Simulations of particle-laden flow with dielectric particles are carried out with varying levels of electrical charging and particle polarization. Simulation results reveal three distinct flow regions. For low particle charge and polarizability, flow is nearly symmetric and nonmeandering. For strong charging and polarization, particles form a continuous and tightly clustered sheet close to one of the walls. Between these extremes, particles form localized particle-rich regions, around which the gas executes a meandering flow. These results indicate that polarization can lead to qualitative changes in the characteristics of particle-laden flows subject to tribocharging.
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TY - JOUR
T1 - Effects of Polarization on Particle-Laden Flows
AU - Kolehmainen, Jari
AU - Ozel, Ali
AU - Gu, Yile
AU - Shinbrot, Troy
AU - Sundaresan, Sankaran
N1 - Funding Information: Kolehmainen Jari * Ozel Ali Gu Yile Shinbrot Troy Sundaresan Sankaran Department of Chemical and Biological Engineering, Princeton University , Olden Street, Princeton, New Jersey 08544, USA * email@example.com 21 September 2018 21 September 2018 121 12 124503 15 June 2018 21 December 2017 © 2018 American Physical Society 2018 American Physical Society Simulations of particle-laden flow with dielectric particles are carried out with varying levels of electrical charging and particle polarization. Simulation results reveal three distinct flow regions. For low particle charge and polarizability, flow is nearly symmetric and nonmeandering. For strong charging and polarization, particles form a continuous and tightly clustered sheet close to one of the walls. Between these extremes, particles form localized particle-rich regions, around which the gas executes a meandering flow. These results indicate that polarization can lead to qualitative changes in the characteristics of particle-laden flows subject to tribocharging. National Science Foundation 10.13039/100000001 CBET-1601986 DMR-1404792 ExxonMobil Research and Engineering Company 10.13039/100006584 Finnish Culture Foundation In this Letter, we examine the effects of particle polarizability on particle-laden flow dynamics. We find that including polarizability produces new and distinct flow regimes in contrast to prior studies that have neglected polarization and consider only neutral or electrically charged particles [1–10] . Since the most pronounced effects of electrical charge are seen in insulating materials and since insulating materials tend to polarize, the study of the effects of polarization is relevant not only to flow and particle elutriation characteristics in gas-fluidized beds of particles [11,12] , but also to a broad range of other applications involving charging of insulators. For example, terrestrial and extraterrestrial dust devils involve insulating materials that charge strongly [13–15] , as do mineral dust aerosols  . In industrial applications, likewise, spontaneous self-organization associated with particle charging has been reported in microelectronic manufacturing  as well as in structural evolution in carbon nanotubes [18,19] . Furthermore, in polyethylene-fluidized bed reactors, particle charging has been linked to particles adhering on reactor walls, known as sheeting [20,21] , which causes costly reactor shutdowns and is an ongoing issue in polymer production  . Furthermore, there has recently been rapid growth in new applications involving charged insulators, such as triboelectric nanogenerators that have been proposed for renewable energy production  . Many of these applications involve insulating materials, and findings of this Letter may be germane. In previous work, Siu et al.  investigated the behavior of granular materials in strong electric fields. They found that applied fields can cause particles to produce novel behaviors ranging from static columns to moving ribbons that are not explained by static charges alone. An experimental study of LaMarche et al.  also showed that the electric field created by a tribocharged Teflon sheet is enough to cause significant dielectrophoretic interactions, and suggested that triboelectrification present in granular flows could lead to similar effects. Furthermore, a recent article by Lee et al.  investigated clustering of