Mon.Not.R.Astron.Soc.000,1–9() Printed21January2009 (MNLATEXstylefilev2.2) Time-dependent simulations of steady C-type shocks S. Van Loo,1⋆, I. Ashmore1, P. Caselli1, S. A. E. G. Falle2, and T. W. Hartquist1 9 1 School of Physicsand Astronomy, University of Leeds, Leeds LS2 9JT, UK 0 2 Department of Applied Mathematics, Universityof Leeds, Leeds LS2 9JT, UK 0 2 n Accepted -.Received-;inoriginalform- a J ABSTRACT 6 1 Using a time-dependent multifluid, magnetohydrodynamic code, we calculated the structure of steady perpendicular and oblique C-type shocks in dusty plasmas. We ] included relevant processes to describe mass transfer between the different fluids, ra- R diative cooling by emission lines and grain charging and studied the effect of single- S sized and multiple sized grains on the shock structure. Our models are the first of . oblique fast-mode molecular shocks in which such a rigorous treatment of the dust h grain dynamics has been combined with a self-consistent calculation of the thermal p - and ionisation structures including appropriate microphysics. At low densities the o grains do not play any significant rˆole in the shock dynamics. At high densities, the r ionisationfractionissufficientlylowthatdustgrainsareimportantchargeandcurrent t s carriers and, thus, determine the shock structure. We find that the magnetic field in a the shock front has a significant rotation out of the initial upstream plane. This is [ most pronounced for single-sized grains and small angles of the shock normal with 1 the magnetic field.Our resultsaresimilar to previousstudies ofsteadyC-type shocks v showingthatourmethodisefficient,rigorousandrobust.Unlikethemethodemployed 1 in the previous most detailed treatment of dust in steady oblique fast-mode shocks, 7 oursallowsareliablecalculationevenwhenchemicalorotherconditionsdeviate from 4 local statistical equilibrium. We are also able to model transient phenomena. 2 1. Key words: MHD – shock waves – ISM: dust – ISM: jets and outflows 0 9 0 : v 1 INTRODUCTION However,for afractional ionisation below 10−7,grains play i an important rˆole in governing the electromagnetic forces X Molecularoutflowsassociatedwithproto-stellarobjects(e.g. (Draine 1980). In the densest regions of molecular clouds ar Bwahlelrye&thLeafrdaact1i9o8n3a)ldiorniviseasthioonckχsiisntloowda(χrk<m1o0le−c6u)l.aTrhcleoulodws where nH > 106 cm−3, the fractional ionisation constraint is usually fulfilled. valuesofχcausethegasandthemagneticfieldtobeweakly Pilipp, Hartquist,& Havnes (1990) included the effect coupled.Chargedparticlesarethenpushedthroughtheneu- of dust grains on the structure of perpendicular steady C- tralgasbyLorentzforces,givingrisetoambipolardiffusion type shocks more rigorously than previous authors (e.g. (Mestel & Spitzer1956).Collisionsbetweenthechargedand DRD).Theirfour-fluidmodelspredictdifferentshockwidths neutral particles accelerate, compress and heat the neutral thanobtainedinsimilarmodelsofDRD.Thismodelwasex- gasaheadoftheshockfrontandamagneticprecursorforms. tendedto obliqueshocks byPilipp & Hartquist (1994) who Iftheshockspeedislowenoughforthegastocoolefficiently, found that in such shocks the tranverse component of the theflowbecomescontinuousinallfluids(e.g.Mullan1971). magneticfieldrotatesaboutthepropagationdirectionofthe SuchshocksarereferredtoasC-typeshocks(Draine1980). shock as long as there is a non-negligible Hall conductivity. Draine, Roberge, & Dalgarno (1983, hereafter DRD) This happens for a wide range of conditions, but Pilipp & calculated the structures of steady perpendicular C-type Hartquistwereunabletofindsolutionsforfast-modeshocks. shocksindiffuseanddensemolecularmediausingasteady- Wardle (1998) pointed out that, to find