\kappa–Distributions in H ii regions

Resolving the electron temperature discrepancies in H ii Regions and Planetary Nebulae: –distributed electrons

David C. Nicholls11affiliation: Research School of Astronomy and Astrophysics, Australian National University, Cotter Rd., Weston ACT 2611, Australia , Michael A. Dopita11affiliation: Research School of Astronomy and Astrophysics, Australian National University, Cotter Rd., Weston ACT 2611, Australia 22affiliation: Astronomy Department, King Abdulaziz University, P.O. Box 80203, Jeddah, Saudi Arabia , & Ralph S. Sutherland11affiliation: Research School of Astronomy and Astrophysics, Australian National University, Cotter Rd., Weston ACT 2611, Australia david@mso.anu.edu.au

The measurement of electron temperatures and metallicities in H ii regions and Planetary Nebulae (PNe) has—for several decades—presented a problem: results obtained using different techniques disagree. What is worse, they disagree consistently. There have been numerous attempts to explain these discrepancies, but none has provided a satisfactory solution to the problem. In this paper, we explore the possibility that electrons in H ii regions and PNe depart from a M-B equilibrium energy distribution. We adopt a “–distribution” for the electron energies. Such distributions are widely found in solar system plasmas, where they can be directly measured. This simple assumption is able to explain the temperature and metallicity discrepancies in H ii regions and PNe arising from the different measurement techniques. We find that the energy distribution does not need to depart dramatically from an equilibrium distribution. From an examination of data from H ii regions and PNe it appears that is sufficient to encompass nearly all objects. We argue that the kappa-distribution offers an important new insight into the physics of gaseous nebulae, both in the Milky Way and elsewhere, and one that promises significantly more accurate estimates of temperature and metallicity in these regions.

Subject headings:
physical data and processes: acceleration of particles, atomic processes, plasmas, atomic data — ISM: H ii regions, planetary nebulae: general, abundances

1. Introduction

Over forty years ago, Vasyliunas (1968) measured the electron energy distributions in the Earth’s magnetosphere using the OGO1 and OGO3 satellites and found that there was a significant high energy (‘suprathermal’) excess, when compared to an equilibrium M-B (M-B) distribution. The best fit to this high energy tail was a power law. He introduced the “–distribution”—a generalized Lorentzian distribution—which provided a good description of the electron energy distribution over the full range of energies.

Since then, –distributions have been the subject of considerable interest in solar system physics. They have been found by direct measurement of electron energies by satellites and space probes in the outer heliosphere, the magnetospheres of all the gas-giant planets, Mercury and the moons Titan and Io, the Earth’s magnetosphere, plasma sheet and magneto-sheath and in the Solar Wind (see references in Pierrard & Lazar (2010)). Evidence is also emerging from IBEX observations that energetic neutral atoms in the interstellar medium, where it interacts with the helio-sheath, exhibit –distributions (Livadiotis et al., 2011). More than 5000 papers in many disciplines on the applications of –distributions had been published prior to 2011 (Livadiotis & McComas, 2011). In solar system plasmas, –distributions arise whenever the plasma is being continually pumped by an energy input of a non-thermal or supra-thermal nature, or by energy transport from elsewhere, so that the system cannot relax to a classical M-B distribution.

To date, despite the extensive adoption of –distributions in analysing solar system plasmas—where they are the rule rather than the exception—the possibility that electron energies are distributed in a non-thermal manner in the photoionized plasma of H ii regions, Planetary Nebulae (PNe), or in the photoionized regions around active galaxies, does not appear to have been considered. Indeed the assumption that the electrons are in M-B equilibrium dates back over 70 years; see for example, Hebb & Menzel (1940).

There are good reasons to question the basis on which temperatures and metallicities are measured in H ii regions and PNe: for example, there have been consistent discrepancies between direct electron temperature () estimates and those obtained using recombination lines. None of the earlier attempts to solve the problem are fully satisfactory—for example, the “” temperature fluctuation method, (Peimbert, 1967)—and some have been completely abandoned (Stasińska, 2004).

In this paper, we explore the implications of electron energies following a –distribution in these photoionized plasmas. We show that assuming a – electron energy distribution is a simple and elegant way to resolve many of the difficulties, and should lead to more consistent temperature measurements and metallicity estimates in H ii regions and PNe.

The paper is organised as follows. In Section (2) we provide the key definitions and formulae for the –distribution. In Section (3) we show that there is a sound basis for H ii regions and PNe having –distributed electrons. In Section (4) we examine the dependence of collisional excitation rates on excitation energy and the value of , and apply this to a detailed study of the particular case of the [O iii] line ratio, the most important ratio used in the determination of electron temperatures in photoionized plasmas. In Section (5) we summarize the temperature discrepancy problem that has bedevilled temperature and metallicity measurements in gaseous nebulae for decades. In Section (6) we examine the observational data from H ii regions and PNe to show how the assumption of a –distribution can explain the temperature discrepancies, and how the value of can be constrained by requiring that different methods of measuring the electron temperature yield the same answer. Appendix A presents additional evidence for the presence of magnetic fields in H ii regions which can give rise to hot-tailed electron energy distributions. In Appendix B, we examine the relationship between the “” method for measuring the effect of temperature fluctuations and the –distribution.

2. The –distribution

2.1. Properties and Definitions

Initially, –distributions were used as an empirical fit to directly measured electron energies in solar system plasmas, and were criticized as lacking a theoretical basis. More recently, the distribution has been shown to arise from entropic considerations. See, for example, Tsallis et al. (1995); Treumann (1999); Leubner (2002), and the comprehensive analysis by Livadiotis & McComas (2009). They explored the so-called –nonextensive entropy statistics in which the entropies of adjacent samples of plasma are not simply additive, and have shown that – energy distributions arise naturally in such plasmas. The requirement for this to occur is that there be long-range interactions between particles, in addition to the short-range Coulombic forces that give rise to M-B equilibration. Although there is ongoing debate over whether the Tsallis statistical mechanics is the best generalisation of Boltzmann-Gibbs statistics, it provides a sound physical basis for the overtly successful use of the –distribution in plasma physics.

There are a number of slightly differing expressions for the energy distributions that can arise from –nonextensive entropy, but the forms are generally similar. Here, we adopt the Vasyliunas form of the distribution as representative of the possible variants. This is referred to by Livadiotis & McComas (2009) as a –distribution of the “second kind”. The successful use of the –distributions to describe physical phenomena in many disciplines, and especially in solar system physics, provides ample justification for exploring their use in H ii regions and PNe.

The –velocity distribution can be expressed (after Vasyliunas, 1968) as:


where is the number of electrons with speeds between and . The velocity is related to , the most probable speed (i.e. the velocity value at the distribution peak) by:


and related to the “physical temperature” of the system, , as defined in Livadiotis & McComas (2009):


where is the electron mass and is the Boltzmann constant.

is a parameter that describes the extent to which the distribution departs from an equilibrium distribution. In the Vasyliunas form, . In the limit as , the velocity distribution reverts to the standard M-B form,


The physical temperature, , also referred to as the kinetic temperature, is a generalisation of the M-B equilibrium temperature, and is related to the energy density (system kinetic energy), , which for a monatomic gas is the internal energy of the system:


Figure 1 shows a family of – velocity distributions with a M-B distribution.

Figure 1.— – velocity distributions (log scale) for from 2 to 50, with Maxwell-Boltzmann distribution.

Expressed in energy terms, the –distribution becomes:


Again, the – energy distribution tends in the limit as to the M-B,


A family of normalized – energy distributions is shown in Figure 2, together with a M-B equilibrium distribution. Note that the peak of the M-B energy distribution occurs at whereas –distributions with the same internal energy peak at .

Figure 2.— – energy distributions (linear scale) for from 2 to 50, with Maxwell-Boltzmann distribution.

The same distributions are shown in Figure 3 but plotted on a log scale. The high energy power-law tail of the –distributions is clearly shown.

Figure 3.— – energy distributions (log scale) for from 2 to 50, with Maxwell-Boltzmann distribution.

Figures 1-3 illustrate the key characteristics of the –distribution: the peak of the distribution moves to lower energies; at intermediate energies there is a population deficit relative to the M-B distribution; and at higher energies the “hot tail” again provides a population excess over the M-B. The distribution behaves as a M-B distribution at a lower temperature, but with a significant high energy excess.

This can be seen in Figure 4, where a M-B distribution is peak-fitted to a =2 distribution. The peak-fitted “core” M-B distribution is in fact at a lower physical temperature than the –distribution to which it is fitted. The low energy “core” occurs because the equilibration timescale is a strong function of energy (), allowing the low-energy electrons to approach an equilibrium distribution. The relationship between the physical temperature of the –distribution, , and the equilibrium temperature of the “core” M-B, , as implied by equation 3, is:

Figure 4.— = 2 energy distribution with peak-fitted Maxwell-Boltzmann distribution core.

