Issue 
A&A
Volume 551, March 2013



Article Number  A75  
Number of page(s)  8  
Section  Planets and planetary systems  
DOI  https://doi.org/10.1051/00046361/201220812  
Published online  25 February 2013 
On vertical variations of gas flow in protoplanetary disks and their impact on the transport of solids
Canadian Institute for Theoretical Astrophysics, University of Toronto, 60 St. Georges Street, Toronto, ON M5S 3H8, Canada
email: ejacquet@cita.utoronto.ca
Received: 28 November 2012
Accepted: 18 January 2013
A major uncertainty in accretion disk theory is the nature and properties of gas turbulence, which drives transport in protoplanetary disks. The commonly used viscous prescription for the MaxwellReynolds stress tensor gives rise to a meridional circulation where flow is outward near the midplane and inward away from it. This meridional circulation has been proposed as an explanation for the presence of hightemperature minerals (believed to be of inner solar system provenance) in comets. However, it has not been observed in simulations of magnetohydrodynamical (MHD) turbulence so far. In this study, we evaluate the extent to which the net transport of solids can be diagnostic of the existence of meridional circulation. To that end, we propose and motivate a prescription for MHD turbulence which has the same free parameters as the viscous one. We compare the effects of both prescriptions on the radial transport of small solid particles and find that their net, vertically integrated radial flux is actually quite insensitive to the flow structure for a given vertical average of the turbulence parameter α, which we explain. Given current uncertainties on disk turbulence, onedimensional models are thus most appropriate to investigate radial transport of solids. A corollary is that the presence of hightemperature material in comets cannot be considered an unequivocal diagnostic of meridional circulation. In fact, we argue that outward transport in viscous disk models with inward net accretion is more properly attributed to turbulent diffusion rather than to the mean flows of the gas.
Key words: accretion, accretion disks / instabilities / magnetohydrodynamics (MHD) / turbulence / comets: general / meteorites, meteors, meteoroids
© ESO, 2013
1. Introduction
Extraterrestrial samples provide ample evidence for significant radial transport in the protoplanetary disk from which the solar system emerged. For instance, carbonaceous chondrites contain hightemperature materials such as refractory inclusions, believed to have formed close to the Sun in the first stages of disk building (Wood 2004), chondrules, formed 1−3 Ma later (Villeneuve et al. 2009), as well as aqueous alteration products indicating the presence of ice when these meteorites accreted. Yet more spectacularly, rare refractory objects and chondrulelike fragments have been identified in dust returned from comet Wild 2 (Zolensky et al. 2006; Bridges et al. 2012).
One way of transporting solids outward from the vicinity of the Sun is through bipolar outflows, as in the Xwind model of Shu et al. (2001, see also Hu 2010); however, whether solids can be present at and efficiently transported from the X point has been called into question by Desch et al. (2010). More recently, scenarios have been proposed where transport is effected inside the disk by turbulent motions of the gas – that same turbulence which would also drive accretion of the disk gas onto the central star (BockeléeMorvan et al. 2002; Boss 2004; Carballido et al. 2005; Johansen & Klahr 2005; Ciesla 2009; Hughes & Armitage 2010; Jacquet et al. 2011; Yang & Ciesla 2012). In early stages, where the disk is massive, such turbulence could be due to gravitational instabilities (Boss 2004) whereas magnetohydrodynamical (MHD) turbulence powered by the magnetorotational instability (MRI; Balbus & Hawley 1998) should dominate afterward. However, the MRI is expected to be suppressed over a significant range of heliocentric distances because of insufficient ionization (Gammie 1996), so that in this region, referred to as the “dead zone”, turbulence should be reduced and have a more hydrodynamical character.
While many studies have restricted attention to onedimensional disk models, where only the vertically averaged turbulence parameter α had to be prescribed, some have attempted to calculate the transport of solids in two or threedimensional disk models (e.g. Hersant et al. 2001; Ciesla 2009; Charnoz et al. 2011; Ciesla 2010a, 2011). Going to 2D or 3D requires however more assumptions on the properties of turbulence to be made despite the considerable uncertainties of accretion disk theory and the diversity of potential turbulence drivers alluded to in the previous paragraph. A widespread prescription models turbulence as an effective viscosity in the averaged dynamical equations of the gas (e.g. Takeuchi & Lin 2002): the circulation resulting from this “viscous” prescription typically involves an outward flow around the disk midplane and inward flows in the “atmosphere”, with the vertically integrated flow being inward (i.e. a positive mass accretion rate). This meridional circulation was found by Ciesla (2007) to improve outward transport of inner solar system material and hence account for the presence of hightemperature minerals in comets. However as yet, the meridional circulation is an essentially theoretical construct that has not yet been observed in numerical simulations of turbulent disks, in particular in the global MHD simulations of Fromang et al. (2011) and Flock et al. (2011). As yet, the vertical structure of the gas flow is uncertain.