triboelectrically charged particles during free fall in vacuum and concluded that dielectrophoresis associated with particle charges plays an important role in particle dynamics and agglomerate formation. In addition, recent fluidization experiments by Fotovat et al. [11,12] revealed weaker entrainment with insulating particles than with conducting particles having otherwise similar particle properties, reinforcing the view that more comprehensive study of particle polarization is merited. Intriguingly, Feng  has even reported that complex electrostatic interactions can cause like-charged dielectric particles to attract one another. In this Letter, we quantify effects of particle polarizability on dynamics of gas-solid flows by simulating a simple vertical periodic channel, where dielectric particles are fluidized by an upward ambient fluid flow against downward gravity. As we will show, dielectric influences produce distinct flow regimes that would not be seen by considering Coulomb forces alone. We simulate a fluidized bed with periodic boundaries in the vertical and in one horizontal direction; in the remaining horizontal direction we fix conducting impermeable walls. The driving gas pressure drop Δ P g , in the vertical direction that supports the particles is adjusted to keep the mean vertical solids flux zero in all simulations. In this Letter, we present simulation results for spherical particles with diameter d p = 150 μ m . The channel is square in cross section, with dimensions 30 d p × 30 d p × 120 d p , and the domain-averaged solid fraction ⟨ ϕ s ⟩ = 0.1 . Triboelectrification occurs when a particle collides with other particles or with the channel walls. The triboelectric charging is modeled by following Laurentie et al.  , in which the charge transfer is driven by a difference in the effective work function φ that depends on the materials under consideration and the electrical potential difference between the contacting surfaces. This charging model has been found to capture particle charging in a granular chute  and in a vibrated granular bed [28,30] . In this model, the effective work function is a lumped parameter that can be determined either empirically  or using density functional theory  . In the present study, all particles are made of the same material, while the wall is made of a different material so that there is an effective work function difference Δ φ between the particles and wall. The maximum charge that a particle may obtain during a collision with the wall, referred to as the equilibrium charge q eq , can be related to the effective work function difference by q eq = 1 2 π ϵ 0 Δ φ d p 2 / ( δ c e + )  . Here, ϵ 0 is the vacuum permittivity, δ c is the electron tunneling distance (taken to be 500 nm in this study), and e + > 0 is the elementary charge. We characterize the extent of Coulombic interactions using the nondimensional number e / g ∝ Δ φ 2 , a shorthand for the ratio of the Coulomb forces at the contact between particles with charges ± q eq to the weight of a particle, m p g (for details, see Supplemental Material  ). We model the induced polarization on particles by applying a simple dielectric polarization law: P = ϵ 0 χ E , where P is the polarization density, E is the electric field, and χ is the particle susceptibility. The electric dipole moment p of a particle is then p = ∫ V p p d V ≈ ϵ 0 α p V p E , where α p is the (dimensionless) polarizability of the particle and V p is its volume. In this way, particle charges are governed by the wall-particle work function difference Δ φ , and polarization is governed by the polarizability α p . Particle and fluid dynamics are solved using an Euler-Lagrange approach, where the locally averaged equations of motion for the fluid phase are solved in an Eulerian framework and the particles are tracked in a Lagrangian fashion by solving Newton’s equations of motion  . Particle collisions are modeled with a Hertzian contact model  , and the drag force is accounted for by Wen and Yu’s empirical drag law  . Electrostatic interactions between particles are modeled using a particle-particle particle-mesh method that accounts for both short-range and long-range effects  . Details of the numerical scheme are given in the Supplemental Material  . At the nonperiodic walls described