# Difference between revisions of "Precursors to splashing of liquid droplets on a solid surface"

(New page: ==Overview== '''Authors:''' Shreyas Mandre, Madhav Mani & Michael P. Brenner '''Source:''' Physical Review Letters, Vol.102, 134502, (2009) '''Soft Matter key words:''' droplets, splash...) |
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+ | Original entry: Nefeli Georgoulia, APPHY 226, Spring 2009 | ||

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==Overview== | ==Overview== | ||

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==Abstract== | ==Abstract== | ||

+ | In this publication authors develop a theoretical model for a droplet splashing against a solid wall, which they confirm by running computer simulations. Contrary to popular belief, they stipulate that high pressure of the air film trapped between the wall and the liquid drop actually prevents the drop from contacting the wall. Instead, the droplet spreads on the thin air film and emits capillary waves. | ||

==Soft Matter Snippet== | ==Soft Matter Snippet== | ||

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− | [[Image: | + | [[Image:shreyas_4.jpg |300px| |thumb| Fig.1 : Shreyas Mandre, Madhav Mani & Michael P. Brenner ]] |

+ | |||

+ | [[Image:shreyas_1.jpg |300px| |thumb| Fig.2 : Shreyas Mandre, Madhav Mani & Michael P. Brenner ]] | ||

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+ | [[Image:shreyas_2.jpg |300px| |thumb| Fig.3 : Shreyas Mandre, Madhav Mani & Michael P. Brenner ]] | ||

+ | |||

+ | |||

+ | It is interesting to take a closer look at the set of equations chosen to describe this fluid dynamics problem. The gas films deforms according to the differential equation: | ||

+ | |||

+ | <math>12 \mu (\rho h)_l = (\rho h^3 p_x)_x</math> | ||

+ | |||

+ | Here <math>\mu</math> is the gas viscosity, <math>\rho_l</math> is the liquid density and <math>\rho_x</math> is the gas density. Accordingly, <math>p_x</math> is the gas pressure and <math>p_l</math> the liquid pressure. Another equation relating the two pressures is: | ||

+ | |||

+ | <math>p_{ll} h_{ll} = \mathcal{H} [p_x + \sigma h_{xxx}]</math> | ||

+ | |||

+ | Where <math>\mathcal{H}</math> is a Hilbert transform. When the drop reaches a critical distance <math>H^*</math> from the wall, gas pressure rises under it and dominates surface tension and inertia.At that value, the pressure causes a dimple on the drop. Subsequently, the pressure develops two maxima as the interfacial curvature steepens rapidly. This is demonstrated in figure 1. | ||

+ | |||

+ | The authors set two parameters: | ||

+ | |||

+ | i) One is the Stokes number <math>St = \frac{\mu}{\rho_l V R}</math>, which relates to the critical distance as <math>H^* = R St^{2/3}</math>. | ||

+ | |||

+ | ii) The other parameter is <math>\epsilon = \frac{P_0}{(R\mu^{-1}V^7\rho_l^4)^{1/3}}</math>, which is obtained by setting equal the gas pressure gradient with the liquid deceleration. At large <math>\epsilon </math> the film thickness obeys the incompressible scaling <math>H \sim RSt^{2/3}</math>, while at small <math>\epsilon</math> compressible effects set in. Figure 2 demonstrates the dimple height <math>H^*</math> as a function of the impact parameters. | ||

+ | |||

+ | In a stroke of elegant simplicity, authors solve the set of equation using dominant balance arguments at the compressible and incompressible limit. When <math>\epsilon > 1</math>, the solution obeys the scaling laws: | ||

+ | |||

+ | <math>l \sim R \frac{U^{1/2}}{St^{2/3}} (\frac{h_{min}}{R})^{3/2}</math> | ||

+ | |||

+ | <math>p_{max} \sim \frac{\mu V}{RSt} (\frac{RU^3}{H_{min}})^{1/2}</math> | ||

+ | |||

+ | However, when <math>\epsilon << 1</math>, the equations obey the scaling laws: | ||