The purpose of this article is to investigate, through analytical calculations, to what extent the net outward transport of small solids can be considered a diagnostic for meridional circulation. We propose and motivate a prescription for the vertical profile of the MaxwellReynolds stress tensor in the case of MHD turbulence and calculate the resulting mean flow of the gas. The prescription, inspired by previous numerical studies, formally depends on the same parameters as the standard “viscous” prescription, allowing a direct comparison. In particular, we compute the net (vertically integrated) radial flux of solids in both prescriptions. It is found that this net flux is weakly dependent on the prescription used, which will be explained, and that therefore meteoritic and cometary properties cannot be used as evidence for a specific vertical flow profile.
This article is organized as follows: in Sect. 2, we introduce general notions on gas turbulence and the two prescriptions considered here. In Sect. 3, we investigate and compare the dynamics of solids in both prescriptions. We discuss the results in Sect. 4 before concluding in Sect. 5.
2. Modeling of gas turbulence
In this section, we introduce the modeling of gas turbulence. After having reviewed general equations, by way of establishing notation, we introduce the two prescriptions of the MaxwellReynolds tensor investigated in this paper, namely the viscous and the MHD prescriptions.
2.1. Generalities
The disk is described in a cylindrical coordinate system, with R the heliocentric distance, z the altitude above the midplane, and φ the azimuthal angle. We note u, ρ, T and the gas velocity, density, temperature and pressure, respectively, with c_{s} the isothermal sound speed . and Ω = v_{K}/R are the Keplerian linear and angular velocities, respectively.
We treat the disk as vertically isothermal^{1} so that vertical hydrostatic equilibrium implies the following density stratification: (1)with the pressure scale height H = c_{s}/Ω and the surface density .
We assume the disk to be turbulent and assume axisymmetry in the sense that variations of any quantity Q in the azimuthal direction may be treated as turbulent fluctuations about a mean . We denote the Eulerian perturbations with . For any quantity Q and a weight function w, we also define the wweighted vertical average of Q as: (2)Because of the pressure gradient and the departure from the equatorial plane for z ≠ 0, u_{φ} is not exactly equal to the Keplerian velocity v_{K}. Indeed, centrifugal balance yields: (3)where we have used z,H ≪ R. Since, generally, ∂P(R,0)/∂R < 0 and ∂lnT/∂R < 0, the flow is subkeplerian (e.g. Fromang et al. 2011; Flock et al. 2011). However, the approximation u_{φ} ≈ v_{K} will be generally sufficient except where derivatives in z will be invoked (in Sect. 2.2).
The angular momentum equation, averaged over turbulent fluctuations, reads (Balbus & Papaloizou 1999): (4)where T_{Rφ} and T_{zφ}, the Rφ and zφ components of the turbulent stress tensor, are defined as: (5)with B the magnetic field and i = R,z. We parameterize T_{Rφ} as: (6)Note that Eq. (6) is only a definition and does not presuppose any prescription of the stress tensor. In particular, α may a priori vary with R and z. The arbitrary factor 3/2 has been introduced to facilitate direct comparison with the turbulent viscosity formalism.
Equation (4) may be rewritten as: (7)From now on, we will drop the overbars. The latter equation may be integrated to yield the vertical densityweighted average ⟨ u_{R} ⟩ _{ρ} (e.g. LyndenBell & Pringle 1974)^{2}: (8)Thus, the net radial transport of gas depends only on ⟨ α ⟩ _{P} as far as turbulence properties are concerned.
We now turn to the two prescriptions for the MaxwellReynolds tensor to be considered in this paper, namely the “viscous” and the “MHD” prescription.
2.2. The viscous prescription
The viscous prescription, first introduced for hydrodynamical turbulence by Boussinesq (1877) and Reynolds (1895) – but see e.g. Schmitt (2007) –, and commonly used in protoplanetary disk contexts (e.g. Urpin 1984; Takeuchi & Lin 2002; Ciesla 2009), assumes that turbulence can be modeled as an effective kinematic viscosity ν, so that: where we have made use of Eq. (3).
Comparing Eq. (9) with Eq. (6) leads to the identification: (11)At this point the viscous prescription is nontautological only in the prescription of T_{zφ}. It is generally further assumed that α is constant, at least vertically, i.e.: (12)The radial velocity may then be calculated from Eq. (7): (13)This flow, parabolic in z, is known as the meridional circulation (see Fig. 1). Typically, the velocity near the midplane is positive (Takeuchi & Lin 2002), but the inward flows away from this region result in a positive net (vertically integrated) mass accretion rate (i.e. toward the Sun; see Eq. (8)). This circulation may be interpreted as follows: at the midplane, the large radial density gradient (ρ ∝ ΣΩ/c_{s}) makes the viscous torque exerted from the inner, more rapidly rotating disk regions greater than that received from the outer, slower rotating disk, hence a net gain of angular momentum and an outward flow; at high altitudes, however, the density gradient is reduced and even switches sign, changing the direction of the effect (e.g. Takeuchi & Lin 2002).