For physical processes that involve low energy electrons such as recombination line excitation, reactions “see” the cool M-B core distribution. In other words, any physical property sensitive to the region of the electron energy distribution around or below the distribution peak will interact with an effective M-B electron energy distribution at a lower temperature than the M-B distribution with the same total internal energy as the –distribution.

Conversely, in processes that depend on the high energy end of the distribution, such as collisional line excitation, the –distribution behaves like a M-B distribution at a higher temperature than one with the same total internal energy. In other words, physical properties sensitive to energies above the peak will behave as if they were interacting with a hotter distribution. The –distribution thus exhibits a “split personality”, depending on the physical process involved. We show below that this behaviour resolves many of the discrepancies between different nebular temperature measurement techniques.

3. What might give rise to –distributions in H ii regions?

Given the plausiblity of –distributions in H ii regions, can we find mechanisms capable of maintaining the hot tails? The answer is, clearly, yes. A high-energy tail in the energy distribution will occur whenever the population of energetic electrons is being pumped in a timescale as short, or of the same order, as the energy re-distribution timescale of the electron population. Such effects may be long-range in nature, such as magnetic reconnection followed by the migration of high-energy electrons along field lines, and by the development of inertial Alfvén waves. We explore additional evidence for the existence of magnetic fields in galactic H ii regions in Appendix A.

Pumping of high energy tails can also be more local in character such as local shocks (driven either by the collision of bulk flows or by supersonic turbulence), or, most simply, by the injection of high-energy electrons through the photoionization process itself. Normal photoionization produces supra-thermal electrons on a timescale similar to the recombination timescale.

Energetic electrons can also be generated by the photoionization of dust (Dopita & Sutherland, 2000). Alternatively, X-ray ionization can produce highly energetic ( keV) inner-shell (Auger process) electrons (e.g. Shull & Van Steenberg (1985); Aldrovandi & Gruenwald (1985); Petrini & Da Silva (1997), and references therein). Processes based on photoionization should become more effective where the source of the ionizing photons has a “hard” photon spectrum. Thus, the likelihood of the ionized plasma having a – electron energy distribution would be high in the case of either photoionization by an Active Galactic Nucleus (AGN), or the case of PNe, in which the effective temperature of the exciting star could range up to °K.

Thus, we have no shortage of possible energy injection mechanisms. The main consideration is whether feeding the energetic population can occur on a timescale which is short compared with the collisional re-distribution timescale, . Because this timescale increases very rapidly with energy, , we would expect there to be a threshold energy above which any non-thermal electrons have a long residence timescale. These can then feed continually down towards lower energies, maintaining a – electron energy distribution. It seems more likely therefore that all photoionized plasmas will show departures from a M-B distribution to some degree. The key question is, is this departure important, and does it produce observable effects in the plasma diagnostics on which we have relied upon hitherto? Again, yes, as we show in Section (4) below.

3.1. Are –distributions stable in their own right?

In addition to the energy injection mechanisms capable of maintaining the excitation of suprathermal distributions, several authors (Livadiotis & McComas (2011) and references therein; Shizgal (2007); Treumann (2001)) have investigated the possibility that the –distribution may remain stable against thermalization longer than conventional thermalization considerations would suggest (e.g. Spitzer (1962)). In particular, distributions with appear to have the capacity, through increasing entropy, of moving to values of lower (Livadiotis & McComas, 2011) i.e. away from (M-B) equilibrium. While the physical application of this aspect of –distributions remains to be explored fully, it suggests that where -nonextensive entropy conditions operate, the suprathermal energy distributions produced exist in “stationary states” where the behaviour is, at least in the short term, time-invariant (Livadiotis & McComas, 2010a). These states may have longer lifetimes than expected classically. This is fully consistent with the numerous observations that in solar system plasmas, – electron and proton energy distributions are the norm. It seems reasonable to expect that such conditions will also be present in H ii regions and PNe.

4. The effect of –distributions on collisional excitation in H ii regions

4.1. Collisional excitation rates

Consider the collisional excitation of an atomic species from energy level to energy level . The rate of collisional population of the upper energy level per unit volume is given in terms of the collision cross-section, , by:


We separate out the strong energy dependence of the collision cross-section , by expressing it in terms of the collision strength, and the energy, :


where is the Planck Constant, is the electron mass, and is the statistical weight of the lower energy state.

The collisional population rate now becomes:


where the appropriate form of the distribution is substituted, giving the well-known collisional population rate formula for a M-B distribution:


For a –distribution, the corresponding rate is:


Adopting the approximation that is independent of energy, the integral parts of the above equations (after taking a factor outside the integrals) reduce to:




respectively. Note that in the limit as , equation transforms into equation , as it should.

It is useful to compare the relative rates of population to an upper state for M-B and –distributions. Taking equations (12) and (13) and assuming constant s, we can derive an analytical equation that expresses the ratio of the population rates:


Figure 5 shows the effect of equation (16) in the enhancement of the collisional excitation rate for : 2 100 compared to the M-B rate for an electron distribution having the same internal energy. Very similar curves were obtained by Owoki & Scudder (1983) in the context of collisional ionization rates in the solar corona. Data for Figure 5 for an extended energy ratio range are given in Table 1.

Figure 5.— The collisional excitation enhancement ratio over a Maxwell-Boltzmann distribution for different –distributions plotted as a function of the excitation threshold energy (expressed as an equivalent temperature) over the kinetic temperature , equation (16). For the –distributions very large enhancements in the collisional excitation rate are possible for high values of . (Extended data in Table 1)

The implication is that collisionally excited UV lines—with higher excitation energies— should show strong enhancements compared to standard theory, while lines in the optical and IR would be relatively little changed, unless the region has a low kinetic temperature. Collisionally excited lines of non-ionized species such as [O i] or [N i] will be differently affected, since the collision strength has a strong energy dependence, increasing above threshold. For these ions the degree of enhancement in the collisional excitation rate compared with the M-B case will be much larger than shown in Figure 6. This could explain a long-standing problem in H ii region models, which tend to systematically underestimate the strength of these lines, compared to observations. New data on the collision strengths of OI and NI, in the context of the –distribution, have implications for using the lines of these neutral species as low-temperature diagnostics in partially ionized regions. We will explore this in a future paper.

4.2. Effect of on [O iii] electron temperatures

The direct method of estimating electron temperature in H ii regions relies on measuring the flux ratios of different excited states from the same atomic species. Most often used are collisional excitation to the and states of [O iii] , which give rise to the forbidden nebular lines at 5007Å and 4959Å, and the “auroral” line at 4363Å. Lines of [O ii], [N ii], [S ii] , [Ne iii], [Ar iii] and [S iii] are also used, when the relevant lines can be observed. The threshold excitation energies for the upper states in these species are different, so the degree of enhancement in a –distribution of electrons will differ from one ion to the next. This fact provides a possible resolution of the discrepancies encountered when measuring temperatures using these different atomic species.

Figure 6.— The lower energy levels and forbidden transitions for the O iii ion.

As a specific and important example, we consider here the excitation of the O iii ion. For reference, the configuration of the lower states which give rise to the forbidden lines used in temperature determinations is illustrated in Figure 6. The threshold excitation temperatures of the excited states are 29,130°K () and 62,094°K (). For a –distribution at temperature °K from Figure 5 the excitation rate to the lower state will be little changed, while the collision excitation rate to the upper state will be strongly enhanced, leading to an overestimate of the true electron temperature computed by formulae such as given by Osterbrock & Ferland (2005). We now proceed to quantify this remark.

For an equilibrium electron energy distribution, the relative population rates can be calculated using equation (11) for the upper and lower excited states. If one assumes for simplicity that the values are energy-independent, the ratio of the two population rates in the M-B case is simply:


In a more accurate analysis, the collision strength is integrated over the energy range to as per equation (11), to give the effective (temperature averaged) collision strength, .

Allowing for other transitions from the state via the branching ratio and correcting for the energies of the two lower state transition photons, the ratio of the fluxes of the (5007 + 4959) to 4363 give a direct measure of the population rates to the two excited states, and therefore of the electron temperature of the energy distribution. Following Osterbrock & Ferland (2005) we can derive a simple equation for the electron temperature, , in terms of the line fluxes, for low density plasmas:


This formula is, of course, an approximation, as it assumes the values and (and therefore of and ) do not depend on temperature. A more accurate iterative formula was given by Izotov et al. (2006). Values of the effective collision strength assuming constant differ slightly from those computed numerically, taking into account the detailed collisional cross section resonances. To identify what effect this would have on determining the electron temperature, we compared electron temperatures derived using constant , the Izotov iterated formula, and the values computed using the detailed collision strengths from Lennon & Burke (1994) and Aggarwal (1993).