a stable shock state multifluid magnetohydrodynamic (MHD) description. structurefor steady oblique fast-mode shocks, one needs to They included a detailed treatment for energy and mo- integratethesteadystateequationsbackwardsintimefrom mentum transfer between different particles, oxygen-based thedownstreamboundary.However,suchamethodrequires chemistryandradiativecooling.Theyalsoassumedthatthe anexactthermal,chemicalandionisationequilibrium.Such ion and electron densities exceed the grain charge density. an equilibrium does not obtain in most shocks of interest. Forinstance,theabundanceofwater,animportantcoolant, ⋆ E-mail:[email protected] is out of equilibrium for about 105 years or more from the 2 S. Van Loo et al. timethegascoolsbelowseveralhundreddegree.Thishigh- (J.B)B J×B (J×B)×B lights the necessity for time-dependent simulations to cal- E=−vn×B+r// B2 +rH B −rAD B2 , culatetheC-typeshockstructure.Ciolek & Roberge(2002) where r is theresistivity along the magnetic field, r the // H were thefirst toinclude afluid description of grain dynam- Hall resistivity and r the ambipolar resistivity. The ex- AD ics in multifluid MHD simulations. However, their study is pressionsoftheresistivitiesaregivenbye.g.Falle(2003)and restricted toperpendicularshocks.Themultifluidapproach depend strongly on the Hall parameter, β =α |B|/K ρ , i i ni n developed by Falle (2003) overcomes this limitation. whichistheratiobetweenthegyrofrequencyofthecharged In this paper we study the structures of steady fast- fluid and collision frequency of the charged fluid with the mode C-typeshocks using time-dependent multifluid MHD neutrals. Substitution of the above expression into the simulations. In Sect. 2 we describe the numerical code and Maxwell-Faraday equation then gives the magnetic induc- the physical processes that we include. Then, we apply the tion equation code to perpendicular and oblique shocks with parameters ∂B ∂M ∂ ∂B similar to those of DRD including a single-sized grain fluid + = R , (7) ∂t ∂x ∂x ∂x (Sect.3)ormultiplegrainfluids(Sect.4).Finally,wediscuss theresults and give ourconclusions in Sect. 5. where M = vn×B is the hyperbolic magnetic flux and R is theresistance matrix which dependson the Hall resistiv- ity, the ambipolar resistivity, and the resistivity along the 2 THE MODEL magnetic field. (For an expression for R, see Falle (2003).) Equations 1 - 7 are solved using the numerical scheme 2.1 Numerical code described by Falle (2003). This scheme uses a second-order hydrodynamic Godunov solver for the neutral fluid equa- Astheionisationfractionwithinmolecularcloudsislow,the tions (Eqs. 1-3). The charged fluid densities are calculated plasma needs to be treated as a multicomponent fluid con- usinganexplicitupwindapproximationtothemassconser- sistingofneutrals,ions,electronsandN dustgrain species. vation equation (Eq. 4), while the velocities and tempera- The governing equations for theneutral fluid are given by turesarecalculatedfromthereducedmomentumandenergy ∂ρ ∂ n + (ρ v ) = s , (1) equations(Eq.5and6).Themagneticfieldisadvancedex- ∂t ∂x n x,n Xj jn plicitly, even though this implies a restriction on the stable time step at high numerical resolution (Falle 2003). ∂ρ v ∂ J×B ∂nt n + ∂x(ρnvx,nvn+pn1x) = c , (2) ∂e ∂ 1 n + v e +p + ρ v2 = J.E+ H(,3) 2.2 Physical processes ∂t ∂x x,n n n 2 n n j h (cid:16) (cid:17)i Xj Thenumericalcodedescribedintheprevioussectionisquite where e = p /(γ−1)+ρ v2/2 is the internal energy per general. In order to investigate the effects of dust grains n n n n unit mass, s the mass transfer rate between the charged in fast-mode shocks it is necessary to specify the source jn fluidj and theneutralfluid,H theenergy sinksorsources terms, i.e. the