earlier, we impose no slip boundary conditions for the fluid, and the electrical potential is fixed at zero. The simulations include both frictional and inelastic particle-wall interactions. At the start of each simulation, the particles are distributed randomly in the simulation domain. In the results presented here, we vary the e / g value between 0 and 7 (27 different values), while α p is varied between 0 and 3 (13 different values), producing a total of 339 simulations, each using 20 626 particles. The system charge saturated typically within ∼ 2 s and every simulation was run for an additional 8 s to obtain time-averaged statistics. Simulation results are summarized in Fig. 1 , with panels (a) and (b) showing the average particle contact coordination number ⟨ Z ⟩ and the scaled gas pressure drop, respectively. Higher ⟨ Z ⟩ values, indicative of a more clustered state of the particles, appear when both e / g and α p are large. We note that without polarizability ( α p = 0 ), strong clustering does not occur for any level of particle charging: a straightforward consequence of Coulomb repulsion. Likewise without particle charging ( e / g = 0 ), there are no electrostatic forces irrespective of polarizability, so both particle charging ( e / g ) and polarizability ( α p ) are needed to generate clustering. As we will see, sheeting of particles along a boundary wall occurs in the “sheeted” region of high e / g and α p , delineated by black broken lines in Fig. 1(a) . 1 10.1103/PhysRevLett.121.124503.f1 FIG. 1. (a) Mean particle contact coordination number ⟨ Z ⟩ (number of particles contacting a given particle), as a function of the dimensionless ratio of Coulombic and gravitational forces ( e / g ) and polarizability ( α p ). The black dashed line shows contour where average particle contact number ⟨ Z ⟩ = 0.8 . (b) Driving gas pressure difference normalized by the suspension weight [ ρ ¯ g = ( ⟨ ϕ s ⟩ ρ p + ⟨ 1 - ϕ s ⟩ ρ g ) g ]. White line, see caption of Fig. 2 . Contour plots have been smoothed and interpolated from the actual simulation values, which can be found from the Supplemental Material  . As we have described, the simulations use a “laboratory frame” in which particle flux is zero, and the weight of the particles is supported by a combination of gas pressure drop and wall friction. The scaled gas pressure drop, Δ P g / L ρ ¯ g , for various combinations of e / g and α p values [corresponding to Fig. 1(a) ] are presented in the form of a contour plot in Fig. 1(b) , where Δ P g / L ρ ¯ g = 1 implies that the weight of the particles is completely supported by the gas. As the electrostatic forces (Coulombic or dielectrophoretic) increase, the particles become increasingly supported by wall resistance. At low e / g values, the extent of particle charging is small and so the strength of the prevailing electric field is small as well; polarization has a negligible effect under these conditions. As e / g increases polarization plays an increasingly important role. The domain-averaged gas-particle slip velocity, u ˜ slip = u ˜ g , z - u ˜ p , z , presented in Fig. 2(a) manifests a more complex dependence on e / g and polarizability than the contact coordination number and pressure drop shown in Fig. 1 . The low contact number region in Fig. 1(a) contains two subregions: one with higher slip velocity and meandering flow pattern [see Fig. 3(a) ] and one with lower slip velocity, exhibiting nearly symmetric, nonmeandering flow. In the higher contact number region of Fig. 1(a) (“sheeted”), the average slip velocity is low. 2 10.1103/PhysRevLett.121.124503.f2 FIG. 2. Flow behavior of nearly symmetric, meandering, and sheeted regions as a function of the dimensionless ratio of Coulombic and gravitational forces ( e / g ) and polarizability ( α p ). (a) Color coding represents the domain-averaged slip velocity ( u ˜ slip = u ˜ g , z - u ˜ p , z ) normalized by the particle terminal velocity u t = 0.432 m / s . Here, u ˜ g , z denotes the Favre-averaged gas velocity, and u ˜ p , z denotes the average velocity of all the particles in the domain. (b) Domain-averaged variance of the Eulerian particle volume fraction field (for Eulerian grid size 3 d p ). The black dashed line shows contour where the average particle contact number ⟨ Z ⟩ = 0.8 [refer to 1(a) ], and the white dashed line identifies both the fastest slip between particles and fluid and the highest variability in particle concentrations. Contour plots have been smoothed and interpolated from the actual simulation values, which can be found from the Supplemental Material  . 