2.3. MRIturbulent disk prescription
Fig. 1
Mean radial velocity of the gas for the viscous (dashed) and the MHD (continuous line) prescriptions. We have taken Σ,T ∝ R^{0.75}, and α(R,0) ∝ R^{a} (with the local value of ⟨ α ⟩ _{P} being 10^{2}), with three values of the exponent a used in the plots. The viscous prescription entails a parabolic flow profile (the socalled meridional circulation) while the MHD prescription entails an inverted Gaussian profile (until the corona, here at  z  > z_{max} = 3.0 H). Here, for a = −1, the vertically integrated flow is outward in both prescriptions. 
Simulations of magnetohydrodynamic turbulence have so far failed to exhibit a meridional circulation (Fromang et al. 2011; Flock et al. 2011) and this may be traced to the discrepancy between the measured stress tensor and that assumed in the viscous prescription (Fromang et al. 2011). As noted by numerous numerical studies (Miller & Stone 2000; Hirose et al. 2006; Flaig et al. 2010; Fromang & Nelson 2006; Dzyurkevich et al. 2010; Sorathia et al. 2010; Fromang et al. 2011, 2013; Flock et al. 2011; Guan & Gammie 2011; Bai & Stone 2012; see also Uzdensky 2012), the vertical profile of T_{Rφ} shows a plateau for  z  lower than a given z_{max}. It then falls off, proportional to the density, in the corona, where magnetic pressure is comparable to the gas pressure, quenching the MRI and leaving a transsonic turbulence there (e.g. Flock et al. 2011). We thus adopt: (14)with θ the Heaviside function, defined as: (15)We thus have (16)with (17)As to α_{max}, we will adopt in numerical applications the fiducial value 1/3 that arises in the ideal MHD limit of the study of Bai & Stone (2011)^{3}. This clearly differs from the viscous prescription.
We hence have: (18)with erfc the complementary Gauss error function defined as: (19)Note that we have made no assumption on the value of α(R,0) or on how it scales with other disk parameters as we focus here on the z dependence of the flow.
Considerably less is known about T_{zφ}. We propose a break at  z  = z_{max} similar to that of T_{Rφ} in the form: (20)with C(R,z) an as yet unspecified smooth function which symmetry about the midplane requires to be odd in z. By requiring that u_{R} as expressed by Eq. (7) be continuous at z = ± z_{max}, we have: (21)which essentially sets the scale of T_{zφ} ~ (H/R)T_{Rφ}^{4}. If we adopt the simplest dependence C(R,z) ∝ z, we obtain: (22)This yields a profile similar to that measured by Fromang et al. (2011).
Equations (14) and (22) constitute what we will refer to as the “MHD prescription”. It is noteworthy that it involves the same free parameters (α(R,0), or equivalently ⟨ α ⟩ _{P}, and its possible radial derivative) as the viscous one.
The mean radial velocity resulting from this prescription may then be calculated. For  z  ≤ z_{max}, (23)and for  z  ≥ z_{max}, (24)The flow is plotted in Fig. 1. In contrast to the meridional circulation, velocities do not change sign (except perhaps in the corona if ∂α(R,0)/∂R ≠ 0). Indeed the stress tensor no longer scales with the density vertically, in contrast to the viscous prescription, and thus the effect of the change in radial density gradient with height (see Sect. 2.2) disappears. Then, the radial velocity does not switch sign, and always has that of its average (at least outside the corona). The profiles are similar to those arising from the global simulations of Fromang et al. (2011). They differ, however, from those of Flock et al. (2011), which resemble an inverted meridional circulation profile, where the positive velocities in the corona correspond to outflows potentially escaping the disk. Such outflows launched from the disk have been also recently studied in local simulations with uniform initial vertical magnetic field (Lesur et al. 2013; Bai & Stone 2012; Fromang et al. 2013) and if present, are thus not captured by our prescription of T_{zφ} (which would not vanish at infinity for outflowlaunching simulations). We shall however argue later that its exact form has little effect on our conclusions. Our prescription for the MaxwellReynolds tensor is thus only intended here to provide a sensible MHD counterpart to the viscous one for comparison purposes. Certainly, more measurements of T_{Rφ} and T_{zφ} in stratified numerical simulations are needed to arrive at a more definitive prescription.
3. Impact on the dynamics of solids
With the two above prescriptions on the gas flow in hand, we now investigate their impact on the dynamics of solids tightly coupled to the gas. We first briefly review the basic concepts of aerodynamic transport of solids in disks, before focusing on the vertical distribution of particles and their net radial motions.
3.1. Generalities
Let us consider a population of identical spherical particles of internal density ρ_{s} and radius a embedded in the gas. We denote by ρ_{p} the density of this population (viewed as a fluid) and (25)their vertically integrated surface density. We also define a normalized solidtogas ratio f by: (26)The effects of gas drag is characterized by a stopping time τ (see e.g. Weidenschilling 1977) from which one can define a measure of the coupling of the particles to the gas on an orbital timescale as (27)which we will take to be ≪ 1 in accordance with our tight coupling assumption.