mass, momentum and energy transfer coef- j for the different fluids, B the magnetic field, E the electric ficients and the energy sources and sinks, to describe the field and J thecurrent given byJ= αρ v . relevant physics. The chemical network that we adopted j j j j In thelimit of small mass densitiPes for thecharged flu- is the one used by Pilipp, Hartquist, & Havnes (1990) and ids, their inertia can be neglected. Also, the charged fluids Pilipp & Hartquist (1994). areinthermalbalanceastheirheatcapacitiesaresmall.For Mass transfer between the ion and electron fluids and thecharged fluid j, theequations then reduceto the neutral fluid is due to cosmic ray ionisation at a rate of10−17 s−1,electronrecombinationwithMg+,dissociative ∂ρ ∂ ∂tj + ∂x(ρjvx,j) = −sjn, (4) recombination with HCO+ and recombination of ions on charged grains. Here we have assumed that the main gas v ×B αjρj E+ j c +ρjρnKjn(vn−vj) = 0, (5) phase ions are Mg+ and HCO+ (Oppenheimer& Dalgarno (cid:16) (cid:17) 1974). The cross-section for these recombination reactions H +G = 0, (6) j jn are taken from Pilipp, Hartquist,& Havnes(1990). where α is thecharge to mass ratio, K the collision rate Mass is also transferred between the ion and electron j jn coefficient of the charged fluid j with the neutrals and G fluidsandthegrainfluidsduetoionneutralisationongrain jn theenergytransferrateperunitvolumebetweenthecharged surfaces. Ions and electrons stick to dust grains upon col- fluidandtheneutralfluid.TheexpressionsforK andG liding with them. Also, they pass on their charge with unit jn jn aregivenbyDraine(1986).Weusethereducedenergyequa- efficiency. The grain charge then critically depends on the tion to calculate the temperatures of the ion and electron electron-grain and ion-grain collision rates (which them- fluids. For the grain fluids, a hydrodynamic approximation selves depends on the electron density and temperature, with zero pressure is appropriate as the thermal velocity the ion density and temperature, and the ion-grain rela- dispersion of the dust grains is small compared to the drift tive streaming speed). The average grain charge is evalu- velocity with theneutrals. ated following Havnes,Hartquist, & Pilipp (1987). Individ- The collisions of thecharged particles with theneutral ual grains can have a charge that differs from the aver- particlesaffecttheevolutionofthemagneticfield.Usingthe age value, but it is mostly within one unit of the average reducedmomentumequationsforthechargedfluids(Eq.5) (Elmegreen 1979). and the expression for the current J, the electric field can Different radiative cooling processes for the neutral beexpressed as (Cowling 1956) and electron fluids are included in the code. The elec- Time-dependent simulations of steady C-type shocks 3 tron gas is cooled by the excitation and subsequent de- Using the upstream fluid properties, the properties far excitation of molecular hydrogen (e.g. DRD). This process downstream of the shock are calculated from the Rankine- only becomes important when the electron fluid temper- Hugionotrelationsforanisothermal,magnetisedshock.For ature exceeds ≈ 1000 K. In the neutral gas, the domi- our initial shock structure we assume that the shock is a nant cooling processes are associated with O, CO, H2 and discontinuity at x = 0 separating the upstream and down- H2O. The radiative transitions for atomic oxygen, i.e. OI stream properties. We follow the evolution of the shock to lines, are calculated using the procedure of DRD. The ra- steady state within the shock frame. diative losses from excited rotational-vibrational states of molecular hydrogen are a fit to the data presented by Hartquist,Dalgarno, & Oppenheimer(1980),whilethoseof CO are calculated by using Hollenbach & McKee (1979). 