Figure 7 shows the relationship between the flux ratio and the electron temperature, using the Osterbrock equation, the Izotov iteration and computed numerically from the Lennon & Burke (1994) and Aggarwal (1993) data. (The values in most common use for are those published by Lennon & Burke (1994), available online via TIPbase (Hummer et al., 1993); or the data from Aggarwal & Keenan (1999), but the latter are only available in abbreviated tabular form.)

Figure 7.— [O iii] line flux ratio vs. temperature for M-B distributed electrons computed from different methods and by different authors

For M-B energy distributions, the use of a constant gives a slightly higher than is obtained using the Lennon & Burke (1994) data, and higher still compared to the data from Aggarwal (1993). At an equilibrium temperature of 20,000°K, the difference between the Izotov value and the L&B data is 130°K and for the Aggarwal data, 285°K.

These differences are of minor import. An altogether different result occurs when we use a –distribution instead of the M-B to calculate the line ratio vs graph. The results are shown in Figure 8. For =100, 50, 20, and 10 the kinetic temperature differences from the M-B equilibrium value at =20,000°K are 180°K, 385°K, 980°K and 2,100 °K. Data for the extended temperature range 5,000 to 20,000°K are given in Table 2. The data are calculated using the detailed collision strengths (from Lennon & Burke (1994)), but assuming constant s makes only a small difference for 6.

As can be seen in Figures 2 and 3, these values of are visually relatively minor deviations from the M-B distribution, but they have a considerable effect. This implies that even –distributions which diverge slightly from equilibrium can have a significant effect on electron temperatures measured using the [O iii] lines. The same result is true for other collisionally excited lines, [O ii], [S ii] and [N ii], but to differing extents, owing to the different collisional excitation energy thresholds for the upper and lower states. The differences in apparent electron temperatures calculated using different collisionally excited species allow us to obtain an estimate of the effective value of for remote H ii regions, as we show in Section (6).

Figure 8.— [O iii] line flux ratio vs kinetic temperature for the range , compared to the computed Lennon & Burke (1994) equilibrium data, labeled Maxwell in the figure. (Extended data in Table 2)

5. The abundance discrepancy problem

Discrepancies between measurements made using various temperature-sensitive ion line ratios have been observed in both H ii regions and PNe. Recombination temperatures (derived from the Balmer and Paschen jumps) are systematically lower than temperatures derived from collisionally excited line ratios. Systematic differences in temperature are also observed between collisionally excited line ratios of different ionic species (García-Rojas & Esteban, 2007; Izotov et al., 2006). This results in systematically different chemical abundances derived by optical recombination lines (ORLs) and collisionally excited lines (CELs), a problem dating back to Wyse (1942), and first discussed in detail by Torres-Peimbert & Peimbert (1977). There are also systematic differences between abundances determined using either direct measurements of ionic temperatures, correcting observed ionic abundances for unseen ionization stages (the method) or using the intensities of strong emission lines relative to the Hydrogen recombination lines (the strong line method). Collectively these are known as the abundance discrepancy problem (García-Rojas et al., 2006; García-Rojas & Esteban, 2007).

The confusion surrounding this issue has been well summarised by Stasińska (2004):

“It has been known for several decades that optical recombination lines [ORL] in PNe and H ii regions indicate higher abundances than collisionally excited lines [CEL]. … … The ORL abundances are higher than CEL abundances by factors of about 2 for most PNe, discrepancies over a factor 5 are found in about 5% of the PNe and can reach factors as large as 20. For a given nebula, the discrepancies for the individual elements C,N,O,Ne are found to be approximately of the same magnitude.
The explanations most often invoked are: i) temperature fluctuations, ii) incorrect atomic data, iii) fluorescent excitation, iv) upward bias in the measurement of weak line intensities, v) blending with other lines, vi) abundance inhomogeneities. None of them is completely satisfactory, some are now definitely abandoned.”

The possibility that the abundance discrepancy problem could be generated by the techniques used to measure abundances was recently investigated by López-Sánchez et al. (2012) using a grid of theoretical models to eliminate any systematics of observational errors. Although systematic errors were found in a number of empirical strong line techniques, the classical electron temperature + ionization correction factor technique works surprisingly well. Clearly the technique itself is not at fault.

Perhaps the most successful attempt to account for the abundance discrepancy problem has been to postulate the existence of small-scale temperature fluctuations as first proposed by Peimbert & Costero (1969), known as the “” method, and applied widely since; see e.g. Peimbert (2003) and references therein. To some extent electron temperature fluctuations (if real) act in a similar way to a –distributed electron population, in that both weight CELs towards higher temperature. However, we are missing an obvious physical explanation of why micro-fluctuations in temperature should exist and persist in the first place.

The approach has major advantages over the method: it is simple; it is consistent over many objects and atomic species; it arises directly from Tsallis q-nonextensive statistics; the physics of ionized plasmas in H ii regions and PNe provides several mechanisms capable of generating the suprathermal distribution tails; it has been shown to describe accurately numerous directly measured electron energy distributions in the solar system; and it explains behaviour over an energy range of at least 3 orders of magnitude, from low energy recombination line electrons to the high ionization energies in the solar corona. The relationship between the approach and the –distribution is explored further in Appendix B.

6. The Determination of

6.1. H ii regions

As noted earlier (equation 8), a –distribution with kinetic temperature can be characterised at low electron energies below the peak of the distribution by a “core” Boltzmann distribution with an effective temperature . Since is systematically lower than , and as it is the energy distribution of these low-energy electrons that determines the recombination temperature (), it is clear that in a –distribution the recombination rate is systematically enhanced. These same low-energy electrons also determine the size of the Balmer and Paschen discontinuities of Hydrogen, so that the measured Balmer and Paschen break temperatures will reflect , rather than .

At the same time, lines with excitation temperatures comparable to may be either mildly enhanced or suppressed in a –distribution, but lines with excitation temperatures well above are strongly enhanced by the power-law tail of high energy electrons present in the –distribution. This has the effect of enhancing the apparent electron temperature inferred using well-known temperature-sensitive line ratios such as [O iii] 4363Å/5007,4959Å, [S ii] 4069,76Å/6717,31Å, [N ii] 5755Å/6548,84Å or [O ii] 7318,24Å/3726,29Å. The degree of enhancement of the inferred temperature, compared to , is strongly dependent on , the excitation temperature of the upper levels involved in these transitions. Those ions in which is much greater than will have their inferred collisional excitation temperature, , very strongly enhanced over , while those for which is comparable to will show little change ().

These properties of the –distribution can be used as the basis for the determination of from spectrophotometric observations of both H ii regions and Planetary Nebulae.

We can test the –distribution hypothesis using the excellent echelle spectrophotometry which has been gathered by a number of authors in recent years. For Galactic H ii regions we have data in M 42 (Esteban et al., 2004), NGC 3576 (García-Rojas et al., 2004), S311 (García-Rojas et al., 2005), M20 & NGC 3603 (García-Rojas et al., 2006), M 8 & M 17 (García-Rojas & Esteban, 2007). For the extragalactic H ii regions we have data for 30 Dor (Peimbert, 2003), NGC5253 (López-Sanchez et al., 2012), NGC 595, NGC 604, VS 24, VS 44, NGC 2365 and K 932 (Esteban et al., 2009).

One of the strongest tests of the validity of the –distribution is the comparison of the [O ii] 7318,24Å/3726,29Å and [S ii] 4069,76Å/6717,31Å temperatures. These ions have very similar ionization potentials and are therefore distributed in a very similar way in the nebula. The photoionization models used by (López-Sánchez et al., 2012) have line emission weighted temperatures in the O ii and S ii zones which differ from each other by less than 400°K over the abundance range times solar. However the excitation temperatures of the lines are quite different. For the [S ii] 4069,76Å lines, °K, and for the [S ii] 6717,31Å °K. In the case of [O ii] 7318,24Å, °K while for the 3726,29Å lines, °K. Thus the [O ii] lines are much more sensitive to the high-energy tail of the –distribution than are the [S ii] lines. On this basis, one would expect higher temperatures to be derived from the [O II] line ratios than from the [S II] line ratios, in the presence of a –distribution.

Figure 9.— Measured temperatures in H ii regions compared with what would be expected if the electrons have a –distribution. Panel (a) compares the inferred excitation temperatures of the [O ii] and [S ii] ions, panel (b) the average of the [O ii] and [N ii] ions with the [S ii] ion. Panels (c) and (d) compare the recombination temperatures given by the mean of the Balmer and the Paschen break temperatures with the mean excitation temperature given by the average of the [O ii] and [N ii] line ratios, panel (c), and that of the [O iii] line ratio, panel (d). Most H ii regions appear to have .

We have computed for the observed data the effect that a –distribution has on the inferred collisional excitation temperature, , of these ions. This is shown in Figure 9 (a). The observations suggest that the [O II] temperatures are indeed higher than the [S II] temperatures, and that this difference can be accounted for in most of the H ii regions by .