Neglecting any feedback of the solids on the gas, the continuity equation averaged over turbulent fluctuations reads: (28)where we have introduced the mean velocity v_{p} of the particles given by (Youdin & Goodman 2005) (29)and also diffusion coefficients D_{RR} and D_{zz} parameterized as: (30)with δ_{R} and δ_{z} dimensionless parameters of order α . We will assume that the radial and vertical Schmidt numbers (31)are vertically constant.
Following Jacquet et al. (2012), we coin: (32)which measure the coupling between particles and gas on a global scale, in the radial and vertical directions, respectively.
3.2. Vertical distribution
Fig. 2
Dusttogas ratio normalized to the column density ratio (f) as a function of z, for both viscous (dashed line) and MRIturbulent prescriptions (solid line) and for three values of the “settling parameter” S_{z} ≡ St/ ⟨ δ_{z} ⟩ _{P}, with ⟨ δ_{z} ⟩ _{P} = 10^{2}. In the viscous prescription, this ratio falls off as a “double Gaussian” whereas it only does so as a Gaussian for the MHD prescription over the bulk of the disk thickness, before decreasing as a “double Gaussian” in the corona (here at  z  > z_{max} = 3.0H). 
Equation (28) is dominated by the vertical flux balance between settling and diffusion. On timescales longer than the vertical mixing timescale (33)the vertical distribution of the particles obeys: (34)where the role of S_{z} as a measure of settling is apparent. It may be noted that our assumption of constant Sc_{z} makes the vertical distribution independent of the prescription of T_{zφ}.
In the viscous prescription, where α, and hence δ_{z} is vertically constant, S_{z} ∝ ρ^{1} so that Eq. (34) may be integrated as (Takeuchi & Lin 2002): (35)a “double Gaussian” which drops rapidly at large  z .
In the MHD prescription, S_{z} is vertically constant for  z  ≤ z_{max} before increasing as ρ^{1} in the corona. This gives: (36)for  z  ≤ z_{max}, and (37)for  z  > z_{max}, with (38)At first the solidtogas ratio falls off only as a Gaussian (because of increasing α counteracting looser coupling due to decreasing ρ) and only in the corona does it decrease as a “double Gaussian” similarly to the viscous prescription case. Thus, a purely Gaussian fit tends to overestimate, and a “double Gaussian” one to underestimate the dust density away from the midplane in this case, as observed by Fromang & Nelson (2009) in their simulations of dust settling in MRIdriven turbulence.
The vertical distribution in both prescriptions is plotted in Fig. 2. Similarly to Fromang & Nelson (2009), we suggest that observations of presentday protoplanetary disks, in probing dust remaining on their surface, could discriminate between the two vertical distributions.
3.3. Net radial flow
Fig. 3
Net vertically averaged velocity v_{p,1D} as a function of S = St(R,0)/ ⟨ α ⟩ _{P} for the viscous prescription (dashed line) and the MHD prescription (solid line), for three values of Sc_{z} (0.1 in blue, 1 in green and 10 in red). The velocities are always inward and we plot here their absolute value. We have taken Σ,T ∝ R^{0.75}, ∂α(R,0)/∂R = 0, δ_{R} = δ_{z} and ⟨ α ⟩ _{P} = 10^{2}. The dotted line corresponds to the simple onedimensional approximation (see Eq. (42)) which is common to both prescriptions and independent of Sc_{z}. The approximation is arbitrarily good in the limits S ≪ 1 and S ≫ 1 and the imparted error does not exceed a factor of two when S ~ 1 except for the viscous prescription at Sc_{z} = 10 where it can reach one order of magnitude. 
We now turn to the radial motions of the particles. Specifically, we want to integrate the continuity Eq. (28) over z and deduce the net radial flow for both prescriptions. Formally, the result of this integration reads: (39)with (40)where (41)is a correction from the diffusion term, which is generally negative (see e.g. Eq. (A.4)), as the disk thickens with increasing heliocentric distance, inducing its “surface” to diffuse particles inward into the rarefied, particledepleted gas.
If we restrict interest to timescales longer than t_{vm}, we can adopt the equilibrium vertical distributions of the previous subsection to calculate the above. Results are presented in Appendix A and v_{p,1D} is plotted in Fig. 3 for different values of the vertical Schmidt number. The main conclusion to draw from this plot is this net velocity is weakly dependent on the exact flow structure and is generally well approximated by (42)a widespread formula in onedimensional calculations (e.g. Cuzzi et al. 2003; Ciesla 2010b; Hughes & Armitage 2010; Yang & Ciesla 2012). Agreement is arbitrarily good when S is either very large or very small, and the deviation is largest for S ~ 1. The deviation is generally less than a factor of 2, except for the viscous prescription if the Schmidt number is large. But even then, the net radial velocity does not (in general) become positive, as had been noted by Takeuchi & Lin (2002), even if they had not included the diffusion correction.
Why does the 1D approximation (42) provide a so good match, at least when Sc_{R} ~ Sc_{z} ~ 1? This stems from the facts that (see also Jacquet et al. 2012):

(i)
In the limitS,S_{z} ≪ 1, particles are wellmixed with the gas and only drift negligibly with respect to it, so that their verticallyaveraged velocity is indistinguishable from that of the gas, ⟨ u_{R} ⟩ _{ρ}.