2.4 Computational details Finally, we use Neufeld & Melnick (1987) to calculate the The size of the computational box is assumed to be a few lossesduetorotationaltransitionsinH2O.Theheatingrate time the shock width. By balancing the ion-neutral drag oftheneutralgasbycosmicraysisfromDRD.Wehavenot force with the Lorentz force, we can estimate the shock included any radiative losses for the ion fluid. From Eq. 6 thickness(e.g. Draine & McKee 1993) and using the expression for G (Draine 1986) we find that i theion temperature, Ti, is given by L =7×1015 vA 10−2cm−3 cm, (9) T =T + mn(v −v )2, (8) i (cid:16)km s−1(cid:17)(cid:18) ni (cid:19) i n 3k n i B wherev istheshockspeed.However,thegrain-neutralfric- s whereT istheneutraltemperature,m theneutralparticle n n tion is comparable tothe ion-neutralfriction for mass and k theBoltzmann constant. B ρ K i < gn, ρ K g in 2.3 Initial conditions or The initial conditions of our simulations are adopted from χ<3×10−9 vs , DRD and similar studies such as Wardle (1998) and km s−1 (cid:16) (cid:17) Chapman & Wardle(2006).Thisallowsacomparisonofour where we substituted the expressions for the collision rates results with those of thesestudies. with the neutrals (Draine 1986) and assumed the relative The neutral fluid has a number density of nH = 104 cm−3 or nH = 106 cm−3 and is composed mainly of speedbetweentheneutralsandthegrainstobeoftheorder v /2. This constraint is fulfilled in the heated precursor for molecular hydrogen so that mn ≈ 2mH. Small amounts bsothdensitiesandtheshockthicknessisdeterminedbythe of other neutral species such as O, CO, and H2O are also grain-neutral drag. The expression for the shock width is present.TheinitialabundancesofO,CO,andH2Oaretaken to be 4.25×10−4 nH, 5 × 10−5nH and 0 respectively. How- similar to Eq. 9 and is given by ever,astheabundancesofOandH2Oevolvesubstantiallyas L =3×108χ vs −1L . (10) gasisheated,theabundancesoftheimportantcoolantsare g km s−1 i (cid:16) (cid:17) recalculated at every time-step. The dominant ions within thegas are assumed,as mentionedabove, tobeHCO+ and Values of χ appropriate for the precursor must be used. Mg+. The ion mass is then mi ≈ 30mH. Also, we assume Flower, Pineau des Forˆets, & Hartquist(1985)firstpointed out that chemistry leads toa large drop in χ in theprecur- that the ions are only singly ionised. sorofmanyshocks.Thenumericaldomainisthenchosento The dust grains are all assumed to be spherical with a radius of a = 0.4µm and a mass of 8.04 ×10−13 g (where be −10Lg 6 x6 10Lg with a free-flow boundary condition g thedensityofthegrainsistaken3gcm−3).Thegraintohy- at the downstream side and fixed inflow at the upstream boundary.We usea uniform grid with 400 cells. drogenmassratiointheunshockedregionhasthecanonical As our initial conditions are discontinuous, the inertia valueof0.01.Thedensitiesoftheionandelectronfluidsand ofthechargedfluid,eventheions,cannotbeneglecteddur- theaveragegrainchargearecalculatedfromionisationequi- ing the initial stages of the evolution. However, the inertial librium.Forthetemperaturesthatweadopt,i.e.T =8.4K n fornH =104 cm−3 andTn=26.7K fornH =106 cm−3,the phase of the charged fluid is short compared to the time to approach a steady configuration (e.g. Roberge & Ciolek average grain charge is quite close to −e and the electron 2007). Although the inertial phase does not affect the final andionnumberdensitiesareroughlythesame,i.e.n ≈n . e i steadyshockstructurehere,thiseffectshouldnotbeignored In the interstellar medium the magnitude of the mag- netic field scales roughly as B ≈ 1µG(nH/cm−3)−1/2 (see for some othertime-dependent models. DRD)sothatB=10−4 GfornH =104cm−3 andB=10−3 G for nH = 