3 10.1103/PhysRevLett.121.124503.f3 FIG. 3. (a) Snapshot taken after 7.5 s of simulation time from e / g = 7 and α p = 0 (no polarization). Background color shows vertical fluid velocity, and particles show the local volume fraction. Yellow (green) particles have local volume fraction above (below) the average volume fraction ( ⟨ ϕ p ⟩ = 0.1 ) and on an average tend to move downward (upward). Only every 20th particle is shown and they are magnified to 2.5 times their actual size for ease of visualization. White arrows identify the particle flow directions. Some particles appear outside the channel due to image perspective. (b) The same plot as in panel (a), but for α p = 3 (largest amount of polarization). (c) Time-averaged vertical particle velocity profile for nonsheeted flow configurations. (d) Vertical particle velocity profile for the sheeted flow configuration. Solid red and purple lines show the profile for panel (a) and (b) flows, respectively. Velocity profiles are normalized by particle terminal velocity: u t = 0.432 m / s . The flow patterns illustrated in the snapshots shown in panels (a) and (b) persist in time (see Supplemental Material  ). As shown in Fig. 2(b) , the distribution of particles in the flow channel is inhomogeneous to some extent even in the absence of electrostatic effects (i.e., near e / g = α p = 0 ). From an examination of snapshots of simulations [cf. Figs. 3(a) and 3(b) ], it appears that this inhomogeneity is associated with a slight enrichment of particles in the vicinity of the walls and the flow-induced dynamic clusters where the particles congregate near each other. Both contribute to particle volume fraction variance, which is nonzero even in the absence of electrostatic effects [see Fig. 2(b) ]. They weaken the gas-particle interaction (i.e., the effective drag coefficient) and increase the gas flow rate required to produce the pressure drop needed to maintain zero particle mass flux. Indeed, the average slip velocity [Fig. 2(a) ] is in excess of the terminal settling velocity of the particle even though the gas is not required to support the entire weight of the particle. When electrostatic effects are included, a number of changes occur. First, stronger particle-wall interactions lower the pressure drop required to support the particles [Fig. 1(b) ]. Second, both the particle volume fraction variance [Fig. 2(b) ] and the required slip velocity to maintain zero particle mass flux [Fig. 2(a) ] vary with e / g and α p in a complex, but largely similar fashion [Figs. 2(a) and 2(b) ]. The Pearson correlation coefficient between the slip velocity and the product of particle volume fraction variance and the pressure drop is 0.86, indicating a strong correlation. This similarity can be understood by noting that the average slip velocity is a measure of the ratio between the pressure gradient and the average drag coefficient. Since the average drag coefficient decreases with an increasing particle volume fraction variance, it stands to reason that slip velocity and volume fraction variance should be correlated. To understand how both slip velocity and volume fraction variance depend on electrostatics, we note that introducing Coulombic interactions (in the absence of polarization) can be expected to cause particle-particle repulsion and wall-particle attraction. Stronger wall-particle attraction in turn draws particles closer to the walls and so lowers the required pressure drop, as illustrated by Fig. 1(b) . This same migration of particles toward the walls increases particle volume fraction variance. Working against this effect, Coulombic repulsion between the particles reduces clustering which lowers the variance. The consequence of these competing effects is seen in Fig. 2(b) . Increasing e / g first decreases the variance corresponding to increased Coulombic repulsion between particles; a further increase in e / g leads to a large increase in the variance due to enhanced lateral segregation. Our simulations at low e / g values (and no