(ii)
In the limit S,S_{z} ≫ 1, particles are concentrated at the midplane and their motion is dominated by dragrelated drift (evaluated in this region), so that their net radial velocity is essentially v_{drift}(R,0).
As the expression (42) captures both limiting behaviors – with diffusion correction v_{p,corr} being negligible in both limits (Jacquet et al. 2012) –, it indeed provides a suitable approximation for all possible values of S. It is noteworthy that the above reasoning is general and extends to prescriptions other than the ones considered in this study, e.g. if one adopts an alternative mathematical expression for T_{zφ} in the MHD prescription^{5}.
In detail, some deviation is expected (and seen in Fig. 3) for S ~ 1 which is outside either above limit, but as the approximations just begin to break down there, the order of magnitude at least should be accurate. If however Sc_{z} is very different from unity, the domain of nonvalidity of the above regimes is wider, and depending on the vertical variations of the velocities, this could impart a more significant error. This is what we see for the viscous prescription if Sc_{z} ≫ 1. Indeed, under such conditions, one can have S < 1 < S_{z}: then, the particles are concentrated around the midplane (since S_{z} > 1) so that their gas velocity has an important contribution from the outwarddirected flows, which is incompletely compensated by the inward dragrelated drift (since S ~ v_{drift}/u_{R} < 1), hence a significantly less negative v_{p,1D}. We note however that large values of the Schmidt number are not expected in the hydrodynamical turbulence which the viscous prescription is intended to model (Prinn 1990; Dubrulle & Frisch 1991), in contrast to MHD turbulence (Carballido et al. 2005; Johansen & Klahr 2005; Johansen et al. 2006), so that this situation appears unlikely anyway.
4. Discussion
From the preceding section, it appears that the net radial transport of particles is weakly sensitive to the vertical flow structure and is well approximated by the onedimensional expression given by Eq. (42). In particular, if the mass accretion rate is positive (toward the Sun), the nondiffusive contribution to the net radial flux should be generally inward.
This might seem paradoxical in the case of the viscous prescription, as then, a population of small (S ≪ 1) particles around the midplane should be transported outward, even in the absence of turbulent diffusion. The paradox lies in our calculation pertaining to timescales longer than the vertical mixing timescale t_{vm} (to warrant use of the equilibrium vertical distribution of particles) and thus to radial scales larger than the corresponding radial excursion (43)So while a finger of material lying near the midplane would undergo some outward transport in the viscous prescription, it would not travel significantly further than this if we ignore radial diffusion. This we can see perhaps more concretely with a simple toy model, which we now present (see also Fig. 4):
Fig. 4
Cartoon of the toy model for meridional circulation. We distinguish between an “outward transport zone” (rightward arrows) and an “inward transport zone” (leftward arrows), which are assigned fractions θ and 1 − θ (θ < 1/2) of the local column density, respectively. Integers n − 1, n, n + 1 represent radial locations whose separation corresponds to one vertical mixing timescale. Vertical mixing is symbolized by double vertical arrows. 
We consider the disk thickness to consist in an “outward transport zone” (the midplane), comprising a fraction θ of material, and an “inward transport zone” (the “atmosphere”). We ignore radial diffusion and consider that both zones transport material at equal and opposite velocities, so that the net flow is inward if θ < 1/2, as we shall henceforth assume. We discretize time and space (in the radial direction), with the temporal and radial steps being t_{vm} and ΔR_{vm}, respectively. Each time step corresponds to two successive motions: advection one radial step forward or backward within each zone, and vertical mixing between the two zones. Thus, if we denote by u_{n,t} the total column density of a contaminant at time t and at radial location n–both natural integers, in units of t_{vm} and ΔR_{vm}–, u_{n,t + 1} is given by: (44)As boundary condition, we set u_{0,t} = 1 (in some arbitrary unit) and as initial condition u_{n,0} = 0 for n ≥ 1.
One can demonstrate^{6} that u_{n,t} determined by Eq. (44) and its boundary and initial conditions satisfies:

(i)
u_{n,t} is a monotonically decreasing function of n.

(ii)
u_{n,t} is a monotonically increasing function of t.

(iii)
0 ≤ u_{n,t} ≤ (θ/(1 − θ))^{n} (with the upper bound being a stationary solution of Eq. (44)).

(iv)
u_{n,t} converges toward (θ/(1 − θ))^{n} as t → + ∞.
Since θ < 1/2, (θ/(1 − θ))^{n} and a fortiori u_{n,t} vanish as n → + ∞ and in practice become negligibly small after several radial steps, corresponding, if we revert to physical units, to a radial excursion much smaller than R. The conclusion from this toy model is thus that no significant outward transport can be achieved without including radial diffusion, even in a meridional circulation context.