106cm−3. The Alfv´en speed of the gas is then the same at both densities, i.e. v =2.2 km s−1. In the far A upstreamregionthemagneticfieldliesinthex,y-planeand 3 C-TYPE SHOCK MODELS ◦ ◦ ◦ ◦ makesanangleof30 ,45 ,60 or90 (perpendicularshock) with the x-axis. We assume that a shock is propagating in In this section we present steady C-type shock structures the positive x-direction with a speed of 25 km s−1. Such a for large single-sized grains. First we discuss perpendicular shock is a strong fast-mode shock with an Alfv´enic Mach shocksandthenshockspropagatingatanobliqueanglewith numberof M ≈11.5. themagnetic field. A 4 S. Van Loo et al. Figure1.TheshockstructureforaperpendicularshockpropagatinginaquiescentregionwithnH=104cm−3(left)andnH=106cm−3 (right). Fromtoptobottom weplotthevelocity inthe x-directionandz-directionfortheneutrals (solid),ions/electrons (dashed) and grains (dotted), the tangential magnetic field and the temperatures of the ions (dashed), electrons (dotted) and the neutrals (solid) as well as the absolute value of the grain charge (dash-dotted). The velocities are normalised with respect to the shock speed and the magneticfieldtothetotalupstreammagneticfield. 3.1 Perpendicular shocks qualitatively similar, our shock widths are about 4 times largerthaninDRD.Thisisduetoalowerfractionalionisa- Figure 1 shows the structures in multiple flow variables for tion in our models which is a consequence of including the perpendicular shocks at different densities. It is clear that chemistry governing the ionisation rather than assuming a bothshockstructuresrepresentC-typeshocks.Asourmod- constantionfluxasDRDdid.Thedragforceofthecharged els are similar to DRD, we can compare our results with particles on the neutrals is then lower as well and is bal- figs.2and3ofDRD.Althoughtheshapesoftheshocksare ancedbythemagneticpressureoveralargerlengthscale.A Time-dependent simulations of steady C-type shocks 5 Figure2.Theshockstructureforanobliqueshockpropagatingatanangleof30◦(left),45◦(middle)and60◦(right)withthemagnetic fieldinaquiescentregionwithnH=104cm−3.Fromtoptobottomweplotthevelocityinthex-direction,y-directionandz-directionfor theneutrals (solid),ions/electrons (dashed) andgrains(dotted), thetangential magnetic fieldinthe y-direction(solid)and z-direction (dashed), and the temperatures of the ions (dashed), electrons (dotted) and the neutrals (solid) as well as the absolute value of the graincharge (dash-dotted). Thevelocities arenormalisedwithrespecttothe shockspeed andthe magneticfieldto thetotal upstream magneticfield. 6 S. Van Loo et al. consequence of the larger shock widths is that the gas has tobebalancedbythePedersencurrent(alongE′).ThisPed- more time to radiate away its energy. The maximum tem- ersen currentgives risetotherotation of themagneticfield perature of the neutrals within the shock front is only 530 around the shock propagation (Pilipp & Hartquist 1994). K for nH = 104cm−3 and 905 K for nH = 106cm−3, while Significant rotation occurs when the Hall conductivity is DRDfound 1223 K and 1334 K respectively. larger than thePedersen conductivity (Wardle1998). Figure 1 shows that the speed of the grains relative to For the nH = 104 cm−3 models, the Hall conductiv- the neutrals is less than the speed of the ions relative to ity is always smaller than the Pedersen conductivity and the neutrals. The difference in relative speeds is due to the there is no significant rotation of the magnetic field (see differentresponseofthechargedfluidstothePedersenalong z-component of magnetic field in Fig. 2). The rotation in- E′ (= E+vn×B) and Hall current along E′×B within creases marginally as the angle, θ, between the direction theshock front. From Eq. 5 we find of shock