As an alterative approach, we show on Figure 9 (b) the average of the inferred collisional excitation temperatures for the [O ii] and [N ii] ions compared with that of the [S ii] ion. For the [O ii] and [N ii] ions the sensitivity to is not as great as for the [O ii] lines alone, but the errors in the temperature determination produced by assumptions about the dust extinction curve are reduced. Again, the [S II] temperatures are lower. The inferred range of is somewhat wider, but most H ii regions are still consistent with .

Because the recombination temperature, , is appreciably lower than the kinetic temperature , which is itself lower than the excitation temperature for collisionally excited line ratios, , a comparison of recombination temperatures and inferred line temperatures is strongly sensitive to the choice of . The recombination temperatures, , should be significantly lower than the collisionally excited line temperatures, , in the presence of a –distribution. Again, this is clearly shown in the analysis of the observed H ii region spectra.

In Figures 9 (c) and (d) we show this comparison for the H ii regions, using the excitation temperature given by the average of the [O ii] and [N ii] line ratios and by the [O iii] line ratio, respectively. How well these determine depends on which of the ionic species is the dominant ionization stage in the nebula. For cooler exciting stars, [O ii] and [N ii] line ratios are the better ones to use, but when the central star(s) is hot enough to ionize helium to He ii in the bulk of the nebula, then the [O iii] line ratio is the better one to use. From Figure 9 (c) and (d) it would appear that , or even higher. Because the upper state of [OIII] has the highest excitation temperature, it is the most sensitive of all the ions to the high energy electrons, and therefore lower values of have greater effects.

6.2. Planetary Nebulae

High quality spectrophotometry also exists for many PNe, although published values of electron temperatures for many ions is rather sparse. However, rather complete data exist for temperatures determined from the Balmer discontinuity and from the [O iii] line ratio. The direct comparison of these should be a fairly reliable means of estimating , since the O iii ion is most often the dominant ionization stage in PNe.

Figure 10.— As figure 9, panel (d), but for planetary nebulae.

We have taken data from Tsamis et al. (2003); Liu et al. (2004); Zhang (2004); Wesson, Liu & Barlow (2005); Wang & Liu (2007) and Fang & Liu (2011). These data are plotted in Figure 10, along with the expectation for and 20. The points with error bars are from Zhang (2004). Again the results are consistent with in most cases, i.e. a mild departure from an equilibrium electron energy distribution. A few points lie above the line of equality of temperatures shown by the dotted line, corresponding to . However, many of these are consistent with no departure from a M-B distribution, within the observational errors. Of course, it is likely that local temperature and density fluctuations in the PNe contribute to the measured results, and it is not obvious what the contributions are from the various effects.

There are two apparent apparent trends in Figure 10: both cooler objects and objects with high [OIII] electron temperatures tend to show greater deviations from equilibrium (smaller inferred ). For high electron temperature objects, the energetic stellar winds from the hot central star are likely to lead to significant suprathermal heating of the ionized plasma, leading to lower values of . Indeed, some of the points identified by name (NGC 2440 and NGC 6302) are famous Peimbert Type I PNe, known to contain the most luminous and massive central stars. Among the rest, IC 4997 is a young PNe which also contains a Wolf-Rayet type central star, subject to rapid mass-loss.

The coolest objects tend to be more metal rich, and/or of lower excitation class. As a result, the excitation is dominated by the high energy tail of the energy distribution, as illustrated in Figure 5: effects for [OIII] become more apparent. These and other characteristics of the –distribution will be the subject of detailed modelling in future papers.

The results for both PNe and H ii regions are consistent with mild departures from equilibrium (). It is interesting to note that in the analysis of the observed spectra, extreme values of are not required. The implied departures from a M-B distribution are quite small, but their effect on the nebular diagnostics is quite gross, with serious implications for the chemical abundance determinations in both classes of object. Large departures from the M-B distribution in either PNe or H ii regions (lower values of ) would in any case not be expected, since at the peak of the energy distribution the mean collision time between electrons is short.

7. Conclusion

In this paper we have explored the implications for temperature and metallicity measurement in H ii regions and PNe of assuming a non-equilibrium – electron energy distribution. We have shown that –distributions provide apparent electron temperatures measured from forbidden line ratios which are systematically higher than the kinetic temperature . Assuming –distributed electron energies appears to resolve the long standing discrepancies in temperatures measured using the collisional excitation lines of different atomic species, and those calculated using the bound-free recombination continuum. Using high quality published spectra, we have shown that for objects where the spectra of more than one appropriate atomic species is identifiable, it is possible to estimate a value for the effective value of . 20 is a good fit to many of the measurements. This value does not require a substantial redistribution of the population to be achieved, meaning that any of several means of generating high energy electrons should be capable of sustaining the non-equilibrium distribution.

The –distribution offers an important new insight into the physics of gaseous nebulae, both in the Galaxy and elsewhere. It is implausible that thermal equilibrium applies throughout in H ii regions and PNe, and the fact that the –distribution is able to explain long standing discrepancies is a strong indication that non-equilibrium is a valid assumption. It should enable more accurate estimates of temperature and metallicity in these regions. A detailed investigation into the implications for metallicity measurements will be provided in a future paper.

The authors would like to thank the anonymous referee for helpful suggestions on the document structure. M. Dopita acknowledges the support of the Australian Research Council (ARC) through Discovery project DP0984657.

Appendix A A. Evidence for magnetic fields in Milky Way H ii regions

In order for magnetic energy to be an important source of non-thermal electrons, we require , the ratio of the thermal to magnetic energy, to be less than unity. Direct measurements of have been made for H ii regions using Faraday rotation observations (Harvey-Smith et. al, 2011; Rodríguez et al., 2012). These reveal values of . However, these measurements do not reveal the full strength of the magnetic field if there is turbulence, they indicate only the size of the organised field. They should therefore be taken as imposing a lower bound on the true magnetic field. However, recent evidence on the warm ionized medium (Gaensler et al., 2011) suggests that magnetic turbulence dominates at small scales. Finally, it is generally believed that the magnetic turbulence in the H i phase leads to equipartition (). Let us take this as a working hypothesis and ask what happens across an ionization front in an H ii region.

Let the H i region be characterized by a density , temperature , pressure , magnetic field and sound speed . The Alfven velocity in the gas is . In the H i region ahead of the ionization front, if we assume that the gas is turbulently supported, , i.e. , on average. We can resolve the magnetic field into components parallel to the gas flow, and perpendicular to the gas flow (in the plane of the ionization front), . These components will fluctuate on the scale of the pressure-supported turbulent cells in the H i region, so they relate to the mean field only in a stochastic fashion.

Now consider what happens on the other side of the ionization front, where the sound speed is , the outflow Mach number is and the hydrodynamic variables are and . The ratio of the densities is obtained by equating the pre-ionization pressure to the post-ionization pressure, accounting for the recoil momentum of the ionized plasma;


The component of the magnetic field perpendicular to the flow direction is stretched (reduced) in the post-ionization zone by the ratio , and the local gas pressure is decreased in the ratio . Therefore:


Thus, all magnetic pressure support is effectively lost in this plane. However, parallel to the flow, the post-shock magnetic field is unchanged by the ionization, and therefore


Thus, the magnetic pressure dominates the thermal pressure in this direction. The turbulent origin of the magnetic field in the molecular cloud ensures that is rapidly fluctuating both in magnitude and direction, which will naturally assist magnetic reconnection and Inertial Alfvén Wave formation.

This magnetic field, highly aligned to the flow direction and showing strong fluctuations on the small scale provides a natural explanation for the filamentary structure of the ionized plasma seen very clearly in the Carina and M17 H ii regions observed by the Advanced Camera for Surveys (ACS) on the Hubble Space Telescope (HST) (see Figure 11, below).

In the case of Carina, the ionized filaments are seen as bright “hairs” originating at the ionization front. These bright regions correspond to the regions of low magnetic field, given that the gas flow from the ionization front has to be force free in the plane of the ionization front. In the case of M17, we are seeing un-ionized regions of low magnetic field and high dust optical depth “combed out” by the expanding ionized plasma. These filaments are only a few AU in diameter, and have an aspect ratio of up to . The implied atomic densities are of order atoms cm.

Note added in proof Our attention has been drawn to simulations of the magnetohydrodynamics of H ii regions by Henney et al. (2009) and Arthur et al. (2011), in which they show that, in their models, , the ratio of thermal to magnetic energy, is usually greater than unity, and that the observed filamentary structures (Figure 11) arise naturally in the simulations. The fact that these features appear to be magnetohydrodynamic in origin is evidence for the widespread presence of magnetic fields in H ii regions.

Figure 11.— Portions of HST images of the Carina nebula (left) and M17 (right) taken with the ACS. These images have been processed by an unsharp mask to bring up the microstructure. Both images display magnetically-dominated microstructures aligned with the outflow direction. The scales of these microfilaments is of order of the size of the solar system.