However, 2D disk models assuming the viscous prescription did include radial diffusion, and did achieve significant outward transport (e.g. Ciesla 2009), but from the above, the latter should be viewed as being caused by the turbulent diffusion rather than the meridional circulation itself. Nonetheless, it does hold that the meridional circulation, in reducing somewhat the inward advective velocities (see Fig. 3) which counteract turbulent diffusion, enhances outward transport relative to the onedimensional approximation, and this can have nonnegligible effects for longrange transport. For example, in the “outward transport” simulation of Ciesla (2009) with Ṁ = 10^{6} M_{⊙}/yr, a crystalline fraction of 40% is obtained (after 10^{5} yr) at 10 AU, where the onedimensional approximation would have predicted 17% (using Eq. (29) of Jacquet et al. 2012). However, the onedimensional model would have retrieved a crystallinity of 40% had we taken Sc_{R} = 0.5 instead of the Sc_{R} = 1 chosen by Ciesla (2009), which is at least equally plausible. Thus, the differences between meridional circulation and the onedimensional approximation circulation are actually within the errors of turbulence parameters. A corollary is that the occurrence of hightemperature materials in the samples returned from comet Wild 2 (Zolensky et al. 2006) is not diagnostic per se of meridional circulation. More generally, net radial transport of early solar system material is no compelling constraint on the vertical variations of the gas flow. The question of the form of the MaxwellReynolds tensor in protoplanetary disks, be it in MRIactive regions or in the dead zone, is thus most appropriately addressed by numerical simulations of gas turbulence, although, as we mentioned earlier, observations of protoplanetary disks could also offer important diagnostics linked to settling.
We caution before closing this section that we have not considered, in this study, the possibility of outflows launched from the disk (e.g. Flock et al. 2011; Bai & Stone 2012; Fromang et al. 2013; Lesur et al. 2013), which would yield a sink term on the righthandside of Eq. (39) – potentially important for vertically wellmixed particles (S_{z} ≪ 1). The possibility and quantitative importance of such outflows has yet to be explored in more details before their impact on the radial motion of solids can be satisfactorily addressed.
5. Conclusion
In this paper, we have considered two possible flow structures in the protoplanetary disk, which correspond to two different prescriptions of the turbulent MaxwellReynolds tensor:

(i)
A viscous prescription, commonly used in the litterature,which typically gives rise to the socalled meridional circulationwith outward flows around the midplane and inward flows awayfrom it.

(ii)
A MHD prescription, which we introduce and motivate, appropriate for magnetohydrodynamical turbulence (without outflows) and where velocities retain the same sign over the bulk of the disk’s thickness.
We have compared their effects on the dynamics of small solids. While, in the vertical direction, the distribution falls off less steeply (as a Gaussian) in the MHD prescription than in the viscous one, it is found that the net radial flux differs little between the two. In fact, this radial flux is well approximated by a commonly used onedimensional formula, which only depends on the vertically averaged turbulence parameter ⟨ α ⟩ _{P}. We have shown that this can be generally expected for any likely prescription of the flow (and not only those considered here).
It thus follows that in itself, evidence of outward transport of inner solar system material to the cometforming region cannot be viewed as diagnostic of meridional circulation, whose physical reality is still controversial. In fact, if the mass accretion rate is positive, this outward transport is rather to be attributed to turbulent diffusion. More generally, the net radial transport of early solar system material does not significantly constrain the flow structure of the gas over the disk’s thickness.
Although this approximation breaks down in the surface layers of the disk (e.g. Chiang & Goldreich 1997), this is of no concern here as this generally affects a small fraction of the surface density of the gas and an even smaller one of that of the (partly settled) solids.
This assumes that T_{zφ} vanishes at infinity, which may not hold in case of steady outflows, but even then, its contribution to ⟨ u_{R} ⟩ _{ρ} is likely negligible (Bai & Stone 2012; Fromang et al. 2013).
We have recast their Eqs. (23) and (25) in terms of our definition of α (Eq. (6)); α_{max} corresponds here to the limit where gas and magnetic pressure are equal.
Note that while our derivation makes T_{zφ} depend on the formally nonlocal quantity ∂z_{max}/∂R, this is not inconsistent with the fact that local simulations can exhibit a nonzero T_{zφ} (see e.g. Fromang et al. 2013) to which the radial gradient of α might adjust.
Acknowledgments
The author thanks Matthieu Gounelle and Sébastien Fromang for interesting discussions on the topic of meridional circulation, as well as an anonymous referee whose comments helped in particular to interpret the qualitative difference between the two flows.