propagation and the magnetic field decreases. The othershockproperties,also,donotchangesignificantlywith vj−vn ≈ βj2 E′×B + βj E′ , (11) θ. The temperatures of the different fluids and the average c 1+βj2 (cid:18) B2 (cid:19) 1+βj2 (cid:18)B(cid:19) grainchargearesimilartotheonesfoundfortheperpendic- ular shock. These results agree well with the θ-dependence where β is the Hall parameter of the charged fluid. For j ofthesteadyshock structurefoundbyChapman & Wardle electrons and ions with |β | ≫ 1, the particles are tied to e,i (2006).Thesimilarityoftheshockstructurefordifferentval- themagnetic field and uesofθ resultsfrom theminorcontributionofthegrainsto ve,i−vn ≈ E′×B. thedragforceontheneutrals.Thegrainsdonotdetermine c B2 thedynamics and drift with theother charged species. At the other extreme, |β |≪1, the charged particles move Significant differences, however, are seen in the nH = withtheneutrals.ForthejnH =106cm−3 models,thegrains 106 cm−3 models. Here, the grains are the dominant con- tributors to the drag force on the neutrals. Furthermore, have a Hall parameter ranging from -0.1 (the upstream thereisasignificant chargeseparation givingrisetoalarge value) to a minimum of -1.5 within the shock front. For these values, the E′ term has a non-negligible contribution Hall conductivity. In Fig. 3 we see that there is a substan- tial rotation of the magnetic field. Also the magnetic field to the drift velocity. For the x-component of the velocity upstream is no longer a stable node, but a spiral node as of the grains, this term only becomes important when the the Hall conductivity changes wave propagation upstream grainsswitchfrommovingwiththeneutralstomovingwith theions and electrons (see Fig. 1).The z-component of the (Wardle 1998; Falle 2003). As for nH =104cm−3, the rota- E′ term,however,hasalargercontributiontothedriftforc- tion decreases for larger θ, while the shock width increases. The rotation of the magnetic field has large conse- ingthegrainstomovewith theneutrals.Thelower density quences for the drift velocity of the charged particles. Fig- model exhibits this effect to a lesser extent as the grain Hall parameter lies between -1 and -20. Then the E′ term ure 3 shows that the velocity structure changes consider- ably with θ. Also, the grains move significantly differently is less important and provides only a small contribution to ◦ thantheionsandelectrons,especially intheθ=30 model thedrift. (seeFig. 3). Along thepropagation direction, electrons and The velocity difference between the ions and electrons ions are decelerated immediately. The grains, however, are withtheneutralsdeterminesthetemperatureofthecharged initially accelerated before being decelerated. Furthermore, particlesthroughcollisionalheating.Themaximumvelocity theylagtheionsandelectrons.Todriftinthedirection op- differenceinthemodelsis≈v givingamaximumiontem- s peratureofafewtimes104 K.Electroncoolingbecomesim- posite to theions and electrons, the grains motion must be dominated bytheE′ term inEq. 11and E′ must bein the portantattemperaturesofabout1000Kreflectedinacon- x siderably lower electron temperature at roughly 3×103 K. samedirectionasthex-componentofE′×B.Thelargedif- ferences in drift velocity are expectedas therotation of the The electron temperature within the shock front is impor- magnetic field is induced by a charge separation (and thus tant for the dynamics of the shock as the average grain large Hallconductivity).Forlarger θ,theHallconductivity charge is androtationdecrease,sothattheions,electrons,andgrains Z e≈−4kbTeag, (12) move more together. As expected, the velocity profile con- g e verges to the perpendicular shock structure (see Fig. 1 and for|Z |≫1andn |Z |≪n (e.g.Draine1980).Otherwise, 3). g g g e theaveragegrain chargeisroughly−1.FromFig.1wefind thattheaveragegrainchargefollowsthisdependenceonthe electrontemperaturewiththeaveragegrainchargereaching 4 MULTIPLE GRAIN SPECIES maximum values of about -250. In Sect. 3 we have assumed a single-sized grain fluid. In molecular clouds, however, the dust has a grain-size distri- 3.2 Oblique shocks bution given by (Mathis, Rumpl,& Nordsieck 1977) For a finite magnetic field component parallel to the shock dn ∝a−3.5, (13) propagation andanon-zeroHallconductivity,theHallcur- da rent along E′×B has a component parallel to the propa- wherednisthenumberdensityofgrainswithradiibetween gation direction of the shock. As the total current in that a and a+da. To take into account the effect of multiple directioniszeroiftheshockissteady,theHallcurrentneeds dustspecies,weincludeanadditionalsmall-grain fluidwith Time-dependent simulations of steady C-type shocks 7 Figure 3.SameasinFig.2,butwithanupstreamdensityofnH=106cm−3. a =0.04µm (i.e. a =a /10) and m =8.03×10−16g (or and,thus,theshockdynamicsasthecollisioncoefficientbe- s s g s m = m /1000). The total mass density of the grain fluid, tween grains and neutrals is proportional to a2 /m (see s g g,s g,s ρ +ρ ,isassumedtobe1%oftheneutralmassdensity(as Draine 1986). From Fig. 4, we see that the shock width s g inourpreviousmodels).Withtheadoptedgrain-sizedistri- is indeed, as expected from Eq. 10, an order of magnitude butionmost ofthemassisinthesmallgrain fluid.Further- smaller than for themodel with single-sized large grains. more, the small grains dominate the grain-neutral friction 8 S. Van Loo et al. Althoughthesmallgrainshaveanaveragechargeabout an order of magnitude smaller than the large grains (see Eq. 12), the small grains have a larger Hall parameter and arestronglycoupledtothemagneticfield.Thevelocityplots inFig.4showthatthesmallgrainsmovewiththeelectrons andions,whilethelargegrainsmovewithvelocitiesbetween those of the neutrals and the other charged particles. The grain charge density is dominated by the small grains and freeelectronsaredepletedfromthegasphase(i.e.n ≫n ). i e Thechargeseparationbetweenthechargedparticlesisthus small and the Hall conductivity is too. The rotation of the magnetic field out of the plane is then negligible. Also, the upstream magnetic field is no longer a spiral node, but a stable node. The inclusion of a second grain species thus changes theshockstructureconsiderably.Includingadditionalgrain species will further affect the shock structure as more dust grains are loading the magnetic field lines. Then the signal speedatwhichdisturbuncespropagatethroughthecharged fluiddecreases.ForsmallPAHabundancesthesignalspeed is close to 25 km s−1 (Flower & Pineau des Forˆets 2003) leadingtothepossibilitythattheresultingshockisaJ-type shock in which thegrain inertia cannot be neglected. 5 SUMMARY AND DISCUSSIONS In this paper we have presented 1D time-dependent multi- fluidMHDsimulationsofperpendicularandobliqueC-type shocksindustyplasmas.Wehaveincludedinournumerical code relevant mass transfer processes, such as electron re- combinationwithMg+ anddissociativerecombinationwith HCO+,andradiativecoolingbyO,CO,H2 andH2O.Also, themassandchargetransferfrom ionsandelectronstothe dust grains is taken into account to calculate the average grain charge. Our models are the first of oblique fast-mode shocksindensemolecularcloudsinwhichafluidtreatment of grain dynamics has been combined with a self-consistent calculation ofthethermalandionisation balancesincluding appropriate microphysics. We have performed simulations with single-sized and with two dust grains species in plas- mas of different density. Dustgrainsdonotchangetheshockdynamicsmuchat