is interesting in the description of the diffusion tensor to model cosmic rays (Effenberger et al. 2012). The role of these types of processes for the turbulence will also be considered in future work.
From these tables the interaction terms for the governing equations can be determined. For the neutral equation it is just the sum of all interaction terms. More care must be taken for the ion governing equation, because the pickup terms can cancel some of the ion terms, for example, the reaction H^{+} + H → H + H^{+} looses an original fast solar wind proton, but gains a slow interstellar hydrogen atom, which does not change the total ion mass.
To describe the interaction terms for the momentum and energy equation, similar tables can now easily be constructed and the governing equations determined.
All Tables
All Figures
Fig. 1 Proton temperature distribution in the dynamic heliosphere (Scherer & Ferreira 2005). Above the solar pole the features of a highspeed stream can be identified. Because of the influence of the PUI_{SH+} the temperature inside the termination shock is a few 10^{5} K, corresponding to thermal energies of up to a few tens of eV. The temperature in the inner heliosheath is 10^{6} K, which was inferred by IBEX (Livadiotis et al. 2011). 

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In the text 
Fig. 2 Charge exchange crosssections as a function of energy per nucleon for protons (left panel), He^{+}ions, and αparticles (right panel) of the solar wind with interstellar helium and hydrogen. In the upper part of the two panels we show the crosssections, while the lower parts show the ratio to σ_{cx}(H^{+} + H → H + H^{+}). The black curve in the panels is the reaction H + H^{+} → H^{+} + H. As can be seen in the lower panel the reactions He^{+} + He, He^{2+} + He, and He^{2+} + He^{+} have similar crosssections as that of H + H^{+} and thus are important in modeling the dynamics of the largescale astrospheric structures. Note the different yaxis scales between different panels. 

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In the text 
Fig. 3 Rate coefficients β(v) = vσ(v) instead of the crosssections as in Fig. 2. We assumed that there is no difference in the relative speeds from the collision integrals and those to be used for the crosssections , i.e., . 

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In the text 
Fig. 4 Electron impact crosssection σ^{ei} in units of 10^{17} cm^{2} per particle, for the three reactions: H + e → H^{+} + 2e, He + e → He^{+} + 2e, and He + e → He^{2+} + 3e. 

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In the text 
Fig. 5 Ratios as defined in Eq. (36). The left panel shows the ratio for hydrogen while the right panel presents the ratio for singly ionized helium. Positive values indicate that the charge exchange process (H + H^{+} → H^{+} + H) dominates, while for negative values the electron impact is more relevant. Note the different scales in the color bars. 

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In the text 
Fig. 6 α parameter throughout the heliosphere. α is the ratio of the modulus of the relative bulk velocity to the thermal speed of the two species, see Eq. (41). 

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In the text 
Fig. 7 Characteristic collision speeds normalized to the thermal speed as a function of the parameter α (left panel) and the relative “error” , r ∈ { c,m,e }. 

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In the text 
Fig. B.1 Relative errors of the fitted characteristic collision speeds, where are the approximations given in Eqs. (B.3)−(B.8). 

Open with DEXTER  
In the text 
Fig. B.2 Ratio h(v) (Eq. (B.10)) of the secondorder integrated Taylorexpansion to the zeroth order for the two Hp charge exchange crosssections discussed by Fite et al. (1962) and Lindsay & Stebbings (2005). The bump between the two downward spikes in the LindsayStebbings curve is negative, but to represent it in a logarithmic scale, its absolute value was taken. See text for restrictions of the fit functions. 

Open with DEXTER  
In the text 