References
 Bai, X.N., & Stone, J. M. 2011, ApJ, 736, 144 [NASA ADS] [CrossRef] [Google Scholar]
 Bai, X.N., & Stone, J. M. 2012, ApJ, submitted [arXiv:1210.6661] [Google Scholar]
 Balbus, S. A., & Hawley, J. F. 1998, Rev. Mod. Phys., 70, 1 [Google Scholar]
 Balbus, S. A., & Papaloizou, J. C. B. 1999, ApJ, 521, 650 [NASA ADS] [CrossRef] [Google Scholar]
 BockeléeMorvan, D., Gautier, D., Hersant, F., Huré, J., & Robert, F. 2002, A&A, 384, 1107 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Boss, A. P. 2004, ApJ, 616, 1265 [NASA ADS] [CrossRef] [Google Scholar]
 Boussinesq, J. 1877, Mémoires présentés par divers savants à l’Académie des Sciences, 23, 1 [Google Scholar]
 Bridges, J. C., Changela, H. G., Nayakshin, S., Starkey, N. A., & Franchi, I. A. 2012, Earth Planet. Sci. Lett., 341, 186 [Google Scholar]
 Carballido, A., Stone, J. M., & Pringle, J. E. 2005, MNRAS, 358, 1055 [NASA ADS] [CrossRef] [Google Scholar]
 Charnoz, S., Fouchet, L., Aleon, J., & Moreira, M. 2011, ApJ, 737, 33 [NASA ADS] [CrossRef] [Google Scholar]
 Chiang, E. I., & Goldreich, P. 1997, ApJ, 490, 368 [NASA ADS] [CrossRef] [Google Scholar]
 Ciesla, F. J. 2007, Science, 318, 613 [NASA ADS] [CrossRef] [PubMed] [Google Scholar]
 Ciesla, F. J. 2009, Icarus, 200, 655 [NASA ADS] [CrossRef] [Google Scholar]
 Ciesla, F. J. 2010a, ApJ, 723, 514 [NASA ADS] [CrossRef] [Google Scholar]
 Ciesla, F. J. 2010b, Icarus, 208, 455 [NASA ADS] [CrossRef] [Google Scholar]
 Ciesla, F. J. 2011, ApJ, 740, 9 [NASA ADS] [CrossRef] [Google Scholar]
 Cuzzi, J. N., Davis, S. S., & Dobrovolskis, A. R. 2003, Icarus, 166, 385 [NASA ADS] [CrossRef] [Google Scholar]
 Desch, S. J., Morris, M. A., Connolly, Jr., H. C., & Boss, A. P. 2010, ApJ, 725, 692 [NASA ADS] [CrossRef] [Google Scholar]
 Dubrulle, B., & Frisch, U. 1991, Phys. Rev. A, 43, 5355 [NASA ADS] [CrossRef] [MathSciNet] [PubMed] [Google Scholar]
 Dzyurkevich, N., Flock, M., Turner, N. J., Klahr, H., & Henning, T. 2010, A&A, 515, A70 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Flaig, M., Kley, W., & Kissmann, R. 2010, MNRAS, 409, 1297 [NASA ADS] [CrossRef] [Google Scholar]
 Flock, M., Dzyurkevich, N., Klahr, H., Turner, N. J., & Henning, T. 2011, ApJ, 735, 122 [NASA ADS] [CrossRef] [Google Scholar]
 Fromang, S., & Nelson, R. P. 2006, A&A, 457, 343 [NASA ADS] [CrossRef] [EDP Sciences] [MathSciNet] [Google Scholar]
 Fromang, S., & Nelson, R. P. 2009, A&A, 496, 597 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Fromang, S., Lyra, W., & Masset, F. 2011, A&A, 534, A107 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Fromang, S., Latter, H. N., Lesur, G., & Ogilvie, G. I. 2013, A&A, in press, DOI: 10.1051/00046361/201220016 [Google Scholar]
 Gammie, C. F. 1996, ApJ, 457, 355 [NASA ADS] [CrossRef] [Google Scholar]
 Guan, X., & Gammie, C. F. 2011, ApJ, 728, 130 [NASA ADS] [CrossRef] [Google Scholar]
 Hersant, F., Gautier, D., & Huré, J.M. 2001, ApJ, 554, 391 [NASA ADS] [CrossRef] [Google Scholar]
 Hirose, S., Krolik, J. H., & Stone, J. M. 2006, ApJ, 640, 901 [NASA ADS] [CrossRef] [Google Scholar]
 Hu, R. 2010, ApJ, 725, 1421 [NASA ADS] [CrossRef] [Google Scholar]
 Hughes, A. L. H., & Armitage, P. J. 2010, ApJ, 719, 1633 [NASA ADS] [CrossRef] [Google Scholar]
 Jacquet, E., Fromang, S., & Gounelle, M. 2011, A&A, 526, L8 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Jacquet, E., Gounelle, M., & Fromang, S. 2012, Icarus, 220, 162 [NASA ADS] [CrossRef] [Google Scholar]
 Johansen, A., & Klahr, H. 2005, ApJ, 634, 1353 [NASA ADS] [CrossRef] [Google Scholar]
 Johansen, A., Klahr, H., & Mee, A. J. 2006, MNRAS, 370, L71 [NASA ADS] [Google Scholar]
 Lesur, G., Ferreira, J., & Ogilvie, G. 2013, A&A, 550, A61 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 LyndenBell, D., & Pringle, J. E. 1974, MNRAS, 168, 603 [NASA ADS] [CrossRef] [Google Scholar]
 Miller, K. A., & Stone, J. M. 2000, ApJ, 534, 398 [NASA ADS] [CrossRef] [Google Scholar]
 Prinn, R. G. 1990, ApJ, 348, 725 [NASA ADS] [CrossRef] [Google Scholar]
 Reynolds, O. 1895, Phil. Trans. R. Soc., 186, 123 [Google Scholar]
 Schmitt, F. G. 2007, Comptes Rendus Mecanique, 335, 617 [Google Scholar]