Appendix B B. The –distribution and the temperature fluctuation (“”) method

As early as 1967, Peimbert proposed that abundance discrepancies might be explained by spatial temperature variations within an H ii region (Peimbert, 1967). The approach is characterized by a parameter, , the mean square fractional temperature fluctuation (assumed to have a Gaussian distribution in space). While it is certain that there are spatial variations in temperature, those caused naturally by the radial temperature variation in the H ii region are usually insufficient to explain observations, and the cause of the larger values of implied by the observations remains unknown. However, the approach has been widely used, with mixed success (e.g. Peña-Guerrero et al. (2012); García-Rojas & Esteban (2007); Esteban (2002); Kingdon & Ferland (1995)). Detailed discussions of the technique are given in Stasińska (2004) and Kingdon & Ferland (1995).

The parameter is estimated by solving equations involving the collisionally excited line temperature(s) and the recombination line temperature (Kingdon & Ferland, 1995). But as Kingdon & Ferland (1995) also argued, “while temperature fluctuations may result in non-negligible abundance corrections in some objects, they are insufficient to resolve the abundance discrepancy”.

There is, however, a connection between the method for resolving abundance discrepancies and the –distribution. Livadiotis et al. (2011) noted that “–distributions can be derived from the superposition of Maxwellian distributions, by considering a non-fixed temperature that is characterised by a certain (continuous or discrete) density distribution of temperatures”. Thus:


where can, in theory, be determined from the expressions in equations 6 and 7. The necessity to include Maxwellian distributions in the series with extreme temperatures to provide the suprathermal tail at high energies, is, of course, non-physical, and the series needs to be truncated. Nonetheless, expressed this way, the –distribution can be seen as a generalization of the method.