polarization) did not reveal meandering flow, but a meandering flow pattern as illustrated in Fig. 3(a) is observed above a threshold value of e / g . A meandering flow pattern is accompanied by a large increase in the variance of particle volume fraction, setting up a path of low resistance for the gas to flow through; as a result, the average slip velocity increases when meandering sets in. These are seen clearly in Figs. 2(a) and 2(b) . The time-average particle flux in such a state is still nearly symmetric [see solid line in Fig. 3(c) ]. Stipulation of periodic boundary conditions in the axial direction influences the threshold e / g value at which meandering sets in. Simulations performed in taller periodic domains produce an onset of meandering flow at lower e / g values (not shown). In fact, a simulation in a periodic domain that is twice as tall yielded a meandering flow even in the absence of electrostatic effects. Thus, including Coulombic interactions lowers the critical axial wavelengths above which meandering flow is obtained, and intensifies the prevalence of meandering flow structures. Simulations performed in wider channels, not shown, manifest analogous trends. Including polarization changes the flow behavior appreciably. First, the dipoles induced by the electric field give rise to an attractive interaction between particles. It is known that even when particles carry the same charge, strong dipole interaction can lead to a net attractive force between particles [26,27] . As a result, the average contact coordination number tends to increase with an increasing polarizability [see Fig. 1(a) ]. Our simulations show that a meandering flow sets in at lower e / g values when polarizability is included. Thus, meandering flows can be expected to be more prevalent in the case of dielectric particles. Increasing particle charging ( e / g ) increases the magnitude of the electric field, which leads to stronger electric dipoles when the particles polarize. This leads to higher interparticle attraction and a higher particle contact coordination number as seen in Fig. 1(a) . In industrial-fluidized beds, elutriation of particles from the bed is of serious concern. As particle agglomerates are less easily elutriated than individual particles, attractive forces between polarizable, charged particles can be expected to lower elutriation, as has been found in a recent experimental study  . Interestingly, an asymmetric flow pattern, which takes the form of a sheetlike structure shown in Fig. 3(b) , emerges in the case of highly polarized particles at large e / g values. As dipole-induced attraction takes place in the direction of the electric field (which is principally in the wall-normal direction), the sheetlike structure also forms parallel to a wall, as opposed to particle clusters typically observed in nondirectional forms of cohesion such as liquid bridges [44,45] or van der Waals forces  . The sharp change in the particle volume fraction variance between the meandering and sheeted regions is associated with this change in the particle flow behavior. Such sheeting of particles has been reported in industrial-fluidized bed polymerization reactors [20–22] , and is undesirable from a reactor performance point of view. In summary, electrostatic interactions due to particle charging and polarization significantly affect confined particle-laden flows. Both particle charging and polarization make meandering flows more prevalent. An asymmetric flow pattern, referred to as sheeted flow, is realized only when particle polarization is taken into consideration. Earlier studies [11,12] have used the ratio of total electrostatic forces to gravitational force to describe the system behavior where the electrostatic forces are evaluated by an expression derived by Feng  that combines polarization and Coulomb forces. In this study, we find that particle polarization can give rise to a qualitatively different flow behavior than a strongly charged system. Therefore, the dielectric polarization of particles should be considered independently from the Coulombic interactions, rather than attempting to lump all electrostatic influences together. The potentially strong influence of polarization even in the absence of an externally imposed electric field reported in this study suggests that one could manipulate flows of dense assemblies of polarizable particles by an applied field—introducing, strengthening, or weakening yield stress in the assembly and thus enabling flow control, an idea widely exploited in the context of electrorheological fluids  . This material is based upon work supported by the National Science Foundation Grants No. CBET-1601986 and No. DMR-1404792. In addition, the authors would like to thank ExxonMobil Res. & Eng. Co., and the Finnish Culture Foundation for funding this research.  