 Shu, F. H., Shang, H., Gounelle, M., Glassgold, A. E., & Lee, T. 2001, ApJ, 548, 1029 [NASA ADS] [CrossRef] [Google Scholar]
 Sorathia, K. A., Reynolds, C. S., & Armitage, P. J. 2010, ApJ, 712, 1241 [NASA ADS] [CrossRef] [Google Scholar]
 Takeuchi, T., & Lin, D. N. C. 2002, ApJ, 581, 1344 [NASA ADS] [CrossRef] [Google Scholar]
 Urpin, V. A. 1984, Sov. Astron., 28, 50 [NASA ADS] [Google Scholar]
 Uzdensky, D. A. 2012 [arXiv:1205.6537] [Google Scholar]
 Villeneuve, J., Chaussidon, M., & Libourel, G. 2009, Science, 325, 985 [NASA ADS] [CrossRef] [PubMed] [Google Scholar]
 Weidenschilling, S. J. 1977, MNRAS, 180, 57 [NASA ADS] [CrossRef] [Google Scholar]
 Wood, J. A. 2004, Geochim. Cosmochim. Acta, 68, 4007 [NASA ADS] [CrossRef] [Google Scholar]
 Yang, L., & Ciesla, F. J. 2012, Meteo. Planet. Sci., 47, 99 [Google Scholar]
 Youdin, A. N., & Goodman, J. 2005, ApJ, 620, 459 [NASA ADS] [CrossRef] [Google Scholar]
 Zolensky, M. E., Zega, T. J., Yano, H., et al. 2006, Science, 314, 1735 [NASA ADS] [CrossRef] [PubMed] [Google Scholar]
Appendix A: exact results for verticallyintegrated radial particle flux in the viscous and MHD prescription
We list here exact results for different quantities allowing one to calculate the net radial flux of solids in the two prescriptions, assuming an equilibrium vertical distribution of the said solids.
Appendix A.1: Viscous prescription
Appendix A.2: MHD prescription
All Figures
Fig. 1
Mean radial velocity of the gas for the viscous (dashed) and the MHD (continuous line) prescriptions. We have taken Σ,T ∝ R^{0.75}, and α(R,0) ∝ R^{a} (with the local value of ⟨ α ⟩ _{P} being 10^{2}), with three values of the exponent a used in the plots. The viscous prescription entails a parabolic flow profile (the socalled meridional circulation) while the MHD prescription entails an inverted Gaussian profile (until the corona, here at  z  > z_{max} = 3.0 H). Here, for a = −1, the vertically integrated flow is outward in both prescriptions. 

In the text 
Fig. 2
Dusttogas ratio normalized to the column density ratio (f) as a function of z, for both viscous (dashed line) and MRIturbulent prescriptions (solid line) and for three values of the “settling parameter” S_{z} ≡ St/ ⟨ δ_{z} ⟩ _{P}, with ⟨ δ_{z} ⟩ _{P} = 10^{2}. In the viscous prescription, this ratio falls off as a “double Gaussian” whereas it only does so as a Gaussian for the MHD prescription over the bulk of the disk thickness, before decreasing as a “double Gaussian” in the corona (here at  z  > z_{max} = 3.0H). 

In the text 
Fig. 3
Net vertically averaged velocity v_{p,1D} as a function of S = St(R,0)/ ⟨ α ⟩ _{P} for the viscous prescription (dashed line) and the MHD prescription (solid line), for three values of Sc_{z} (0.1 in blue, 1 in green and 10 in red). The velocities are always inward and we plot here their absolute value. We have taken Σ,T ∝ R^{0.75}, ∂α(R,0)/∂R = 0, δ_{R} = δ_{z} and ⟨ α ⟩ _{P} = 10^{2}. The dotted line corresponds to the simple onedimensional approximation (see Eq. (42)) which is common to both prescriptions and independent of Sc_{z}. The approximation is arbitrarily good in the limits S ≪ 1 and S ≫ 1 and the imparted error does not exceed a factor of two when S ~ 1 except for the viscous prescription at Sc_{z} = 10 where it can reach one order of magnitude. 

In the text 
Fig. 4
Cartoon of the toy model for meridional circulation. We distinguish between an “outward transport zone” (rightward arrows) and an “inward transport zone” (leftward arrows), which are assigned fractions θ and 1 − θ (θ < 1/2) of the local column density, respectively. Integers n − 1, n, n + 1 represent radial locations whose separation corresponds to one vertical mixing timescale. Vertical mixing is symbolized by double vertical arrows. 

In the text 
Current usage metrics show cumulative count of Article Views (fulltext article views including HTML views, PDF and ePub downloads, according to the available data) and Abstracts Views on Vision4Press platform.
Data correspond to usage on the plateform after 2015. The current usage metrics is available 4896 hours after online publication and is updated daily on week days.
Initial download of the metrics may take a while.