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1.596E+00 1.228E+00 1.142E+00 1.081E+00 1.043E+00 1.020E+00 1.008E+00 1.004E+00
0.1 1.225E+00 1.119E+00 1.079E+00 1.047E+00 1.026E+00 1.012E+00 1.005E+00 1.002E+00
0.2 9.944E-01 1.031E+00 1.025E+00 1.017E+00 1.010E+00 1.005E+00 1.002E+00 1.001E+00
0.3 8.414E-01 9.596E-01 9.795E-01 9.905E-01 9.956E-01 9.982E-01 9.994E-01 9.997E-01
0.4 7.348E-01 9.017E-01 9.408E-01 9.672E-01 9.828E-01 9.921E-01 9.970E-01 9.985E-01
0.5 6.577E-01 8.544E-01 9.079E-01 9.469E-01 9.713E-01 9.866E-01 9.949E-01 9.975E-01
0.6 6.008E-01 8.157E-01 8.800E-01 9.293E-01 9.612E-01 9.817E-01 9.929E-01 9.965E-01
0.7 5.579E-01 7.841E-01 8.566E-01 9.141E-01 9.523E-01 9.774E-01 9.912E-01 9.957E-01
0.8 5.254E-01 7.584E-01 8.370E-01 9.011E-01 9.446E-01 9.736E-01 9.897E-01 9.949E-01
0.9 5.006E-01 7.377E-01 8.209E-01 8.902E-01 9.380E-01 9.703E-01 9.884E-01 9.943E-01
1.0 4.820E-01 7.213E-01 8.080E-01 8.813E-01 9.326E-01 9.676E-01 9.873E-01 9.937E-01
1.1 4.682E-01 7.086E-01 7.978E-01 8.742E-01 9.282E-01 9.654E-01 9.864E-01 9.933E-01
1.2 4.583E-01 6.993E-01 7.902E-01 8.688E-01 9.248E-01 9.636E-01 9.857E-01 9.929E-01
1.3 4.518E-01 6.930E-01 7.849E-01 8.650E-01 9.225E-01 9.624E-01 9.852E-01 9.927E-01
1.4 4.481E-01 6.894E-01 7.818E-01 8.628E-01 9.211E-01 9.617E-01 9.849E-01 9.925E-01
1.5 4.470E-01 6.882E-01 7.808E-01 8.620E-01 9.206E-01 9.614E-01 9.848E-01 9.925E-01
1.6 4.481E-01 6.893E-01 7.818E-01 8.628E-01 9.211E-01 9.617E-01 9.849E-01 9.925E-01
1.7 4.512E-01 6.926E-01 7.846E-01 8.649E-01 9.224E-01 9.624E-01 9.852E-01 9.927E-01
1.8 4.562E-01 6.979E-01 7.893E-01 8.683E-01 9.247E-01 9.636E-01 9.857E-01 9.929E-01
1.9 4.631E-01 7.053E-01 7.956E-01 8.731E-01 9.278E-01 9.652E-01 9.864E-01 9.933E-01
2.0 4.716E-01 7.145E-01 8.037E-01 8.792E-01 9.318E-01 9.674E-01 9.873E-01 9.937E-01
2.1 4.819E-01 7.257E-01 8.135E-01 8.866E-01 9.367E-01 9.700E-01 9.884E-01 9.942E-01
2.2 4.939E-01 7.387E-01 8.249E-01 8.953E-01 9.424E-01 9.730E-01 9.896E-01 9.949E-01
2.3 5.075E-01 7.536E-01 8.381E-01 9.054E-01 9.490E-01 9.765E-01 9.911E-01 9.956E-01
2.4 5.229E-01 7.704E-01 8.529E-01 9.167E-01 9.565E-01 9.805E-01 9.927E-01 9.965E-01
2.5 5.400E-01 7.892E-01 8.694E-01 9.293E-01 9.648E-01 9.850E-01 9.946E-01 9.974E-01
2.6 5.589E-01 8.099E-01 8.877E-01 9.432E-01 9.740E-01 9.899E-01 9.966E-01 9.984E-01
2.7 5.797E-01 8.327E-01 9.077E-01 9.585E-01 9.841E-01 9.953E-01 9.989E-01 9.996E-01
2.8 6.024E-01 8.575E-01 9.296E-01 9.752E-01 9.951E-01 1.001E+00 1.001E+00 1.001E+00
2.9 6.272E-01 8.845E-01 9.533E-01 9.932E-01 1.007E+00 1.008E+00 1.004E+00 1.002E+00
3.0 6.541E-01 9.138E-01 9.790E-01 1.013E+00 1.020E+00 1.014E+00 1.007E+00 1.004E+00
3.1 6.833E-01 9.455E-01 1.007E+00 1.034E+00 1.034E+00 1.022E+00 1.010E+00 1.005E+00
3.2 7.149E-01 9.796E-01 1.037E+00 1.056E+00 1.048E+00 1.030E+00 1.013E+00 1.007E+00
3.3 7.491E-01 1.016E+00 1.069E+00 1.080E+00 1.064E+00 1.038E+00 1.017E+00 1.009E+00
3.4 7.859E-01 1.056E+00 1.103E+00 1.106E+00 1.081E+00 1.047E+00 1.020E+00 1.010E+00
3.5 8.257E-01 1.098E+00 1.140E+00 1.134E+00 1.099E+00 1.056E+00 1.024E+00 1.012E+00
3.6 8.686E-01 1.144E+00 1.179E+00 1.163E+00 1.118E+00 1.066E+00 1.028E+00 1.014E+00
3.7 9.147E-01 1.193E+00 1.221E+00 1.194E+00 1.137E+00 1.076E+00 1.032E+00 1.016E+00
3.8 9.645E-01 1.245E+00 1.266E+00 1.227E+00 1.159E+00 1.087E+00 1.037E+00 1.019E+00
3.9 1.018E+00 1.301E+00 1.313E+00 1.262E+00 1.181E+00 1.099E+00 1.041E+00 1.021E+00
4.0 1.076E+00 1.361E+00 1.364E+00 1.299E+00 1.204E+00 1.111E+00 1.046E+00 1.023E+00
4.1 1.138E+00 1.425E+00 1.418E+00 1.339E+00 1.229E+00 1.123E+00 1.051E+00 1.026E+00
4.2 1.204E+00 1.493E+00 1.476E+00 1.380E+00 1.255E+00 1.137E+00 1.057E+00 1.029E+00
4.3 1.276E+00 1.566E+00 1.537E+00 1.424E+00 1.282E+00 1.150E+00 1.062E+00 1.031E+00
4.4 1.353E+00 1.644E+00 1.603E+00 1.471E+00 1.311E+00 1.165E+00 1.068E+00 1.034E+00
4.5 1.437E+00 1.728E+00 1.672E+00 1.520E+00 1.341E+00 1.180E+00 1.074E+00 1.037E+00
4.6 1.526E+00 1.817E+00 1.746E+00 1.572E+00 1.373E+00 1.196E+00 1.080E+00 1.040E+00
4.7 1.622E+00 1.913E+00 1.825E+00 1.627E+00 1.406E+00 1.212E+00 1.087E+00 1.044E+00
4.8 1.726E+00 2.015E+00 1.909E+00 1.685E+00 1.441E+00 1.229E+00 1.093E+00 1.047E+00
4.9 1.837E+00 2.124E+00 1.998E+00 1.747E+00 1.478E+00 1.247E+00 1.100E+00 1.050E+00
5.0 1.957E+00 2.241E+00 2.092E+00 1.812E+00 1.516E+00 1.265E+00 1.107E+00 1.054E+00
5.1 2.087E+00 2.365E+00 2.193E+00 1.881E+00 1.557E+00 1.285E+00 1.115E+00 1.057E+00
5.2 2.226E+00 2.499E+00 2.300E+00 1.953E+00 1.599E+00 1.305E+00 1.122E+00 1.061E+00
5.3 2.376E+00 2.642E+00 2.414E+00 2.030E+00 1.643E+00 1.325E+00 1.130E+00 1.065E+00
5.4 2.537E+00 2.794E+00 2.535E+00 2.110E+00 1.689E+00 1.347E+00 1.138E+00 1.069E+00
5.5 2.712E+00 2.958E+00 2.665E+00 2.196E+00 1.738E+00 1.369E+00 1.146E+00 1.073E+00
5.6 2.899E+00 3.133E+00 2.802E+00 2.286E+00 1.789E+00 1.393E+00 1.155E+00 1.077E+00
5.7 3.102E+00 3.320E+00 2.948E+00 2.382E+00 1.842E+00 1.417E+00 1.164E+00 1.081E+00
5.8 3.320E+00 3.520E+00 3.104E+00 2.482E+00 1.898E+00 1.442E+00 1.173E+00 1.086E+00
5.9 3.555E+00 3.735E+00 3.270E+00 2.589E+00 1.956E+00 1.468E+00 1.183E+00 1.090E+00
6.0 3.809E+00 3.965E+00 3.447E+00 2.702E+00 2.017E+00 1.495E+00 1.192E+00 1.095E+00
6.1 4.083E+00 4.211E+00 3.636E+00 2.821E+00 2.081E+00 1.523E+00 1.202E+00 1.100E+00
6.2 4.379E+00 4.475E+00 3.836E+00 2.947E+00 2.148E+00 1.552E+00 1.213E+00 1.105E+00
6.3 4.698E+00 4.758E+00 4.050E+00 3.080E+00 2.219E+00 1.582E+00 1.223E+00 1.110E+00
6.4 5.043E+00 5.061E+00 4.279E+00 3.221E+00 2.292E+00 1.613E+00 1.234E+00 1.115E+00
6.5 5.415E+00 5.386E+00 4.522E+00 3.369E+00 2.369E+00 1.645E+00 1.245E+00 1.120E+00
6.6 5.818E+00 5.735E+00 4.781E+00 3.527E+00 2.450E+00 1.679E+00 1.257E+00 1.126E+00
6.7 6.252E+00 6.109E+00 5.058E+00 3.694E+00 2.535E+00 1.713E+00 1.268E+00 1.131E+00
6.8 6.722E+00 6.510E+00 5.354E+00 3.870E+00 2.624E+00 1.749E+00 1.281E+00 1.137E+00
6.9 7.229E+00 6.941E+00 5.669E+00 4.057E+00 2.717E+00 1.787E+00 1.293E+00 1.143E+00
7.0 7.778E+00 7.403E+00 6.005E+00 4.255E+00 2.814E+00 1.825E+00 1.306E+00 1.148E+00
7.1 8.371E+00 7.900E+00 6.365E+00 4.464E+00 2.917E+00 1.865E+00 1.319E+00 1.154E+00
7.2 9.013E+00 8.433E+00 6.748E+00 4.686E+00 3.024E+00 1.907E+00 1.332E+00 1.161E+00
7.3 9.707E+00 9.006E+00 7.158E+00 4.921E+00 3.136E+00 1.950E+00 1.346E+00 1.167E+00
7.4 1.046E+01 9.621E+00 7.596E+00 5.170E+00 3.254E+00 1.995E+00 1.360E+00 1.173E+00
7.5 1.127E+01 1.028E+01 8.064E+00 5.434E+00 3.378E+00 2.041E+00 1.375E+00 1.180E+00
7.6 1.215E+01 1.099E+01 8.565E+00 5.714E+00 3.508E+00 2.089E+00 1.390E+00 1.187E+00
7.7 1.310E+01 1.176E+01 9.100E+00 6.010E+00 3.644E+00 2.139E+00 1.405E+00 1.194E+00
7.8 1.413E+01 1.258E+01 9.672E+00 6.325E+00 3.787E+00 2.190E+00 1.421E+00 1.201E+00
7.9 1.525E+01 1.346E+01 1.028E+01 6.659E+00 3.937E+00 2.244E+00 1.437E+00 1.208E+00
8.0 1.646E+01 1.441E+01 1.094E+01 7.013E+00 4.094E+00 2.299E+00 1.453E+00 1.215E+00
8.1 1.777E+01 1.544E+01 1.164E+01 7.389E+00 4.259E+00 2.356E+00 1.470E+00 1.223E+00
8.2 1.919E+01 1.654E+01 1.239E+01 7.787E+00 4.433E+00 2.416E+00 1.488E+00 1.230E+00
8.3 2.073E+01 1.773E+01 1.319E+01 8.211E+00 4.615E+00 2.478E+00 1.505E+00 1.238E+00
8.4 2.240E+01 1.900E+01 1.405E+01 8.660E+00 4.807E+00 2.542E+00 1.524E+00 1.246E+00
8.5 2.421E+01 2.038E+01 1.497E+01 9.138E+00 5.008E+00 2.608E+00 1.542E+00 1.254E+00
8.6 2.617E+01 2.186E+01 1.596E+01 9.645E+00 5.219E+00 2.677E+00 1.562E+00 1.263E+00
8.7 2.829E+01 2.345E+01 1.702E+01 1.018E+01 5.441E+00 2.748E+00 1.581E+00 1.271E+00
8.8 3.060E+01 2.517E+01 1.815E+01 1.076E+01 5.675E+00 2.822E+00 1.601E+00 1.280E+00
8.9 3.310E+01 2.702E+01 1.936E+01 1.137E+01 5.921E+00 2.899E+00 1.622E+00 1.288E+00
9.0 3.582E+01 2.902E+01 2.066E+01 1.201E+01 6.179E+00 2.979E+00 1.643E+00 1.297E+00
9.1 3.877E+01 3.117E+01 2.206E+01 1.270E+01 6.450E+00 3.062E+00 1.665E+00 1.307E+00
9.2 4.196E+01 3.350E+01 2.356E+01 1.343E+01 6.736E+00 3.148E+00 1.687E+00 1.316E+00
9.3 4.544E+01 3.600E+01 2.516E+01 1.421E+01 7.037E+00 3.237E+00 1.710E+00 1.325E+00
9.4 4.920E+01 3.870E+01 2.689E+01 1.504E+01 7.353E+00 3.329E+00 1.733E+00 1.335E+00
9.5 5.330E+01 4.161E+01 2.874E+01 1.592E+01 7.686E+00 3.426E+00 1.757E+00 1.345E+00
9.6 5.774E+01 4.476E+01 3.072E+01 1.686E+01 8.037E+00 3.525E+00 1.782E+00 1.355E+00
9.7 6.257E+01 4.815E+01 3.285E+01 1.786E+01 8.406E+00 3.629E+00 1.807E+00 1.365E+00
9.8 6.781E+01 5.182E+01 3.514E+01 1.893E+01 8.794E+00 3.736E+00 1.833E+00 1.376E+00
9.9 7.351E+01 5.577E+01 3.760E+01 2.006E+01 9.204E+00 3.848E+00 1.859E+00 1.386E+00
10.0 7.970E+01 6.004E+01 4.024E+01 2.127E+01 9.635E+00 3.964E+00 1.886E+00 1.397E+00