+ | |||

+ | <math>l \sim R \frac{\rho_l U^2}{P_0} (\frac{R P_0}{\mu V})^{\gamma/2} (\frac{h_{min}}{R})^{1 +\gamma}</math> | ||

+ | |||

+ | <math>p_{max} \sim P_0 (\frac{R P_0}{\mu V})^{\gamma/2} (\frac{h_{min}}{R})^{-\gamma}</math> | ||

+ | |||

+ | Where <math>\gamma</math> comes from the equation of state of the gas. On figure 3, authors compare their model predictions with experimental data of ethanol drops splashing on a solid surface (open and closed symbols corresponding to 1st and 2nd regime). The agreement is impressive! |

## Latest revision as of 01:39, 24 August 2009

Original entry: Nefeli Georgoulia, APPHY 226, Spring 2009

## Overview

**Authors:** Shreyas Mandre, Madhav Mani & Michael P. Brenner

**Source:** Physical Review Letters, Vol.102, 134502, (2009)

**Soft Matter key words:** droplets, splashing, capillary waves, surface tension, pressure, thin film

## Abstract

In this publication authors develop a theoretical model for a droplet splashing against a solid wall, which they confirm by running computer simulations. Contrary to popular belief, they stipulate that high pressure of the air film trapped between the wall and the liquid drop actually prevents the drop from contacting the wall. Instead, the droplet spreads on the thin air film and emits capillary waves.

## Soft Matter Snippet

It is interesting to take a closer look at the set of equations chosen to describe this fluid dynamics problem. The gas films deforms according to the differential equation:

<math>12 \mu (\rho h)_l = (\rho h^3 p_x)_x</math>

Here <math>\mu</math> is the gas viscosity, <math>\rho_l</math> is the liquid density and <math>\rho_x</math> is the gas density. Accordingly, <math>p_x</math> is the gas pressure and <math>p_l</math> the liquid pressure. Another equation relating the two pressures is:

<math>p_{ll} h_{ll} = \mathcal{H} [p_x + \sigma h_{xxx}]</math>

Where <math>\mathcal{H}</math> is a Hilbert transform. When the drop reaches a critical distance <math>H^*</math> from the wall, gas pressure rises under it and dominates surface tension and inertia.At that value, the pressure causes a dimple on the drop. Subsequently, the pressure develops two maxima as the interfacial curvature steepens rapidly. This is demonstrated in figure 1.

The authors set two parameters:

i) One is the Stokes number <math>St = \frac{\mu}{\rho_l V R}</math>, which relates to the critical distance as <math>H^* = R St^{2/3}</math>.

ii) The other parameter is <math>\epsilon = \frac{P_0}{(R\mu^{-1}V^7\rho_l^4)^{1/3}}</math>, which is obtained by setting equal the gas pressure gradient with the liquid deceleration. At large <math>\epsilon </math> the film thickness obeys the incompressible scaling <math>H \sim RSt^{2/3}</math>, while at small <math>\epsilon</math> compressible effects set in. Figure 2 demonstrates the dimple height <math>H^*</math> as a function of the impact parameters.

In a stroke of elegant simplicity, authors solve the set of equation using dominant balance arguments at the compressible and incompressible limit. When <math>\epsilon > 1</math>, the solution obeys the scaling laws:

<math>l \sim R \frac{U^{1/2}}{St^{2/3}} (\frac{h_{min}}{R})^{3/2}</math>

<math>p_{max} \sim \frac{\mu V}{RSt} (\frac{RU^3}{H_{min}})^{1/2}</math>

However, when <math>\epsilon << 1</math>, the equations obey the scaling laws:

<math>l \sim R \frac{\rho_l U^2}{P_0} (\frac{R P_0}{\mu V})^{\gamma/2} (\frac{h_{min}}{R})^{1 +\gamma}</math>

<math>p_{max} \sim P_0 (\frac{R P_0}{\mu V})^{\gamma/2} (\frac{h_{min}}{R})^{-\gamma}</math>

Where <math>\gamma</math> comes from the equation of state of the gas. On figure 3, authors compare their model predictions with experimental data of ethanol drops splashing on a solid surface (open and closed symbols corresponding to 1st and 2nd regime). The agreement is impressive!