nH =104cm−3andtheshockstructuresforobliqueandper- pendicularshocks are quitesimilar. Grains, however, domi- natetheshockdynamicsathigh densities(nH =106cm−3). For oblique shocks, the magnetic field in the shock front is not confined to the upstream magnetic field plane. The amountofrotationobtaineddependsontheHallandPeder- senconductivities.Forsingle-sizedgrainstherotationissig- nificantandincreaseswithsmallerθastheHallconductivity inthesemodelsiscomparabletothePedersenconductivity. Forsomemodels,themagneticfieldattheupstreamsideof theshock even spirals around the direction of shock propa- gation. When we include an additional small grain species, the rotation mostly disappears. The small grains which carry most of the charge move with the ions and electrons Figure 4. Similarto the 45◦ model of Fig. 3, but for two grain reducing the Hall conductivity. Our models corroborate fluids.Thesmallgrainsareindicatedonthevelocitycomponents the main qualitative conclusions of previous studies (DRD figureswithathin-dottedline,whiletheiraveragechargeisgiven Pilipp & Hartquist1994;Wardle1998;Chapman & Wardle byathindashed-dotted line. 2006; Guillet, Pineau des Forˆets, & Jones 2007), showing thatournumericalmethodisefficient,rigorous,androbust. Time-dependent simulations of steady C-type shocks 9 In addition, we have succeeded in taking a significant step DraineB.T.,RobergeW.G.,DalgarnoA.,1983,ApJ,264, by developing the first oblique shock code capable of pro- 485 ducing reliable results for comparisons with observations. Elmegreen B. G., 1979, ApJ, 232, 729 Previousobliqueshockmodelswererestricted byless rigor- Falle S.A. E. G., 2003, MNRAS,344, 1210 ous treatments of either the grain dynamics or the thermal Flower D. R., Pineau des Forˆets G., 2003, MNRAS, 343, and ionisation balances. 390 However,ourmodeldoeshavesomerestrictions.Firstly, FlowerD.R.,PineaudesForˆetsG.,HartquistT.W.,1985, wedeterminethedrift velocities ofthegrains solely bybal- MNRAS,216, 775 ancingthegrain-neutralfriction with theLorentzforce and Guillet V., Pineau desForˆets G., Jones A.P., 2007, A&A, neglect their inertia. While small dust grains can be con- 476, 263 sidered inertialess, large grains have a drag length, i.e. the GusdorfA.,CabritS.,FlowerD.R.,PineaudesForˆetsG., length scale for gas drag to decelerate the grains, that in 2008a, A&A,482, 809 some cases is comparable to the length scale for magnetic GusdorfA.,PineaudesForˆetsG.,CabritS.,FlowerD.R., fieldcompression(Ciolek & Roberge2002).Therefore,large 2008b, A&A,490, 695 graininertiacannotalwaysbeneglected.Secondly,forsmall Hartquist T. W., Dalgarno A., Oppenheimer M., 1980, grains, the average grain charge is close to the elementary ApJ,236, 182 charge. 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In the vicinity of protostellar 425 objects the abundance of SiO is significantly en- Mestel L., Spitzer L., Jr., 1956, MNRAS,116, 503 hanced (e.g. Martin-Pintado, Bachiller, & Fuente 1992; Mullan D. J., 1971, MNRAS,153, 145 Jim´enez-Serra et al. 2004).It is thought that theSiO emis- Neufeld D.A., Melnick G. J., 1987, ApJ,322, 266 sion arises from the interaction of a protostellar jet with OppenheimerM., Dalgarno A.,1974, ApJ, 192, 29 local dense clumps (Lefloch et al. 1998). Grain sputtering Pilipp W., Hartquist T. W., Havnes O., 1990, MNRAS, withinC-typeshocksreleasestheSiOdepletedonthegrains 243, 685 backintothegasphase(Caselli, Hartquist, & Havnes1997; Pilipp W., Hartquist T. W., 1994, MNRAS,267, 801 Schilkeet al. 1997). Numerical models using steady C-type Roberge W. G., Ciolek G. E., 2007, MNRAS,382, 717 shocks indeed show good agreement with recent obser- Schilke P., Walmsley C. 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