10.1 8.643E+01 6.466E+01 4.308E+01 2.256E+01 1.009E+01 4.085E+00 1.914E+00 1.408E+00
10.2 9.374E+01 6.964E+01 4.613E+01 2.393E+01 1.057E+01 4.210E+00 1.942E+00 1.420E+00
10.3 1.017E+02 7.503E+01 4.940E+01 2.539E+01 1.107E+01 4.340E+00 1.972E+00 1.431E+00
10.4 1.103E+02 8.084E+01 5.293E+01 2.695E+01 1.161E+01 4.475E+00 2.001E+00 1.443E+00
10.5 1.197E+02 8.713E+01 5.671E+01 2.861E+01 1.217E+01 4.616E+00 2.032E+00 1.455E+00
10.6 1.300E+02 9.393E+01 6.079E+01 3.038E+01 1.276E+01 4.762E+00 2.063E+00 1.467E+00
10.7 1.411E+02 1.013E+02 6.517E+01 3.228E+01 1.338E+01 4.913E+00 2.096E+00 1.479E+00
10.8 1.532E+02 1.092E+02 6.988E+01 3.429E+01 1.404E+01 5.071E+00 2.129E+00 1.492E+00
10.9 1.663E+02 1.178E+02 7.495E+01 3.645E+01 1.474E+01 5.235E+00 2.162E+00 1.504E+00
11.0 1.806E+02 1.271E+02 8.040E+01 3.875E+01 1.547E+01 5.406E+00 2.197E+00 1.517E+00
11.1 1.962E+02 1.371E+02 8.627E+01 4.120E+01 1.625E+01 5.584E+00 2.232E+00 1.531E+00
11.2 2.131E+02 1.480E+02 9.259E+01 4.382E+01 1.706E+01 5.768E+00 2.269E+00 1.544E+00
11.3 2.316E+02 1.598E+02 9.940E+01 4.662E+01 1.793E+01 5.961E+00 2.306E+00 1.558E+00
11.4 2.516E+02 1.725E+02 1.067E+02 4.961E+01 1.884E+01 6.161E+00 2.344E+00 1.572E+00
11.5 2.735E+02 1.863E+02 1.146E+02 5.280E+01 1.980E+01 6.369E+00 2.384E+00 1.586E+00
11.6 2.973E+02 2.012E+02 1.231E+02 5.622E+01 2.082E+01 6.585E+00 2.424E+00 1.601E+00
11.7 3.232E+02 2.173E+02 1.323E+02 5.986E+01 2.190E+01 6.811E+00 2.465E+00 1.616E+00
11.8 3.514E+02 2.348E+02 1.421E+02 6.376E+01 2.303E+01 7.045E+00 2.507E+00 1.631E+00
11.9 3.821E+02 2.538E+02 1.528E+02 6.793E+01 2.423E+01 7.290E+00 2.551E+00 1.646E+00
12.0 4.156E+02 2.743E+02 1.642E+02 7.238E+01 2.551E+01 7.544E+00 2.595E+00 1.662E+00
12.1 4.520E+02 2.965E+02 1.766E+02 7.715E+01 2.685E+01 7.809E+00 2.641E+00 1.678E+00
12.2 4.917E+02 3.205E+02 1.899E+02 8.224E+01 2.827E+01 8.086E+00 2.688E+00 1.694E+00
12.3 5.349E+02 3.466E+02 2.042E+02 8.769E+01 2.977E+01 8.373E+00 2.736E+00 1.711E+00
12.4 5.821E+02 3.748E+02 2.197E+02 9.352E+01 3.136E+01 8.673E+00 2.785E+00 1.727E+00
12.5 6.334E+02 4.054E+02 2.364E+02 9.977E+01 3.305E+01 8.985E+00 2.835E+00 1.744E+00
12.6 6.894E+02 4.386E+02 2.544E+02 1.064E+02 3.483E+01 9.311E+00 2.887E+00 1.762E+00
12.7 7.504E+02 4.746E+02 2.739E+02 1.136E+02 3.671E+01 9.650E+00 2.940E+00 1.780E+00
12.8 8.169E+02 5.136E+02 2.948E+02 1.213E+02 3.871E+01 1.000E+01 2.995E+00 1.798E+00
12.9 8.894E+02 5.558E+02 3.175E+02 1.294E+02 4.082E+01 1.037E+01 3.051E+00 1.816E+00
13.0 9.684E+02 6.017E+02 3.419E+02 1.382E+02 4.306E+01 1.076E+01 3.108E+00 1.835E+00
13.1 1.055E+03 6.514E+02 3.682E+02 1.476E+02 4.543E+01 1.116E+01 3.167E+00 1.854E+00
13.2 1.149E+03 7.053E+02 3.967E+02 1.577E+02 4.794E+01 1.158E+01 3.227E+00 1.873E+00
13.3 1.251E+03 7.638E+02 4.274E+02 1.685E+02 5.060E+01 1.201E+01 3.289E+00 1.893E+00
13.4 1.363E+03 8.272E+02 4.606E+02 1.801E+02 5.342E+01 1.247E+01 3.353E+00 1.913E+00
13.5 1.485E+03 8.960E+02 4.964E+02 1.925E+02 5.641E+01 1.294E+01 3.418E+00 1.934E+00
13.6 1.618E+03 9.707E+02 5.351E+02 2.057E+02 5.958E+01 1.344E+01 3.485E+00 1.955E+00
13.7 1.763E+03 1.052E+03 5.770E+02 2.200E+02 6.294E+01 1.396E+01 3.554E+00 1.976E+00
13.8 1.921E+03 1.140E+03 6.221E+02 2.353E+02 6.650E+01 1.450E+01 3.625E+00 1.998E+00
13.9 2.094E+03 1.235E+03 6.709E+02 2.516E+02 7.028E+01 1.506E+01 3.697E+00 2.020E+00
14.0 2.282E+03 1.339E+03 7.237E+02 2.692E+02 7.429E+01 1.565E+01 3.772E+00 2.042E+00
14.1 2.487E+03 1.451E+03 7.807E+02 2.881E+02 7.854E+01 1.627E+01 3.848E+00 2.065E+00
14.2 2.712E+03 1.574E+03 8.423E+02 3.083E+02 8.305E+01 1.691E+01 3.927E+00 2.089E+00
14.3 2.957E+03 1.706E+03 9.089E+02 3.300E+02 8.784E+01 1.758E+01 4.007E+00 2.112E+00
14.4 3.224E+03 1.850E+03 9.810E+02 3.532E+02 9.292E+01 1.828E+01 4.090E+00 2.137E+00
14.5 3.516E+03 2.007E+03 1.059E+03 3.782E+02 9.832E+01 1.901E+01 4.175E+00 2.161E+00
14.6 3.834E+03 2.177E+03 1.143E+03 4.050E+02 1.040E+02 1.978E+01 4.262E+00 2.186E+00
14.7 4.182E+03 2.362E+03 1.234E+03 4.338E+02 1.101E+02 2.058E+01 4.352E+00 2.212E+00
14.8 4.561E+03 2.562E+03 1.333E+03 4.647E+02 1.166E+02 2.142E+01 4.444E+00 2.238E+00
14.9 4.976E+03 2.780E+03 1.439E+03 4.979E+02 1.234E+02 2.229E+01 4.539E+00 2.264E+00
15.0 5.428E+03 3.017E+03 1.555E+03 5.336E+02 1.307E+02 2.321E+01 4.636E+00 2.291E+00
15.1 5.923E+03 3.274E+03 1.679E+03 5.719E+02 1.385E+02 2.416E+01 4.736E+00 2.319E+00
15.2 6.462E+03 3.554E+03 1.814E+03 6.130E+02 1.467E+02 2.516E+01 4.839E+00 2.347E+00
15.3 7.052E+03 3.858E+03 1.961E+03 6.572E+02 1.554E+02 2.621E+01 4.944E+00 2.376E+00
15.4 7.696E+03 4.189E+03 2.119E+03 7.047E+02 1.647E+02 2.730E+01 5.053E+00 2.405E+00
15.5 8.399E+03 4.548E+03 2.290E+03 7.557E+02 1.746E+02 2.845E+01 5.164E+00 2.434E+00
15.6 9.168E+03 4.939E+03 2.475E+03 8.106E+02 1.851E+02 2.965E+01 5.279E+00 2.464E+00
15.7 1.001E+04 5.364E+03 2.676E+03 8.696E+02 1.963E+02 3.090E+01 5.396E+00 2.495E+00
15.8 1.092E+04 5.826E+03 2.893E+03 9.330E+02 2.082E+02 3.221E+01 5.517E+00 2.526E+00
15.9 1.193E+04 6.328E+03 3.129E+03 1.001E+03 2.208E+02 3.359E+01 5.642E+00 2.558E+00
16.0 1.302E+04 6.874E+03 3.384E+03 1.074E+03 2.343E+02 3.503E+01 5.770E+00 2.591E+00
16.1 1.422E+04 7.468E+03 3.660E+03 1.153E+03 2.486E+02 3.653E+01 5.901E+00 2.624E+00
16.2 1.553E+04 8.115E+03 3.959E+03 1.238E+03 2.638E+02 3.811E+01 6.036E+00 2.658E+00
16.3 1.695E+04 8.818E+03 4.283E+03 1.329E+03 2.800E+02 3.976E+01 6.176E+00 2.692E+00
16.4 1.852E+04 9.583E+03 4.634E+03 1.427E+03 2.972E+02 4.150E+01 6.319E+00 2.727E+00
16.5 2.022E+04 1.042E+04 5.014E+03 1.533E+03 3.156E+02 4.331E+01 6.466E+00 2.763E+00
16.6 2.209E+04 1.132E+04 5.427E+03 1.647E+03 3.351E+02 4.521E+01 6.617E+00 2.799E+00
16.7 2.413E+04 1.231E+04 5.873E+03 1.769E+03 3.559E+02 4.720E+01 6.773E+00 2.836E+00
16.8 2.636E+04 1.338E+04 6.357E+03 1.900E+03 3.781E+02 4.929E+01 6.933E+00 2.874E+00
16.9 2.880E+04 1.455E+04 6.882E+03 2.042E+03 4.017E+02 5.147E+01 7.098E+00 2.913E+00
17.0 3.147E+04 1.582E+04 7.451E+03 2.195E+03 4.268E+02 5.377E+01 7.267E+00 2.952E+00
17.1 3.438E+04 1.720E+04 8.068E+03 2.359E+03 4.536E+02 5.617E+01 7.442E+00 2.992E+00
17.2 3.757E+04 1.871E+04 8.737E+03 2.536E+03 4.821E+02 5.869E+01 7.621E+00 3.033E+00
17.3 4.105E+04 2.034E+04 9.462E+03 2.726E+03 5.125E+02 6.134E+01 7.806E+00 3.074E+00
17.4 4.487E+04 2.213E+04 1.025E+04 2.931E+03 5.449E+02 6.411E+01 7.996E+00 3.116E+00
17.5 4.904E+04 2.407E+04 1.110E+04 3.152E+03 5.795E+02 6.702E+01 8.192E+00 3.160E+00
17.6 5.360E+04 2.619E+04 1.203E+04 3.390E+03 6.163E+02 7.007E+01 8.393E+00 3.204E+00
17.7 5.858E+04 2.849E+04 1.303E+04 3.647E+03 6.556E+02 7.327E+01 8.601E+00 3.248E+00
17.8 6.404E+04 3.100E+04 1.412E+04 3.923E+03 6.975E+02 7.663E+01 8.814E+00 3.294E+00
17.9 7.001E+04 3.374E+04 1.530E+04 4.221E+03 7.421E+02 8.015E+01 9.034E+00 3.341E+00
18.0 7.654E+04 3.671E+04 1.658E+04 4.541E+03 7.897E+02 8.385E+01 9.261E+00 3.388E+00
18.1 8.368E+04 3.996E+04 1.797E+04 4.887E+03 8.405E+02 8.774E+01 9.494E+00 3.437E+00
18.2 9.149E+04 4.349E+04 1.948E+04 5.260E+03 8.947E+02 9.182E+01 9.734E+00 3.486E+00
18.3 1.000E+05 4.734E+04 2.112E+04 5.662E+03 9.525E+02 9.610E+01 9.981E+00 3.537E+00
18.4 1.094E+05 5.153E+04 2.290E+04 6.095E+03 1.014E+03 1.006E+02 1.024E+01 3.588E+00
18.5 1.196E+05 5.610E+04 2.483E+04 6.563E+03 1.080E+03 1.053E+02 1.050E+01 3.640E+00
18.6 1.308E+05 6.108E+04 2.692E+04 7.066E+03 1.150E+03 1.103E+02 1.077E+01 3.694E+00
18.7 1.431E+05 6.651E+04 2.920E+04 7.610E+03 1.225E+03 1.155E+02 1.105E+01 3.748E+00
18.8 1.565E+05 7.242E+04 3.167E+04 8.196E+03 1.305E+03 1.210E+02 1.133E+01 3.804E+00
18.9 1.712E+05 7.887E+04 3.435E+04 8.828E+03 1.391E+03 1.267E+02 1.163E+01 3.860E+00
19.0 1.873E+05 8.589E+04 3.726E+04 9.510E+03 1.482E+03 1.328E+02 1.194E+01 3.918E+00
19.1 2.048E+05 9.355E+04 4.042E+04 1.025E+04 1.580E+03 1.391E+02 1.225E+01 3.977E+00
19.2 2.241E+05 1.019E+05 4.385E+04 1.104E+04 1.684E+03 1.458E+02 1.257E+01 4.037E+00
19.3 2.452E+05 1.110E+05 4.758E+04 1.190E+04 1.795E+03 1.528E+02 1.291E+01 4.099E+00
19.4 2.682E+05 1.209E+05 5.163E+04 1.282E+04 1.914E+03 1.602E+02 1.325E+01 4.161E+00
19.5 2.935E+05 1.317E+05 5.603E+04 1.382E+04 2.041E+03 1.679E+02 1.361E+01 4.225E+00
19.6 3.211E+05 1.435E+05 6.081E+04 1.490E+04 2.176E+03 1.761E+02 1.397E+01 4.290E+00
19.7 3.514E+05 1.564E+05 6.600E+04 1.606E+04 2.321E+03 1.847E+02 1.435E+01 4.356E+00
19.8 3.845E+05 1.704E+05 7.164E+04 1.731E+04 2.476E+03 1.937E+02 1.474E+01 4.424E+00
19.9 4.208E+05 1.857E+05 7.777E+04 1.867E+04 2.642E+03 2.032E+02 1.514E+01 4.493E+00
20.0 4.606E+05 2.024E+05 8.444E+04 2.013E+04 2.819E+03 2.132E+02 1.555E+01 4.564E+00