1 D. Schmidt , R. Schmidt , and J. Dent , J. Geophys. Res. Atmos. 103 , 8997 ( 1998 ). JGRDE3 0148-0227 10.1029/98JD00278  2 J. F. Kok and N. O. Renno , Phys. Rev. Lett. 100 , 014501 ( 2008 ). PRLTAO 0031-9007 10.1103/PhysRevLett.100.014501  3 M. D. Hogue , C. I. Calle , P. S. Weitzman , and D. R. Curry , J. Electrost. 66 , 32 ( 2008 ). JOELDH 0304-3886 10.1016/j.elstat.2007.08.007  4 K. M. Forward , D. J. Lacks , and R. M. Sankaran , Geophys. Res. Lett. 36 ( 2009 ). GPRLAJ 0094-8276 10.1029/2009GL038589  5 M. Hassani , R. Zarghami , H. Norouzi , and N. Mostoufi , Powder Technol. 246 , 16 ( 2013 ). POTEBX 0032-5910 10.1016/j.powtec.2013.05.007  6 M. Korevaar , J. Padding , M. Van Der Hoef , and J. Kuipers , Powder Technol. 258 , 144 ( 2014 ). POTEBX 0032-5910 10.1016/j.powtec.2014.03.020  7 S. Naik , S. Sarkar , B. Hancock , M. Rowland , Y. Abramov , W. Yu , and B. Chaudhuri , Powder Technol. 297 , 211 ( 2016 ). POTEBX 0032-5910 10.1016/j.powtec.2016.04.013  8 C. Pei , C.-Y. Wu , and M. Adams , Powder Technol. 304 , 208 ( 2016 ). POTEBX 0032-5910 10.1016/j.powtec.2016.08.030  9 Y. Yang , C. Zi , Z. Huang , J. Wang , M. Lungu , Z. Liao , Y. Yang , and H. Su , Powder Technol. 308 , 422 ( 2017 ). POTEBX 0032-5910 10.1016/j.powtec.2016.12.032  10 J. Kolehmainen , A. Ozel , C. M. Boyce , and S. Sundaresan , AIChE J. 63 , 1872 ( 2017 ). AICEAC 0001-1541 10.1002/aic.15541  11 F. Fotovat , T. A. Alsmari , J. R. Grace , and X. T. Bi , Powder Technol. 316 , 157 ( 2017 ). POTEBX 0032-5910 10.1016/j.powtec.2016.10.063  12 F. Fotovat , J. R. Grace , and X. T. Bi , AIChE J. 63 , 1194 ( 2017 ). AICEAC 0001-1541 10.1002/aic.15514  13 N. O. Renno , A.-S. Wong , S. K. Atreya , I. de Pater , and M. Roos-Serote , Geophys. Res. Lett. 30 ( 2003 ). GPRLAJ 0094-8276 10.1029/2003GL017879  14 W. Farrell , P. Smith , G. Delory , G. Hillard , J. Marshall , D. Catling , M. Hecht , D. Tratt , N. Renno , M. Desch , J. Geophys. Res. Planets 109 ( 2004 ). JGPLEH 2169-9100  15 T. Pähtz , H. Herrmann , and T. Shinbrot , Nat. Phys. 6 , 364 ( 2010 ). NPAHAX 1745-2473 10.1038/nphys1631  16 Y. Shao , M. R. Raupach , and J. F. Leys , Aust. J. Soil Res. 34 , 309 ( 1996 ). ASORAB 0004-9573 10.1071/SR9960309  17 S. V. Vladimirov and K. Ostrikov , Phys. Rep. 393 , 175 ( 2004 ). PRPLCM 0370-1573 10.1016/j.physrep.2003.12.003  18 I. Levchenko , K. Ostrikov , A. Rider , E. Tam , S. Vladimirov , and S. Xu , Phys. Plasmas 14 , 063502 ( 2007 ). PHPAEN 1070-664X 10.1063/1.2744353  19 M. Meyyappan , L. Delzeit , A. Cassell , and D. Hash , Plasma Sources Sci. Technol. 12 , 205 ( 2003 ). PSTEEU 0963-0252 10.1088/0963-0252/12/2/312  20 G. Hendrickson , Chem. Eng. Sci. 61 , 1041 ( 2006 ). CESCAC 0009-2509 10.1016/j.ces.2005.07.029  21 D. Song and P. Mehrani , Powder Technol. 316 , 166 ( 2017 ). POTEBX 0032-5910 10.1016/j.powtec.2017.01.031  22 E. J. Markel , R. O. Hagerty , R. W. Impelman , R. B. Pannell , and C. F. Saladino (2013), U.S. Patent No. 8,378, 040 ( 2013 ).  23 Z. L. Wang , Nature (London) 542 , 159 ( 2017 ). NATUAS 0028-0836 10.1038/542159a  24 T. Siu , W. Pittman , J. Cotton , and T. Shinbrot , Granular Matter 17 , 165 ( 2015 ). GRMAFE 1434-5021 10.1007/s10035-015-0550-8  25 K. R. LaMarche , F. J. Muzzio , T. Shinbrot , and B. J. Glasser , Powder Technol. 199 , 180 ( 2010 ). POTEBX 0032-5910 10.1016/j.powtec.2010.01.006  26 V. Lee , S. Waitukaitis , M. Miskin , and H. Jaeger , Nat. Phys. 11 , 733 ( 2015 ). NPAHAX 1745-2473 10.1038/nphys3396  27 J. Q. Feng , Phys. Rev. E 62 , 2891 ( 2000 ). PLEEE8 1063-651X 10.1103/PhysRevE.62.2891  28 J. Laurentie , P. Traoré , and L. Dascalescu , J. Electrost. 71 , 951 ( 2013 ). JOELDH 0304-3886 10.1016/j.elstat.2013.08.001  29 S. Naik , S. Saurabh , G. Vipul , H. Bruno , Y. Abramov , W. Yu , and B. Chaudhuri , Int. J. Pharm. 