Table 1Collisional Excitation Rate ratios (see Fig. 5)
(°K) Maxwell
5000 29.7012 48.1983 72.5995 138.179 322.942 914.582 2365.64 3551.70 5678.96
5500 29.4789 46.8930 69.0278 125.368 270.262 674.143 1513.02 2121.70 3117.32
6000 29.2609 45.6613 65.7814 114.480 229.899 515.460 1032.33 1372.76 1891.11
6500 29.0469 44.4974 62.8208 105.148 198.350 406.285 741.598 945.508 1238.84
7000 28.8369 43.3962 60.1122 97.0852 173.257 328.495 555.442 684.565 861.973
7500 28.6308 42.3530 57.6269 90.0701 152.988 271.388 430.514 516.106 629.358
8000 28.4285 41.3637 55.3402 83.9261 136.389 228.376 343.322 402.263 477.847
8500 28.2299 40.4242 53.2305 78.5127 122.629 195.251 280.418 322.330 374.680
9000 28.0348 39.5313 51.2794 73.7162 111.094 169.241 233.734 264.362 301.772
9500 27.8433 38.6815 49.4707 69.4446 101.329 148.467 198.235 221.147 248.601
10000 27.6551 37.8721 47.7904 65.6223 92.9877 131.622 170.664 188.154 208.767
10500 27.4702 37.1003 46.2259 62.1868 85.8035 117.779 148.851 162.440 178.225
11000 27.2886 36.3637 44.7665 59.0863 79.5699 106.266 131.311 142.033 154.330
11500 27.1102 35.6602 43.4024 56.2774 74.1239 96.5858 117.002 125.577 135.302
12000 26.9348 34.9875 42.1252 53.7234 69.3362 88.3683 105.179 112.119 119.912
12500 26.7623 34.3438 40.9273 51.3936 65.1029 81.3305 95.2955 100.973 107.292
13000 26.5928 33.7274 39.8019 49.2613 61.3397 75.2547 86.9487 91.6369 96.8137
13500 26.4262 33.1366 38.7429 47.3043 57.9780 69.9709 79.8335 83.7378 88.0182
14000 26.2623 32.5699 37.7450 45.5029 54.9612 65.3451 73.7166 76.9927 80.5612
14500 26.1012 32.0260 36.8034 43.8406 52.2424 61.2705 68.4173 71.1849 74.1819
15000 25.9426 31.5035 35.9135 42.3027 49.7824 57.6609 63.7940 66.1462 68.6799
15500 25.7867 31.0013 35.0715 40.8766 47.5483 54.4468 59.7342 61.7444 63.8991
16000 25.6333 30.5183 34.2739 39.5513 45.5125 51.5708 56.1483 57.8745 59.7166
16500 25.4823 30.0534 33.5173 38.3170 43.6512 48.9858 52.9635 54.4524 56.0347
17000 25.3338 29.6057 32.7988 37.1652 41.9444 46.6528 50.1207 51.4099 52.7748
17500 25.1876 29.1742 32.1158 36.0884 40.3747 44.5389 47.5714 48.6915 49.8733
18000 25.0437 28.7582 31.4658 35.0798 38.9272 42.6167 45.2751 46.2514 47.2781
18500 24.9020 28.3569 30.8466 34.1336 37.5891 40.8628 43.1986 44.0517 44.9463
19000 24.7625 27.9695 30.2562 33.2444 36.3492 39.2574 41.3137 42.0609 42.8424
19500 24.6252 27.5953 29.6926 32.4074 35.1975 37.7835 39.5966 40.2524 40.9365
20000 24.4900 27.2337 29.1543 31.6185 34.1256 36.4266 38.0273 38.6038 39.2038

Note. – (1) Maxwell figures computed using Lennon & Burke (1994) data.

Table 2[OIII] Line flux ratios vs kinetic temperature (see Fig. 8)
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