491 , 58 ( 2015 ). IJPHDE 0378-5173 10.1016/j.ijpharm.2015.05.081  30 J. Kolehmainen , P. Sippola , O. Raitanen , A. Ozel , C. M. Boyce , P. Saarenrinne , and S. Sundaresan , Chem. Eng. Sci. 173 , 363 ( 2017 ). CESCAC 0009-2509 10.1016/j.ces.2017.08.006  31 See Supplemental Material at http://link.aps.org/supplemental/10.1103/PhysRevLett.121.124503 for simulation details, which includes Refs. [32–39].  32 T. B. Anderson and R. Jackson , Ind. Eng. Chem. Fundam. 6 , 527 ( 1967 ). IECFA7 0196-4313 10.1021/i160024a007  33 P. Pepiot and O. Desjardins , Powder Technol. 220 , 104 ( 2012 ). POTEBX 0032-5910 10.1016/j.powtec.2011.09.021  34 A. Ozel , J. Kolehmainen , S. Radl , and S. Sundaresan , Chem. Eng. Sci. 155 , 258 ( 2016 ). CESCAC 0009-2509 10.1016/j.ces.2016.08.014  35 Z. Zhou , S. Kuang , and A. Yu , J. Fluid Mech. 661 , 482 ( 2010 ). JFLSA7 0022-1120 10.1017/S002211201000306X  36 C. Kloss , C. Goniva , A. Hager , S. Amberger , and S. Pirker , Prog. Comput. Fluid Dyn. 12 , 140 ( 2012 ). PCFDAB 1468-4349 10.1504/PCFD.2012.047457  37 C. Goniva , C. Kloss , N. Deen , J. Kuipers , and S. Pirker , Particuology 10 , 582 ( 2012 ). 1674-2001 10.1016/j.partic.2012.05.002  38 K. Johnson , Contact Mechanics ( Cambridge University Press , Cambridge, 1987 ).  39 A. Renzo and F. P. Di Maio , Chem. Eng. Sci. 59 , 525 ( 2004 ). CESCAC 0009-2509 10.1016/j.ces.2003.09.037  40 J. Capecelatro and O. Desjardins , J. Comput. Phys. 238 , 1 ( 2013 ). JCTPAH 0021-9991 10.1016/j.jcp.2012.12.015  41 P. Cundall and O. Strack , Geotechnique 29 , 47 ( 1979 ). GTNQA8 0016-8505 10.1680/geot.1918.104.22.168  42 C. Wen and Y. H. Yu , Chem Eng Prog, Symp Ser 62 , 100 ( 1966 ). CEPSAB 0069-2948  43 J. Kolehmainen , A. Ozel , C. M. Boyce , and S. Sundaresan , AIChE J. 62 , 2282 ( 2016 ). AICEAC 0001-1541 10.1002/aic.15279  44 V. Richefeu , M. S. El Youssoufi , and F. Radjai , Phys. Rev. E 73 , 051304 ( 2006 ). PRESCM 1539-3755 10.1103/PhysRevE.73.051304  45 C. M. Boyce , A. Ozel , J. Kolehmainen , S. Sundaresan , C. A. McKnight , and M. Wormsbecker , AIChE J. 63 , 2520 ( 2017 ). AICEAC 0001-1541 10.1002/aic.15761  46 Y. Gu , S. Chialvo , and S. Sundaresan , Phys. Rev. E 90 , 032206 ( 2014 ). PRESCM 1539-3755 10.1103/PhysRevE.90.032206  47 T. C. Halsey , Science 258 , 761 ( 1992 ). SCIEAS 0036-8075 10.1126/science.258.5083.761 Funding Information: This material is based upon work supported by the National Science Foundation Grants No. CBET-1601986 and No. DMR-1404792. In addition, the authors would like to thank ExxonMobil Res. & Eng. Co., and the Finnish Culture Foundation for funding this research. Publisher Copyright: © 2018 American Physical Society.
PY - 2018/9/21
Y1 - 2018/9/21
N2 - Simulations of particle-laden flow with dielectric particles are carried out with varying levels of electrical charging and particle polarization. Simulation results reveal three distinct flow regions. For low particle charge and polarizability, flow is nearly symmetric and nonmeandering. For strong charging and polarization, particles form a continuous and tightly clustered sheet close to one of the walls. Between these extremes, particles form localized particle-rich regions, around which the gas executes a meandering flow. These results indicate that polarization can lead to qualitative changes in the characteristics of particle-laden flows subject to tribocharging.
AB - Simulations of particle-laden flow with dielectric particles are carried out with varying levels of electrical charging and particle polarization. Simulation results reveal three distinct flow regions. For low particle charge and polarizability, flow is nearly symmetric and nonmeandering. For strong charging and polarization, particles form a continuous and tightly clustered sheet close to one of the walls. Between these extremes, particles form localized particle-rich regions, around which the gas executes a meandering flow. These results indicate that polarization can lead to qualitative changes in the characteristics of particle-laden flows subject to tribocharging.
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U2 - 10.1103/PhysRevLett.121.124503
DO - 10.1103/PhysRevLett.121.124503
M3 - Article
C2 - 30296164
AN - SCOPUS:85053805510
VL - 121
JO - Physical Review Letters
JF - Physical Review Letters
SN - 0031-9007
IS - 12
M1 - 124503